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Measuring the stability of fundamental constants with a network of clocks
EPJ Quantum Technology volume 9, Article number: 12 (2022)
Abstract
The detection of variations of fundamental constants of the Standard Model would provide us with compelling evidence of new physics, and could lift the veil on the nature of dark matter and dark energy. In this work, we discuss how a network of atomic and molecular clocks can be used to look for such variations with unprecedented sensitivity over a wide range of time scales. This is precisely the goal of the recently launched QSNET project: A network of clocks for measuring the stability of fundamental constants. QSNET will include stateoftheart atomic clocks, but will also develop nextgeneration molecular and highly charged ion clocks with enhanced sensitivity to variations of fundamental constants. We describe the technological and scientific aims of QSNET and evaluate its expected performance. We show that in the range of parameters probed by QSNET, either we will discover new physics, or we will impose new constraints on violations of fundamental symmetries and a range of theories beyond the Standard Model, including dark matter and dark energy models.
1 Introduction
The Standard Model of particle physics and the Standard Model of cosmology form the current foundation of fundamental physics. The cosmological model introduces two new forms of energy: dark matter and dark energy. Astrophysical observations suggest that these two forms of energy account for 95% of the energy balance of our universe [1], with only the remaining 5% described by the Standard Model of particle physics. Dark matter is understood to be a nonrelativistic form of matter not accounted for by the Standard Model of particle physics and that is believed to play a crucial role in the dynamics of galaxies. Dark energy, usually in the form of a cosmological constant, is instead postulated to explain the observed accelerated expansion of the universe. The precise natures of both dark matter and dark energy remain an open question.
The two Standard Models rely on a large number of fundamental constants. Crucially, in these models all fundamental constants are assumed to be immutable in space and time and to have had the same value throughout the history of the universe. Challenging this central assumption could be the key to solving the dark matter and dark energy enigmas, and also to understand how to unify particle physics and gravity into a unified theory of nature. Many models of physics beyond these Standard Models lead to a cosmological time evolution of physical constants [2–8] and, in many of these models, all constants vary if one does [9]. In other models with ultra light new particles, e.g., models of ultra light dark matter, fundamental constants can have an effective spacetime dependence due to the interactions between these ultra light particles and those of the Standard Model of particle physics [10–14].
On the opposite end of the energy spectrum with respect to the theories just mentioned, quantum technologies allow us to perform extremely precise measurements. It has recently been realised that such an exceptional precision is a formidable tool for performing tests of fundamental physics [15]. Atomic clocks in particular can now reach uncertainties as low as 1 part in 10^{18} and below [16, 17], and this has been exploited to provide some of the tightest constraints on presentday temporal variations of the fine structure constant, α, and the electrontoproton mass ratio, μ, two of the fundamental constants of the Standard Model of particle physics [18–21]. Furthermore, the networking of clocks for detection of dark matter or dark energy signatures is emerging as an effective way to increase detection sensitivity and confidence, and also to expand the range of dark sector phenomena that can be probed [22–27].
In this article, we present the science case of the recently launched QSNET project: ‘A network of clocks for measuring the stability of fundamental constants’ [28]. The project represents a multidisciplinary effort, bringing together theoretical and experimental physicists from a wide range of research communities. It is our primary aim here to review and summarise the physics and phenomenology linked to variations of fundamental constants. At the same time, we describe how atomic and molecular clocks can be used to measure variations of fundamental constants, and discuss the typical range of parameters in which these clocks operate.
QSNET will network a range of stateoftheart clocks and nextgeneration clocks that feature enhanced sensitivity to variations of fundamental constants. The initial stage of QSNET is summarised in Fig. 1; it includes existing Sr, Yb^{+} and Cs atomic clocks at the National Physical Laboratory (NPL) in London and several new clocks currently being developed: a \(\text{N}_{2}^{+}\) molecular ion clock at the University of Sussex, a CaF molecular optical lattice clock at Imperial College London, and a Cf highly charged ion clock at the University of Birmingham. As the project progresses, this national network can be expanded and linked with other clocks across the globe. We evaluate the potential sensitivities of these clocks to variations of α and μ over different timescales. We then estimate the impact of the QSNET performance on specific dark matter and dark energy models, soliton models, and violations of fundamental symmetries.
This article is organised as follows: in Sect. 2, we review the theory about variations of fundamental constants. In Sect. 3, we describe how atomic and molecular clocks can be used to detect variations of fundamental constants, and how networking clocks brings both scientific and technological advantages. We then provide a description of the QSNET clocks and derive their expected performance. In Sect. 4, we consider how frequency comparisons between pairs of these clocks can probe the parameter space of specific dark matter, dark energy and soliton models. Additionally, we discuss how QSNET can perform tests of violations of fundamental spacetime symmetries, grand unification theories and quantum gravity. Section 5 is finally devoted to the conclusions.
2 Theoretical framework
The study of a possible time variation of the parameters of the fundamental laws of nature, such as the fine structure constant, has a long history. In particular, there were early speculations about a cosmological time change of Newton’s constant \(G_{N}\) [31–35]. Dirac’s large numbers hypothesis is based on his comparison of the strength of gravity to those of other forces of nature. Indeed, for elementary particles, gravity is about 30 to 40 orders of magnitude weaker than electromagnetism, for example. Dirac speculated that this may not be a mere coincidence but instead could imply a cosmology with some unusual features. He speculated that the strength of gravity, which is fixed by Newton’s constant, is inversely proportional to the age of the universe: \(G_{N} \propto 1/t\); the mass of the universe would be proportional to the square of the universe’s age \(M \propto t^{2}\). Therefore what we consider physical constants would not actually be constant, but their values could depend on the age of the universe. Dirac’s hypothesis has been ruled out by cosmological observations, but the interest of the physics community in a possible cosmological time evolution of physical constants has not ceased [36], further motivated by possible astrophysical observations of a cosmological time evolution of fundamental constants; see e.g. [37, 38].
The Standard Model of particle physics (Standard Model hereafter) and the Standard Model of cosmology (ΛCDM model hereafter, where Λ stands for a cosmological constant and CDM for cold dark matter) are extremely successful at describing all particle physics experiments performed thus far on Earth and all observations in cosmology and astrophysics. There are, however, serious limitations to these models. The most obvious one is that the ΛCDM model posits that 85% of all matter of the universe is described by cold dark matter, which is not accounted for by the Standard Model. Furthermore, the ΛCDM model assumes that General Relativity is the correct theory for gravity on all scales. It is however well known that General Relativity is not easy to reconcile with quantum field theory, which is the mathematical framework used to formulate the Standard Model.
Another issue is that both General Relativity and quantum field theories are not very predictive in the following sense: there is no fundamental guiding principle to tell us which fields to introduce in our models or which gauge symmetries to impose. Furthermore, while we may have the correct differential equations to describe the evolution of the universe and the interactions between particles, we do not have a theory of initial conditions.
There is also no specific reason to have three generations of particles or why leptons and quarks need to be introduced. These particles are introduced because they are found in nature, but without experimental guidance theorists would not have been able to determine how many fields to introduce or how to gauge these particles. There is also no basic reason why Lorentz invariance and its local version which lead to General Relativity are symmetries of spacetime. One could have imagined other fundamental symmetries of space and time.
Furthermore, these models have a number of fundamental constants that cannot be calculated from first principles. Within the Standard Model alone, there are 28 such fundamental parameters (note that 22 of these parameters are needed to describe fermion masses). In these 28 constants, we include also Newton’s constant which describes the strength of the gravitational interactions. The number of fundamental constants is even larger if we include the speed of light c, the Planck constant h, and other cosmological parameters such as the cosmological constant or the nonminimal coupling of the Higgs boson to the Ricci scalar. The absence of a theory of fundamental constants is a problem with our current understanding of nature. Indeed, modern theories of nature are based on renormalisable quantum field theories. Within this mathematical framework, it is impossible to calculate the value of the coupling constants from first principles. There is only one class of quantumfieldtheoretical models with no free parameters [39], but these models are an exception and they are far from describing the real world. Additionally, all such fundamental constants are taken to be invariable in space and time. However, as discussed here below, many theoretical frameworks that attempt to describe physics beyond the Standard Model predict or allow variations of the fundamental constants.
Because quantum gravity does not seem to be described by a renormalizable quantum field theory, extensions such as noncommutative geometry [40] or string theory [41, 42] have been considered. While it is difficult to make the link between these models and the real world, they are interesting because in principle they allow us to calculate some, if not all, fundamental constants. In particular, within string theory, coupling constants are fixed by the expectation values of moduli, which are scalar fields, and are thus calculable, at least in principle.
Some extensions of the Standard Model, and in particular models that couple gravity to the Standard Model, such as inflationary models or quintessence, require or allow a time dependence of the parameters of the model. In models with extradimensions, such as Kaluza–Klein models or string theory, fundamental constants are often given by the expectation values of moduli fields which depend on the size of compactified extradimensions. As the size of these extradimensions could vary during the cosmological evolution of the universe, fundamental constants could also have a cosmological time evolution [43]. Probing the cosmological time evolution of fundamental constants is therefore important, because this tests the validity of models with extradimensions and may help us develop a theory of fundamental constants.
Recently, it has been realised that other physical phenomena could mimic a timevariation of fundamental constants. For example, very light scalar fields which could account for dark matter could lead to an effective time variation of fundamental constants. A cosmological time evolution or time dependence of the coupling constants of the Standard Model can be parametrised by a scalar field ϕ which couples to the electron \(\psi _{e}\) (with mass \(m_{e}\)), light quarks (u, d and squarks) \(\psi _{q}\) (with mass \(m_{q}\)), the photon \(A_{\mu}\) or gluons \(G^{a}_{\mu}\) according to
with \(\kappa =\sqrt{4 \pi G_{N}}\), \(F_{\mu \nu}=\partial _{\mu}A_{\nu}\partial _{\nu}A_{\mu}\) and \(G_{\mu \nu}=\partial _{\mu}G_{\nu}\partial _{\nu}G_{\mu}i g_{s} [G_{\mu},G_{\nu}]\), where \(g_{s}\) is the QCD coupling constant. The \(d^{(i)}_{j}\) are numerical constants which determine the strength of the interactions between the scalar field and Standard Model particles, which can be stronger than the gravitational one if \(d^{(i)}_{j}>1\) or weaker if \(d^{(i)}_{j}<1\). We could also add to Eq. (1) couplings to the field strength of the neutrinos, heavier leptons and quarks, electroweak gauge bosons of the Standard Model and to the Higgs boson, but these particles usually do not play an important role for very low energy tabletop experiments such as clocks and we shall thus not include these couplings at this stage. Note that these operators are dimension5 operators as they are suppressed by one power of the reduced Planck scale \(M_{P}=1/\sqrt{8 \pi G_{N}} \).
For some applications, it might be necessary to consider scalar fields that transform under some discrete, global or gauge symmetry, in which case the simplest coupling to matter is given by dimension6 operators
In other words, the interactions of the scalar field with stable matter are suppressed by two powers of the reduced Planck scale.
These Lagrangians can account for a variety of physical phenomena:

Scalar dark matter models in which case the magnitude of ϕ is related to the density of dark matter, see Sect. 4.1.

Quintessencelike models, see Sect. 4.2.

A generic hidden sector scalar field [44].

Kaluza–Klein models/moduli models [43]. In these models the size of compactified extradimensions can be described by a generic scalar field (the moduli field); if the size of extradimensions changes with cosmological time, the scalar field would have a cosmological time evolution. Generically speaking, in string theory coupling constants are moduli fields. Each coupling constant has its moduli field and its expectation value fixes the value of the coupling constant.

Dilaton field models, see e.g. [41, 42]. These are similar to moduli models, but dilaton fields are expected to couple universally to matter, like gravity. These models include Brans–Dicke fields and also scalar fields that are coupled nonminimally to the Ricci scalar R.

Soliton models, transient phenomena, cosmic strings, domain walls, and kink solutions would also be accounted for by a simple scalar field; see Sect. 4.3.
One expects on very general grounds that quantum gravity will generate an interaction between any scalar field ϕ and regular matter with \(d_{j}^{(i)}\sim {\mathcal{O}}(1)\), whether such a coupling exists or not when gravity decouples [44–48]. However, very light scalar fields coupling linearly to regular matter (i.e. dimension5 operators) are essentially ruled out by the Eöt–Wash torsion pendulum experiment [49–52] for \(d_{j}^{(1)}\sim {\mathcal{O}}(1)\). Indeed, Eöt–Wash’s data imply that if \(d_{j}^{(1)}\sim 1\), the mass of the scalar field must satisfy \(m_{\phi}>10^{2}\text{ eV}\). If a neutral scalar field with \(m_{\phi}<10^{2}\text{ eV}\) and a linear coupling to regular matter was found by some experiment, we would learn that dimension5 operators are not generated by quantum gravity. On the other hand, nonlinear couplings are far less constrained by current experiments (see Sect. 4.5). This provides a very important test of quantum gravity [44–48].
Besides tests of quantum gravity, a time variation of fundamental parameters would enable tests of grand unified theories [53–64], because in grand unified models, shifts in, e.g., the fine structure constant α and the coupling constant of quantum chromodynamics \(\alpha _{s}\) are related. The same can apply also to shifts in lepton and quark masses. In grand unified theories, the relations between the different fundamental parameters are strongly model dependent. This is why very lowenergy measurements can be used to probe very high energy theories (see Sect. 4.5). Spacetime variations of the fine structure constant have also been studied in the context of violations of fundamental symmetries [65–67]. More generally, similar experimental techniques for probing the stability of fundamental constants have led to stringent constraints on violations of Lorentz and CPT invariance, diffeomorphism invariance and the equivalence principle [68] (see Sect. 4.4). Definitions of various spacetime transformations can be found in, e.g. Ref. [69].
We hope this short introduction to the theoretical framework underlying QSNET will have convinced the reader of the richness of the science that can be investigated by probing the time variation of fundamental constants. We can study cosmology by looking for a field responsible for the expansion of the universe, but also astrophysics by searching for extremely light dark matter. We can also probe fundamental high energy theories of particle physics and the symmetries of an ultraviolet complete theory of everything. Indeed, in the next sections, we will show that one can probe fundamental physics at the Planck scale and test grand unification physics, quantum gravity, and the fundamental symmetries of nature with tabletop experiments.
3 Clock network
In this section we describe how atomic and molecular clocks can be used to detect variations of fundamental constants, and we discuss the advantages of a networked approach. We then describe the clocks of the QSNET network and derive the performance that could be achieved in terms of sensitivities to variations of α and μ.
3.1 Clocks and fundamental constants
All atomic and molecular energy spectra depend on the fundamental constants of the Standard Model. For example, the scale of atomic transitions is set by the Rydberg constant, which can be written as
with both the electron mass \(m_{e}\) and the fine structure constant α being fundamental constants of the Standard Model. It follows that, if these constants vary either in space or time, then so do atomic and molecular spectra. Clocks based on atoms or molecules rely on using the frequency of a spectral line to set the rate at which a clock ‘ticks’. Changes in the spectra will therefore result in changes in the clock frequencies. The narrower the spectral line, the more precisely the clock frequency can be determined and the better the resolution for detecting any changes. The most favourable species to be used for clocks are therefore those which possess transitions that are narrow in frequency (forbidden at least to first order) and not easily perturbed by changes in background electric or magnetic fields. Optical atomic clocks have already been demonstrated to achieve fractional frequency instabilities and inaccuracies at the level of 10^{−18} and below [16, 17], making them among the most precise measurement instruments ever built. Highprecision spectroscopy with atomic clocks has therefore provided some of the tightest constraints on variations of α and the electrontoproton mass ratio \(\mu =m_{e}/m_{p}\) [18–21], with \(m_{p}\) the proton mass.
Depending on the nature of the transition employed, different clocks are more or less sensitive to variations of specific fundamental constants. To illustrate this, let us express the frequency of clocks employing optical transitions as
with A a constant depending on the specific atomic species and transition and \(F_{\mathrm{opt}}(\alpha )\) describing the relativistic correction to the specific transition. In contrast, microwave (MW) clocks utilise transitions between hyperfine energy levels, whose frequency can be written as
where B is a constant that depends on the specific atomic species and transition and \(F_{\mathrm{MW}}(\alpha )\) is the relativistic correction to the specific MW transition. Finally, the frequency of molecular clocks based on vibrational transitions can be expressed as
with C a constant depending on the specific molecule and transition used.
The sensitivity of a certain atomic or molecular transition \(\nu _{i}\) to variations of a fundamental constant \(X=\{\alpha ,\mu \}\) is characterised by a sensitivity coefficient \(K_{X}\), which we define as
The larger the value of \(K_{X}\), the more sensitive a specific transition is to variations of X. From Eq. (7), and using Eqs. (4), (5) and (6), it follows that
The sensitivities of optical and MW transitions to variations of α are calculated by numerically varying the value of α in the computation of atomic spectra [70, 71]. Note that the magnitude of \(K_{\alpha}\) generally increases in heavier atomic systems due to increased relativistic effects [72–74]. Similarly, we obtain
To measure variations of fundamental constants using atomic or molecular clocks, the frequency of one clock relative to another, i.e. their frequency ratio, needs to be measured over time. As dimensionless quantities, frequency ratios also avoid any ambiguities of whether the system of units employed in the measurements is varying over time or not. For a given frequency ratio \(R=\nu _{1}/\nu _{2}\), the sensitivity to variations of a certain fundamental constant X is proportional to the difference between the sensitivity coefficients, i.e.:
Ratios of transitions with similar sensitivity coefficients are therefore almost insensitive to variations of X, whereas comparing two transitions with large magnitudes of \(K_{X}\) and of opposite signs greatly boosts the sensitivity. In the case of combinations of transitions that are sensitive to variations of more than one fundamental constant, the different contributions are weighted with the corresponding values of \(K_{X,1}K_{X,2}\).
From Eqs. (8) and (9), it follows that the ratio between the transition frequencies of two optical or two microwave clocks is only appreciably sensitive to variations of α via the transitionspecific relativistic correction factors \(F(\alpha )\). However, a ratio between an optical clock and a microwave clock is sensitive both to variations of α and μ as is a frequency ratio between a molecular vibrational transition and an optical atomic transition.
3.2 Networks of clocks for measuring the stability of fundamental constants
To perform the clocktoclock comparisons needed to measure variations of fundamental constants, clocks can be networked online using either satellite [24] or fibre links [26], or offline via timestamping of measurements [25].
In QSNET, the clocks in the network will be linked with optical fibres. Over distances of several hundred kilometres, the frequency uncertainties introduced by phase noise in the optical fibre links can be cancelled to a level well below the measurement uncertainties from the clocks themselves. The signal that is sent through the fibres will be an optical carrier frequency from a transfer laser, around \(1.5~\mu{\mathrm{m}}\) in wavelength. A frequency comb at each end of the fibre will be used to measure the local clock frequency relative to the transfer laser, and the exact frequency of the transfer laser cancels out in the ratio of the clock frequencies. Large networks of telecom fibres already exist; however, it is important to cancel the phase noise that is picked up by the light along the fibre route. This is standard practice in optical frequency transfer for precision metrology. The phase noise is monitored by setting up an interferometer with a fraction of light that has been backreflected from the far end of the fibre being compared against the incident light. A correction signal can then be applied to an acoustooptic modulator to cancel the noise.
Existing telecom fibres can be used for the networking, but some modifications are required to ensure the infrastructure is suitable for transferring ultrastable optical frequencies between the clocks. Most notably, any telecom equipment that relies on opticaltoelectrical conversion along the fibre route must be replaced or circumvented by alloptical amplifiers to avoid scrambling the phase of the transfer laser. The alloptical amplifiers must also be bidirectional to allow backreflected light to be used in the interferometer for phasenoise cancellation. Changing the amplifiers affects all channels on a fibre and, for this reason, amplifiers cannot be switched out on fibres carrying live telecom signals to other users. It is therefore necessary to use ‘dark fibres’, i.e. existing telecom fibres that have no other users at present. Dark fibre routes are available between all the partners in QSNET. A recent demonstration, transferring ultrastable frequencies along a 2220km dark fibre link, has shown that noise from the link can be cancelled to the level of 10^{−16} in 10 s [75] and much lower with longer averaging times. This is already sufficient to avoid degrading comparisons between the pairs of clocks proposed in QSNET and strategies exist to reduce the link noise even further, as clocks improve in the future.
This networked approach is an important aspect of the QSNET project. While each clock pair is an excellent detector for searches of variations in fundamental constants, by combining them into a network, better sensitivities, very high detection confidence, and new capabilities can be achieved. The networked approach brings both technological and scientific advantages:
Technological advantages

A network makes it possible to compare two clocks in different locations, thus exploiting the resources and expertise spread across different institutes. No single institution has the range of expertise required to run a sufficiently large and diverse set of clocks with different sensitivities to variations of fundamental constants. A network makes it easy to compare a diverse range of systems, such as highly charged ion clocks, molecular clocks and nuclear clocks, as well as more standard atomic clock systems.

Validation of the results can be achieved with simultaneous measurements from multiple pairs of clocks. Ideally, the clocks should be in different environments and with different sensitivities to systematic frequency offsets.
Physics advantages

Networks enable probing of spacetime correlations [23]. These correlations increase the detection confidence and provide added information, such as the speed and directionality of the oscillating dark matter fields discussed in Sect. 4.1.

Networking is the only possibility of detecting transient events linked to macroscopic dark objects, such as topological defects, solitons, Qballs and dark stars. This is discussed in Sect. 4.3. Correlation functions across the network are important in discriminating noise from transient effects linked to darksector fields [76].

Networking is ideal for implementing dark matter detection using both variations of α and μ, which is instrumental in discriminating between models that predict a variation of the unified coupling constant or a timevariation of the unification scale, or both; see the discussion in Sect. 4.5 and e.g. [77–79] and references therein.

Similarly, using a network of different types of sensors can veto noise and make it possible to determine the origin of a signal. For example, in a clock network combined with the Global Network of Optical Magnetometers for Exotic Physics (GNOME), correlation of readouts from optical and nonoptical magnetometers can be used to rule out magnetic artifacts, such as solar wind [76].

Having N pairs of clocks within the coherence length of oscillating darksector fields can improve the limit from a single pair of clocks by a factor \(\sqrt{N}\) [23], increasing the signal to noise ratio.

It has been suggested that a global network of entangled clocks could give an international time scale with unprecedented stability and accuracy [80]. There are also suggestions of how to use entanglement in local networks to measure noncommuting observables, e.g. different components of a field [81], or to deal with nuisance parameters [82]. Those ideas for using quantum correlations across a network might, in the future, be used to improve the precision when estimating nonlocal parameters, i.e. ones that are a function of the values at the different spatially separated sensors [83]. The question of how to measure such correlations through an optical fibre network is a good topic for future research.
3.3 The QSNET network
In this subsection we discuss the clocks being developed within QSNET. As summarised in Fig. 1, these include Yb^{+} and Cf highly charged ion clocks with enhanced sensitivity to variations of α; Cs, \(\text{N}_{2}^{+}\) and CaF clocks, that are most sensitive to variations of μ; and a Sr clock, that has \(K_{\mu}=0\) and \(K_{\alpha}\) close to zero. For the established clocks, we discuss the stateoftheart and provide the current measurement limits set by systematic uncertainties. For the nextgeneration molecular and highly charged ion clocks, we instead predict their systematic uncertainties based on realistic assumptions. More details are provided in Appendix A.
3.3.1 Established standards
Atomic clocks are already very welldeveloped on certain atomic transitions, particularly those which are used as frequency standards in national measurement institutes. In QSNET, three established clocks will be used in the network: a microwave ^{133}Cs clock, and optical clocks based on ^{87}Sr and ^{171}Yb^{+}. More details are given in Appendix A.1 about these systems and the current stateoftheart performances that have been achieved.
Of all the species used for atomic clocks, caesium is the most common. This is because the definition of the SI second is based on fixing the value of the transition frequency between the ^{133}Cs hyperfine ground states to be exactly \(9\text{,}192\text{,}631\text{,}770\text{ Hz}\). See Fig. 2 for the relevant energy levels involved in this microwave clock transition. The highest accuracy Cs clocks rely on laser cooling the atoms in a magnetooptical trap and then launching them vertically in a ‘fountain’ configuration. These fountain clocks allow the atoms to pass twice through a microwave cavity: once on the way up and then a second time on the way down. The two interactions with the microwave cavity constitute separated Ramsey pulses that drive the clock transition. The Ramsey dark time is \({\sim} 1\text{ s}\), leading to Ramsey fringes with a linewidth at the Hz level. There are several stateofthe art Cs fountain clocks around the world [84–88], all operating with fractional frequency uncertainties at the level of \(1\text{}2 \times 10^{16}\) from systematic shifts; see Appendix A.1.1. A caesium clock is useful in the QSNET network because its transition frequency is sensitive to changes in both the fine structure constant (\(K_{ \alpha} = 2.83\)) and the electrontoproton mass ratio (\(K_{\mu} = 1\)).
The fermionic isotope of strontium, ^{87}Sr, is one of the most commonly used species for optical atomic clocks. The ‘forbidden’ \({}^{1}{\mathrm{S}}_{0} \rightarrow {}^{3}{\mathrm{P}}_{0}\) transition at 698 nm provides a suitable clock transition with a linewidth of \(2\pi \times 1\text{ mHz}\), as shown in Fig. 2. The cooling transitions are readily accessible with diode lasers and clouds of about 10^{4} atoms can be trapped in an optical lattice potential, formed from a standing wave of laser light. The standing wave is tuned close to a ‘magic wavelength’ at 813 nm, where the differential polarisability between ground and excited states is zero, leading to cancellation of the AC Stark shift. The ^{87}Sr clock has very small sensitivity factors, \(K_{\alpha} = +0.06\) and \(K_{\mu} = 0\). This is useful when comparing against clocks with larger sensitivities because it allows the corresponding frequency ratio to have a large differential sensitivity to variations in the constants. The current stateoftheart for the ^{87}Sr optical lattice clock has an estimated fractional frequency uncertainty from systematic shifts of \(2.0 \times 10^{18}\) [89]. The uncertainty budget is discussed in Appendix A.1.2.
Finally, QSNET will exploit singlycharged ytterbium, ^{171}Yb^{+}, which has two optical clock transitions that are used as frequency references, as shown in Fig. 2. One is based on the electric quadrupole (E2) transition \({}^{2}{\mathrm{S}}_{1/2} \rightarrow {}^{2}{\mathrm{D}}_{3/2}\) at 436 nm with a \(\text{linewidth} = 2\pi \times 3\text{ Hz}\), while the other is based on the electric octupole (E3) transition \({}^{2}{\mathrm{S}}_{1/2} \rightarrow {}^{2}{\mathrm{F}}_{7/2}\) at 467 nm with a linewidth ∼ nHz. Both of these transitions have a good sensitivity to changes in the fine structure constant, but the octupole transition is significantly more sensitive with \(K_{\alpha}^{E3} = 5.95\), compared to the electric quadrupole transition with \(K_{\alpha}^{E2} = +1.00\) [29]. The E3 transition is also less perturbed than the E2 transition by background electric and magnetic fields, giving rise to a lower uncertainty contribution from systematic shifts for the E3 transition frequency. The current stateoftheart for the E3 transition of ^{171}Yb^{+} has an estimated fractional frequency uncertainty from systematic shifts of \(2.7 \times 10^{18}\) [90]. The uncertainty budget is discussed in Appendix A.1.3.
3.3.2 Molecular clocks
We propose a molecular lattice clock based on the fundamental vibrational transition in CaF, which has a frequency \(f_{0} = 17.472\text{ THz}\), an estimated linewidth of 0.7 Hz, and \(K_{\mu}=0.5\). The main ideas for such a clock were presented in [91]. Figure 3 shows the relevant energy levels of CaF. The electronic transitions \(A ^{2}\Pi _{1/2}X^{2}\Sigma ^{+}\) and \(B ^{2}\Sigma ^{+}X^{2}\Sigma ^{+}\) are used to lasercool the molecules to a few μK using the methods described in [92–96]. They can then be loaded into an optical dipole trap [97] or an optical lattice. For the clock transition, we choose to drive the Raman transition from \( v,N,F,m \rangle =  0,0,F,m \rangle \) to \( 1,0,F,m \rangle \). All four choices of \((F,m)\) are useful for controlling systematic shifts. By choosing a transition that leaves N unchanged, the upper and lower states have almost identical properties, so Zeeman, DC Stark and AC Stark shifts all cancel to high accuracy. Furthermore, because \(N=0\) in both states, problematic tensor Stark shifts are eliminated. In the optical lattice, the molecules are deep in the Lamb–Dicke regime which eliminates firstorder Doppler shifts. A 3D lattice also eliminates collisional shifts. Furthermore, the \(N=01\) rotational transition at 20.5 GHz can be used to measure the lattice intensity and the local electric and magnetic fields to high accuracy, further improving the accuracy of the clock. In Appendix A.2 we discuss a set of parameters that will allow us to reach a fractional frequency uncertainty from systematic shifts of \({\simeq}7.5\times 10^{18}\).
The QSNET network will include a second molecular clock with comparable sensitivity to variation of μ but different systematic uncertainties. Recently, molecular nitrogen ions have been proposed as a candidate for precision spectroscopy [98]. The vibrational clock transition at 129.4 THz has an estimated linewidth on the order of nHz and a sensitivity of \(\mathrm{K}_{\mu}= 0.5\).^{Footnote 1} The systematic shifts are predicted to be comparable with the current best optical clocks, facilitating frequency measurements at an uncertainty below 10^{−18}. Within nitrogen molecular ions, there are two promising transitions with small systematic shifts and high sensitivity to changes in the electrontoproton mass ratio, as shown in Fig. 3. The direct transition between the rovibrational ground state \(\nu =0\), \(N=0\) and the \(\nu =2\), \(N=2\) state is electricquadrupole allowed and has been demonstrated by Germann et al. [99]. The transition between the \(\nu =0\), \(N=0\) and the \(\nu =2\), \(N=0\) states with a transition frequency of 129.4 THz has not been investigated yet but was proposed in [98] and exhibits smaller systematic shifts for the \(I=0\) isotopomer. \(\text{N}_{2}^{+}\) has a \(\text{X}^{2}\Sigma _{g}^{+}\) ground state described by Hund’s case (b) with the angular momentum being solely the electron’s spin. Hence, the interaction with external magnetic fields is dominated by the interaction with the electron’s magnetic moment. While there is a strong linear Zeeman shift between the magnetic sublevels of \(1.4~\text{MHz}/\mu \text{T}\), the differential shift of the two clock levels is exactly zero. Also, the quadratic Zeeman shift is zero, which makes transitions between the states with the same magnetic quantum number insensitive to external magnetic fields even at the second order. Due to the Σ character of the electronic ground state, there is no permanent quadrupole moment which can interact with the trap electric field in the rotational ground state. Hence, the \(\text{X}^{2} \Sigma _{g}^{+}\), \(N=0\) ground state does not show a quadrupole shift. This is particularly important because, to conduct high resolution spectroscopy, molecular ions need to be trapped alongside atomic ions for sympathetic cooling and state detection. This inevitably results in a local electric field gradient that would cause a quadrupole shift. In Appendix A.3 we evaluate that the fractional frequency uncertainty from systematic shifts for \(\text{N}_{2}^{+}\) is \({\simeq}3.9\times 10^{18}\) under conditions that can be easily reached in current experiments.
3.3.3 Highly charged ion clocks
Novel technological platforms are currently being explored to develop clocks with enhanced sensitivity to variations of α. There are two promising avenues that could be followed. One regards the development of a nuclear clock [100, 101]. The other involves the use of various transitions in highly charged ions (HCI) [102–104]. The estimates of potential accuracy of nuclear and HCI clocks are similar, but HCI do not have the complication of 150 nm clock transition wavelength that also imply the design of new frequency combs with sufficient power. Recent experimental breakthroughs [105, 106] allow the HCIs to be cooled to temperatures below 1 mK, where high resolution spectroscopy and advanced techniques such as quantum logic spectroscopy can be used [105, 107].
HCIs are good candidates for searching for variation of the fine structure constant α: they are less sensitive to external perturbations due to their compact electronic cloud and their sensitivity to variation of α is enhanced due to larger relativistic effects. A vast number of highly charged ions can exist in stable form, however to reach the level of accuracy and stability needed to measure variations of α, it is required that they: (i) feature optical transitions (≃200–1000 nm); (ii) have lifetimes of the excited clock state between 1 and 10^{4} s; (iii) have high sensitivities to variations of α. Additionally, it is desirable that other strong transitions could be used for cooling and/or detection, and that the clock levels are suitable for cancellation of various systematic shifts. Another desirable feature is a relatively simple electronic structure to enable precision calculation of the atomic properties and significantly easier spectra identification. A handful of HCIs which satisfy all of these requirements have been identified, among them the californium ionisation states Cf^{15+} and Cf^{17+} that have been chosen for the QSNET project. The lowlying level structures for Cf^{15+} and Cf^{17+} are shown in Fig. 4 [30], together with the corresponding K enhancement factors [104]. The Cf^{15+} HCI features a clock transition at 618 nm with \(K_{\alpha}=+47\) and a predicted linewidth of order mHz, while the Cf^{17+} HCI has a clock transition at 485 nm with \(K_{\alpha}=43.5\) and a linewidth of \({\simeq}0.5\text{ Hz}\). In Appendix A.4 we evaluate that under realistic conditions, it would be possible to reach fractional frequency uncertainty on the order of 10^{−19} for both ionisation states. Additionally, the possibility of realising a dual clock cotrapping Cf^{15+} and Cf^{17+} is particularly appealing due to the opposite sign of the large K coefficients of the clock transitions and the cancelling of any residual common systematic effect. Finally, both ionisation states of Cf feature a relatively strong M1 transition that could be used for direct detection.
3.4 Predicted performance
In this subsection we estimate the sensitivity of the QSNET clocks to variations of α and μ on different timescales. The fractional frequency uncertainty with which the clocks can be operated will depend on both the inaccuracy, as determined by the systematic uncertainties described in the subsection above and Appendix A, and the instability. Ignoring additional factors of order 1, the fractional frequency instability for the different clocks can be estimated according to [108]:
where Δν and \(\nu _{0}\) are the linewidth and frequency of the probed transition, N is the number of atoms, \(T_{c}\) is the cycle time of the experiment and τ is the total measurement time. Under the assumption that the probe time \(T_{p}\) completely dominates the measurement cycle time, then \(T_{c} = T_{p}\). Futhermore, assuming the natural linewidth of the atomic transition is sufficiently small, then the resolved linewidth will be determined by the Fourier transform limit of the probe time, \(\Delta \nu \sim 1/T_{p}\). Accordingly, the fractional frequency instability can be expressed as
For each clock, we calculate the fractional uncertainty as
where \(\sigma _{i}\) is the inaccuracy for the specific clock, as reported in Sect. 3.3 and calculated in Appendix A. For CaF and Cs we set \(T_{p}=190\) and 1000 ms, respectively,^{Footnote 2} while for all the other clocks \(T_{p}=500\text{ ms}\). For Sr and Cs clocks the number of atoms are \(N\simeq 10^{4}\) and \(5\times 10^{6}\) respectively, while for the CaF clock we aim to use \(N=10^{4}\) molecules. For all the ion clocks \(N=1\). The resulting fractional uncertainties as a function of the integration time τ are reported in Fig. 5(a). From the values of σ for each clock it is then possible to estimate the sensitivity to variations of α or μ using Eq. (10). The results are reported in Fig. 5(b) and (c) for the clocktoclock comparisons that deliver the best performance.
It is a wellknown consequence of general relativity that time runs at different rates in different gravity potentials, where the term ‘gravity potential’ includes both gravitational and centrifugal components. If a clock on the surface of the Earth experiences a height change of 1 cm, this will change the frequency of the clock by one part in 10^{18}. When looking for variations in fundamental constants at this level of precision, care must therefore be taken to avoid confusion with any frequency changes brought about by gravitational effects. For two clocks operated in the same location (and at the same height), gravitational effects are commonmode and will not alter the frequency ratio between the clocks. However, if two clocks are in different locations, as proposed in QSNET, they can be subject to gravity potential differences. Any static difference in the gravity potential (for example due to a constant height offset between the clocks) will lead to a constant offset in the frequency ratio and is irrelevant for QSNET, which is concerned only with temporal changes in frequency ratios as a signature of changes in fundamental constants. It is therefore only timevarying differences in the gravity potential that might need to be taken care of. Such timevarying effects can arise from a variety of sources including solid Earth tides, ocean tides and nontidal mass redistributions in the atmosphere and oceans [109]. By far the largest contribution to timevarying gravity potentials is from solid Earth tides, which can create fractional changes in individual clock frequencies with peaktopeak variations up to \(5\times 10^{17}\) over timescales of several hours. However, the effect on the frequency ratio between two clocks depends on the gravity potential difference between them. The clocks involved in QSNET are all located in the UK, within 2 degrees of longitude of each other, thus sharing a large commonmode component in the timevarying potential. This means that the largest timevarying effect from gravity potentials on the frequency ratios involved in QSNET is at or below the level of 10^{−18} over several hours. Both solid Earth tides and ocean tides are highly predictable and their effects can be modelled and subtracted from the data. In particular, they are oscillatory in nature with characteristic timescales of several hours so are easily distinguished from oscillations at all other timescales. Furthermore, in the case of an oscillating darkmatter field (see Sect. 4.1), the signal is expected to be nearly monochromatic with a quality factor of \(Q \sim 10^{6}\), which is higher than that for oscillatory changes in Earth’s gravity potential. Far smaller frequency offsets can also arise from nontidal mass redistributions, which can include gravity potential effects that are nonperiodic and hard to predict, such as the influence of local weather conditions. Disturbances from these nonperiodic effects on an individual clock frequency would produce transient offsets, similar to those caused by any other localised disturbances in a specific laboratory. The networked approach, however, is resilient to these local disturbances. Transient effects are disregarded unless they are correlated with other independent frequency ratios that have been measured in different locations. This avoids mistaking technical noise in a given system for evidence of new physics on a global scale. In summary, careful attention should be paid to the frequency offsets created by timevarying gravity potentials but they do not prevent the searches for new physics using the network of clocks proposed in QSNET.
4 Phenomenology
In this section, we evaluate how QSNET can probe some specific dark matter and dark energy models, namely ultra light dark matter models in Sect. 4.1, quintessence dark energy models in Sect. 4.2, and solitonic dark sector models in Sect. 4.3. Additionally, we show in Sect. 4.4 that QSNET can probe fundamental spacetime symmetries. Finally, in Sect. 4.5 we discuss how QSNET can provide stringent tests of grand unification theories and quantum gravity. In this section, unless explicitly stated otherwise, we employ the natural units \(\hbar = c = 1\).
4.1 Dark matter
Dark matter comprises about 85% of the total matter content of the universe. To date, all available evidence for dark matter has involved the gravitational effects of dark matter on “visible” ordinary matter. Nevertheless, it is generally expected that dark matter should also interact nongravitationally with ordinary matter, albeit feebly. Over the past few decades, the majority of experimental efforts in direct dark matter searches with terrestrial detectors have focused on weaklyinteracting massive particles (WIMPs) in the \({\sim}\mathrm{GeV}\text{}\mathrm{TeV}\) mass range [110]. In light of the continued absence of strong experimental evidence for WIMPs, there has been growing interest over the past decade in performing searches for darkmatter candidates other than WIMPs, in particular for feeblyinteracting, lowmass bosonic particles [111–113]. The axion (a pseudoscalar particle) is the leading candidate to explain the strong CP problem of quantum chromodynamics [114–121], whilst also being an excellent candidate for cold dark matter [122–124].
Lowmass spinless bosons may be produced nonthermally via the “vacuum misalignment” mechanism [122–124] and subsequently form a coherently oscillating classical field, which in the rest frame is given by:
which occurs, for example, in the case of the harmonic potential \(V(\phi ) = m_{\phi}^{2} \phi ^{2} / 2\) when \(m_{\phi}\gg H\), where \(m_{\phi}\) is the boson mass and H is the Hubble parameter that describes the relative rate of expansion of the universe. The scalar field in Eq. (14) carries an energy density, averaged over a period of oscillation, of \(\langle \rho _{\phi} \rangle \approx m_{\phi}^{2} \phi _{0}^{2} / 2\). Since presentday dark matter must be cold, all of the boson energies satisfy \(E_{\phi}\approx m_{\phi}c^{2}\), which implies that the oscillations of the field in Eq. (14) are temporally coherent on sufficiently small time scales (and are also spatially coherent on sufficiently small length scales). Over time, the galactic dark matter is expected to have become virialised, attaining a rootmeansquare speed of \({\sim}10^{3} c\) in our local galactic region. The typical spread in the boson energies is hence \(\Delta E_{\phi}/ E_{\phi}\sim \langle v_{\phi}^{2} \rangle / c^{2} \sim 10^{6}\), implying a coherence time of \(\tau _{\mathrm{coh}} \sim 2 \pi / \Delta E_{\phi}\sim 10^{6} T_{\mathrm{osc}}\), where \(T_{\mathrm{osc}} \approx 2 \pi / m_{\phi}\) is the period of oscillation. In other words, the oscillations of the bosonic field are practically monochromatic, with an associated quality factor of \(Q \sim 10^{6}\). The spatial gradients associated with the field \(\phi (t,\boldsymbol{x}) \approx \phi _{0} \cos ( m_{\phi}t  m_{\phi}\boldsymbol{v}_{\phi}\cdot \boldsymbol{x} )\) give rise to a coherence length of \(\lambda _{\mathrm{coh}} \sim 2\pi / (m_{\phi}\sqrt{\langle v_{\phi}^{2} \rangle })\), which is ∼10^{3} times the Compton wavelength. On time and length scales exceeding the coherence time and coherence length, respectively, the stochastic nature of the bosonic field needs to be taken into account [23, 125]. In particular, the bosonic field amplitudes \(\phi _{0}\) are expected to follow a Rayleightype distribution, while the bosonic particle velocities \(\boldsymbol{v}_{\phi}\) are expected to follow a Maxwell–Boltzmanntype distribution.
In Appendix B.1, we discuss the relevant range of bosonic darkmatter particle masses, which is \(10^{21}~\mathrm{eV} \lesssim m_{\phi}\lesssim 1~\mathrm{eV}\), corresponding to oscillation frequencies in the range \(10^{7}~\mathrm{Hz} \lesssim f \lesssim 10^{14}~\mathrm{Hz}\). The lower end of this frequency range corresponds to periods of oscillation of the order of a month and the upper end corresponds to the infrared region of the electromagnetic spectrum. Searching for possible particlelike signatures of such lowmass dark matter is practically impossible, since the kinetic energies of nonrelativistic verylowmass particles are extremely small and typically many orders of magnitude below the energy thresholds of conventional WIMP detectors. On the other hand, it may be possible to take advantage of wavelike signatures of lowmass bosonic dark matter due to the large number density of the bosons. While searches for wavelike signatures of the oscillating classical field in Eq. (14) via its gravitational effects (e.g., using pulsar timing methods [126, 127]) are limited to the lowest allowable darkmatter particle masses, much larger ranges of darkmatter particle masses may be probed if the bosonic field interacts nongravitationally with fields from the Standard Model sector.
In particular, atomic clocks are excellent detectors to search for “scalartype” interactions, either via comparisons with other clocks [10–12, 21, 128–130] or via referencing against cavities [11, 25, 131, 132]. The QSNET clock network is particularly wellsuited to search for scalartype interactions of a spinless darkmatter field with the electromagnetic field and electron. From Eq. (1), the lowest order of such interactions involves the first power of the scalar field ϕ:
where we have defined \(1/\Lambda _{\gamma}\longleftrightarrow \kappa d_{e}^{(1)}\) and \(1/\Lambda _{e} \longleftrightarrow \kappa d_{m_{e}}^{(1)}\). The parameters \(\Lambda _{\gamma ,e}\) denote the effective newphysics energy scales of the underlying model; higher energy scales correspond to feebler interactions (for comparison, the effective energy scale associated with the usual gravitational interaction is set by the reduced Planck scale).
Comparing the interactions in Eq. (15) with the corresponding terms in the Standard Model Lagrangian, \(\mathcal{L}_{\text{Standard Model}} \supset  F_{\mu \nu} F^{\mu \nu} / 4  e J_{\mu}A^{\mu} m_{e} \bar{\psi} \psi \), where −e is the electric charge carried by an electron, \(J^{\mu}= \bar{\psi} \gamma ^{\mu}\psi \) is the electromagnetic 4current and \(A^{\mu}\) is the electromagnetic 4potential, shows that the oscillating field in Eq. (14) induces the following apparent oscillations of the electromagnetic fine structure constant α and the electron mass [11]:
If the linearinϕ interactions in Eq. (15) are precluded, e.g. if the underlying model admits a \(Z_{2}\) symmetry under the \(\phi \to  \phi \) transformation, then the lowestorder interactions would involve the second power of the scalar field ϕ, as described by Eq. (2). It follows that Eqs. (15) and (16) are modified according to [11, 12]:
The apparent oscillations of the fundamental constants in Eqs. (16) and (18) would cause atomic and molecular transition frequencies to undergo small oscillations about their mean values. Therefore, from Eq. (10) we obtain that the comparison of two atomic transition frequencies in time would also undergo small oscillations:
where the signal frequency is given by \(f_{\mathrm{signal}} \approx m_{\phi}c^{2} / h\) in the case of linearinϕ interactions (15) or \(f_{\mathrm{signal}} \approx 2 m_{\phi}c^{2} / h\) in the case of quadraticinϕ interactions (17).
As discussed in Sect. 3.1, the sensitivity coefficients \(K_{X}\) in Eq. (19) depend on the specific transitions under consideration. All of the transitions that will be utilised within the QSNET network are summarised in Fig. 1. The estimated performances of QSNET are discussed in Sect. 3.4, and are reported in Fig. 5. From these, we can estimate the sensitivity of the QSNET network to apparent oscillations of the fundamental constants induced by an oscillating darkmatter field via linearinϕ and quadraticinϕ interactions. The results are reported in Figs. 6 and 7, respectively. In this case, the signaltonoise ratio (SNR) generally improves with the total measurement time \(t_{\mathrm{int}}\) as \(\mathrm{SNR} \propto t_{\mathrm{int}}^{1/2}\). We assume \(t_{\mathrm{int}} = 1~\mathrm{year}\), with individual data points sampled every \(\tau =1~\mathrm{s}\). Additional details are discussed in Appendix B.2.
In Figs. 6 and 7, we assume that the ultralowmass bosons saturate the observed dark matter abundance when possible. For the boson masses \(m_{\phi}\lesssim 10^{21}~\mathrm{eV}\), for which bosons cannot comprise the entirety of the observed dark matter, we assume that such bosons make up a maximally allowable fraction of the dark matter, which is \(\mathcal{O}(10\%)\) in this case (see also Appendix B.1). Since the newphysics energy scales appear in the clockbased observables in the combination \(\sqrt{\rho _{\phi}} / \Lambda _{X}\) or \(\sqrt{\rho _{\phi}} / \Lambda '_{X}\), the sensitivity to \(\Lambda _{X}\) or \(\Lambda '_{X}\) is only weakened by a factor of ≈3 in this case, compared to the case when dark matter is saturated entirely by these bosons.
In the case of linearinϕ interactions, we also show existing limits from previous searches for oscillating darkmatter signatures via clock comparisons [21, 128, 129], clockcavity comparisons [132], optical interferometry [133] and a resonantmass detector [134], as well as complementary bounds from searches for equivalenceprincipleviolating forces [135–138]. In the case of the clock and cavitybased bounds, we have taken into account a degradation factor of ≈3 due to only partial sampling of the distribution of stochasticallyfluctuating scalarfield amplitudes [139]. In the case of quadraticinϕ interactions, we also present existing limits from previous searches for oscillating darkmatter signatures via clock comparisons [12, 130], as well as complementary types of bounds from searches for equivalenceprincipleviolating forces [14] and measurements and calculations pertaining to big bang nucleosynthesis [12]. The limits on linearinϕ interactions from searches for equivalenceprincipleviolating forces do not involve any assumptions about the possible contribution of the ϕbosons towards the observed darkmatter abundance, whereas all of the other types of limits do. We remark that, in the case of \(\phi ^{2}\) couplings, the bosonic darkmatter field can be screened near Earth’s surface; however, such screening is negligible for the majority of the parameter space that is relevant for the QSNET clock experiments [14].
From our analysis, we see that the QSNET network has the potential to probe large regions of previously unexplored parameter space in models of oscillating scalar darkmatter fields.
4.2 Dark energy
It is now well established that our universe has been undergoing accelerated expansion over the past several billion years. A cosmological constant in Einstein’s equations that is characterised by an energy scale of \(\Lambda \sim 10^{3}\text{ eV}\) can account for this observed acceleration. Together with the cold dark matter, this corresponds to the ΛCDM cosmological model. While current cosmological data are fully consistent with the presence of a cosmological constant, the tiny energy scale \({\sim} 10^{3}\text{ eV}\) is unexplained and much smaller than other relevant energy scales in nature, such as the Planck scale in gravity or the electroweak scale in particle physics. This observation has motivated a class of models known as quintessence, in which the cosmological constant is replaced by a dynamical scalar field; see, e.g., [140] for a review. In quintessence models, gravity is described by General Relativity and the matter content of the universe consists of radiation, dark matter, visible matter and quintessence, which is a scalar field ϕ that evolves on a cosmological time scale. If the quintessence field couples to visible matter, fundamental constants could be slowly evolving with cosmological time. In particular, if the quintessence field couples linearly to matter as in Eq. (1), then slow changes in the values of the fundamental constants may leave an imprint on clock experiments.
The classical equation of motion for a scalar field ϕ with potential \(V(\phi )\) in an expanding universe reads as follows:
where \(H(t)\) is the Hubble parameter that describes the relative rate of expansion of the universe and the Lagrangian \(\mathcal{L}_{\mathrm{int}} (\phi )\) encodes the nongravitational interactions of the scalar field with ordinary matter. A wide variety of potentials that admit a slow evolution of ϕ at the present day are possible; see, e.g., Refs. [141–153]. The key features of quintessence models can be understood by considering the simple example of the harmonic potential \(V (\phi ) = m_{\phi}^{2} \phi ^{2} / 2\) and the limiting case of sufficiently feeble interactions, in which case the classical equation of motion (20) simplifies to:
which represents the equation of motion for a damped harmonic oscillator. In the strongly overdamped regime when \(m_{\phi}\ll 3H/2\), ϕ remains approximately constant over time and so does not appreciably affect the values of the fundamental constants. On the other hand, in the strongly underdamped regime when \(m_{\phi}\gg 3H/2\), the scalar field begins oscillating well before the present day, similarly to the case of scalarfield dark matter discussed in Sect. 4.1, and so does not explain the observed dark energy. Appreciable changes in the scalar field ϕ and consistency with dark energy therefore can only occur when \(m_{\phi}\sim H_{0} \sim 10^{33}~\mathrm{eV}\), where \(H_{0}\) is the present Hubble scale; in this case, the apparent values of the fundamental constants would change slowly and linearly with time during the present epoch.
The most stringent bound on linear drifts in α at redshifts \(z \lesssim 0.5\) comes from optical clock comparison measurements with Yb^{+} and is at the level \(d\ln (\alpha )/dt \lesssim 10^{18}~\mathrm{yr}^{1}\) [20]. This bound is one and two orders of magnitude, respectively, more stringent than bounds pertaining to the Oklo phenomenon [154–157] and meteorite dating [158]; see Table 1 for a summary of the bounds. The bounds from two optical clock measurements separated in time can be improved with longer time intervals between the measurements. In QSNET, there are clocks with differential sensitivities to α that are ≃10 times greater than those used in present slowdrift constraints. Meanwhile, the most stringent limit on \(d_{e}^{(1)}\) via searches for equivalenceprincipleviolating forces comes from the MICROSCOPE mission [137] and is at the level \(d_{e}^{(1)} \lesssim 10^{4}\) [14, 138]. The quantity \(d\ln (\alpha )/dt\) and parameter \(d_{e}^{(1)}\) can be related within specific scalarfield models; e.g., in the model considered in Refs. [146, 147], \(d\ln (\alpha )/dt\) at the present day can vary from \({\sim} 10^{17}~\mathrm{yr}^{1}\) to \({\sim} 10^{23}~\mathrm{yr}^{1}\) when taking into account the current MICROSCOPE bound. We thus see that clocks within the QSNET network have the potential to probe unconstrained regions of parameter space in darkenergytype models involving scalar fields.
It is worth mentioning however that there is already some tension between quintessence and constraints from the Eöt–Wash and MICROSCOPE experiments. Indeed, quantum gravity predicts that linear coupling constants of order one will be generated [159] between a quintessence field and visible matter. Linear couplings of the quintessence field with \(d^{(1)}_{e}\) or \(d^{(1)}_{m_{e}}\) of order one are ruled out by Eöt–Wash and MICROSCOPE for a field of mass 10^{−33} eV. In that sense, QSNET clocks will provide a direct test of quantum gravity and quintessence.
4.3 Solitons
Under certain conditions, spinless bosons may form structured “dark objects”, such as solitons. Solitons can be either topological or nontopological in nature. Topological solitons are made up of one or more fields that acquire stability due to the presence of two or more vacua, which are energetically equivalent but topologically distinguishable (e.g., due to a difference in the sign or overall phase associated with a field at the positions of the vacua). Such objects may be produced during a cosmological phase transition [160]. Topological solitons may arise in a variety of dimensionalities, namely: zerodimensional monopoles [161, 162], onedimensional strings [163, 164] and twodimensional domain walls [165]. Monopoles, being practically pressureless, are a good candidate to explain the observed dark matter, while strings and domain walls may only comprise a subdominant fraction of the dark components [166, 167]. A notable example of a nontopological soliton is the Qball [168, 169], a monopolelike soliton that is a good candidate for dark matter.
Recent interest in utilising spatiallyseparated clocks to study dark sector phenomena has mainly focused on macroscopic scalarfield topological domain walls [22, 24–27, 170]. The simplest model admitting topological domain walls involves a single real scalar field ϕ with the following \(\phi ^{4}\) potential (see, e.g., [22, 27, 165]):
where λ is a dimensionless parameter. The potential in Eq. (22) admits two energetically equivalent, but topologically distinct minima at \(\phi = \pm \phi _{0}\), separated by a potential barrier of height \(\lambda \phi _{0}^{4} / 4\). The \(Z_{2}\) symmetry associated with the potential (22) is spontaneously broken, since the vacuum states are not invariant under the \(\phi \to \phi \) transformation. If there exist two spatially separated regions of space with topologically distinct vacua, then a domain wall forms between the two vacua, with the following transverse “kink” profile (in the rest frame of the wall) [165]:
where the transverse size of the wall is set by \(d = \sqrt{2 / ( \lambda \phi _{0}^{2})} = 1/m_{\phi ,\mathrm{eff}}\) (\(m_{ \phi ,\mathrm{eff}}\) is the effective scalar mass) and may in principle range in size from the microscopic scale up to a sizeable fraction of the observable universe. The regions on either side of the wall are referred to as domains, by analogy with the familiar ferromagnetic domains in condensed matter physics. The energy density inside a wall is given by \(\rho _{\mathrm{inside}} \sim \phi _{0}^{2} / d^{2}\). For a network of walls with an average energy density of \(\rho _{\mathrm{walls}}\) and an average separation between adjacent walls of \(L = v_{\mathrm{wall}} \mathcal{T}\), there is a simple relation between the domainwall parameters:
where \(v_{\mathrm{wall}}\) is the typical speed of passage of domain walls through Earth and \(\mathcal{T}\) is the average time between encounters of a wall with Earth. Domain walls with the potential (22) have large spatial components in the associated energymomentum tensor that give significant deviations from the equation of state for nonrelativistic matter; numerical simulations indicate that such domain walls travel at semirelativistic speeds \(v_{\mathrm{wall}} \sim c\) [166, 171, 172]. Furthermore, the consideration of the gravitational effects of domain walls on photons originating from the cosmic microwave background constrains the presentday energy density stored in a network of domain walls to less than ∼10^{−5} times that of the presentday critical density of the universe [27, 166, 173]; i.e., \({\sim} 10^{10}~\mathrm{GeV/cm}^{3}\) or ∼10^{−10} times the local Galactic darkmatter energy density. Therefore, domain walls cannot account for all of the dark matter.
If the scalar field ϕ interacts nongravitationally with fields from the Standard Model sector, then there may be characteristic observable signatures in terrestrial experiments. Due to the smallness of the maximally allowed value of \(\rho _{\mathrm{walls}}\) and hence \(\phi _{0}\), the scalartype linearinϕ interactions in Eq. (15) are strongly constrained by traditional searches for equivalenceprincipleviolating forces which do not depend on \(\phi _{0}\).^{Footnote 3} Therefore, we focus on the scalartype quadraticinϕ interactions in Eq. (17), which were previously considered in Refs. [22, 24–27, 170]. Comparing the interactions in Eq. (17) with the corresponding terms in the Standard Model Lagrangian, \(\mathcal{L}_{\text{Standard Model}} \supset  F_{\mu \nu} F^{\mu \nu} / 4  e J_{\mu}A^{\mu} m_{e} \bar{\psi} \psi \), we see that the apparent values of α and the electron mass are given by:
where the subscript ‘0’ refers to the local fundamental constant value when \(\phi = 0\). The passage of a domain wall, e.g., with the transverse profile in (23), through a point or region of space is expected to induce transient changes in the apparent values of the fundamental constants (the values of the fundamental constants are the same prior to and after the passage of a domain wall, and differ only in the central region of a wall during the wall’s passage), which can be sought with clock [22, 24, 26] and cavitybased [11, 25, 131, 170] measurements, ideally using a network of spatiallyseparated detectors.
For a sufficiently small detector, the signal duration is given by \(\Delta t \sim d / v_{\mathrm{wall}}\), if a wall passes through the detector (and Earth) in an unperturbed manner. However, it has been pointed out in [27] that the interactions in Eq. (17) cause ordinary matter (e.g., within Earth, Earth’s atmosphere, and the apparatus itself) to create a repulsive potential that may affect the propagation of domain walls near bodies of ordinary matter. The precise outcome for a domain wall incident on a strongly repulsive potential requires further detailed investigation; for the purposes of the present discussion, we make the simple assumption adopted in Refs. [22, 24–26, 170], namely that the passage of a wall proceeds in an unperturbed fashion. When a domain wall of cosmological origin is far away from Earth, the “back action” of ordinary matter inside Earth on the scalar field via Eq. (17) induces quasistatic apparent variations of the fundamental constants with height above Earth’s surface, which can be sought with clock comparison measurements at different heights; see [27] for details.
In Fig. 8, we present the estimated sensitivity of the QSNET network to apparent transient variations of the fundamental constants induced by the passage of domain walls, assuming that data are continuously collected every \({\sim} 1~\mathrm{s}\) over the course of \(1~\mathrm{year}\). We assume that domain walls make up a maximally allowable fraction of the dark components, which is ∼10^{−5} at the present day. We further assume that the average time between encounters of a wall with Earth is given by \(\mathcal{T} = 1~\mathrm{year}\), with adjacent walls wellseparated (\(\Delta t \ll \mathcal{T}\)), that domain walls propagate at semirelativistic speeds \(v_{\mathrm{wall}} \sim c\), and that the backaction effects of Earth and the apparatus on the incident domain walls can be neglected (transient signals may be qualitatively different when backaction effects are strong [27]).
For comparison, we also show limits from previous searches for transient variations of the fundamental constants using the GPS network of clocks [24], and searches for quasistatic apparent variations of the fundamental constants with height above Earth’s surface using clock comparison measurements at different heights and accelerometers as well as comparisons of atomic and molecular spectra in groundbased laboratory and lowdensity astrophysical environments [27]. Note that we have rescaled the limits in [24] and [27] to account for differences in the assumed values of \(\rho _{\mathrm{walls}}\) and \(v_{\mathrm{wall}}\) compared with the present article.
Our analysis shows that the QSNET network has the potential to probe unexplored regions of parameter space in domainwall scalarfield models, specifically in regions of parameter space where the backaction effects of Earth and the apparatus are negligible [27]. We note that QSNET may have more extensive reach in other models of solitons, such as monopoles [161, 162, 168, 169]; these possibilities require further detailed study. Additionally, exploiting the network configuration, QSNET could provide information about the speed and direction of propagation of the domain walls or other dark objects.
4.4 Violation of fundamental symmetries
Fundamental symmetries are central concepts and guiding principles in physics. The study of spacetime symmetries dates back hundreds of years to the insights of Galileo, Newton, and other contemporaries, and forms the foundations of modern particle and gravitational theories. Lorentz invariance is a spacetime symmetry at the heart of the Standard Model and General Relativity. It roughly states that physical laws are independent of the relative orientation and velocity of an experiment in spacetime. As a consequence, the measurement outcomes of two otherwise identical experiments of distinct spacetime orientation must be based on the same laws of physics, with results connected by the Lorentz transformation.
Spacetime symmetries have been studied in a number of newphysics scenarios, including stringbased approaches [174–180], loop quantum gravity [181, 182], noncommutative field theory [183–187], highenergy electrodynamics [188, 189], and modifiedgravity theories [69, 190–196]. A subset of these works suggest Lorentzviolating effects may exist and be detectable in experiments with exceptional sensitivity, including those of QSNET. Indeed, recent years have witnessed a significant expansion in experimental searches for small violations of Lorentz invariance involving nearly every subfield of physics [68]. If such effects do exist, current constraints suggest they are quite small. Given the present absence of any Lorentzviolating signal, a prudent approach is to use modelindependent methods based on effective field theory (EFT) [197]. In the context of Lorentz violation, this framework exists and is known as the StandardModel Extension (SME) [198–200].^{Footnote 4} The SME action includes all known physics in addition to possible Lorentzviolating and invariant terms,
where \(S_{\text{SM}}\) is the Standard Model action, \(S_{\text{EH}}\) is the Einstein–Hilbert action, and \(S_{\text{LV}} \ll S_{\text{SM}}\), \(S_{\text{EH}}\) includes in principle an infinite number of terms in EFT consistent with the choice of fields and preserved symmetries. Note that since CPT violation implies Lorentz violation in EFT, all possible CPTviolating operators in EFT are included in the SME by construction [199]. Also note that violations of other fundamental symmetries, such as the weak equivalence principle, have also been developed within the SME framework [203]. See, e.g., Ref. [204] for a recent account of several applications. An example term modifying conventional quantum electrodynamics (QED) is
The SME coefficient \(c_{\mu \nu}\) is coupled to the fermion ψ and controls the strength of Lorentz violation. In general, the inclusion of a nonzero \(c_{\mu \nu}\) results in rich phenomenological signatures, including modified kinematic effects, quantum corrections, and shifts in atomic spectra [198, 205, 206].
Clockcomparison experiments,^{Footnote 5} including those based on atomic clocks, are ideal systems for precision tests of Lorentz violation [207–210]. Since these experiments involve comparatively low energies, operators of lowest mass dimension \(d = 3, 4\) involving the free propagation of electrons and nucleons are expected to represent the dominant experimental signals. This describes the extension of the free QED Lagrange density
where \(\psi = \{\psi _{e}, \psi _{p}, \psi _{n}\}\) stands for an electron, proton, or neutron field. The generalised kinetic and mass matrices are
where the first two terms on the righthand side of each equation—\(\gamma _{\nu}\) and m—are the conventional fourdimensional gamma matrices and fermion mass, respectively. Note the inclusion of the \(c_{\mu \nu}\) coefficient from Eq. (27). The coefficients \(c_{\mu \nu}\), \(d_{\mu \nu}\), \(e_{\nu}\), \(f_{\nu}\), \(g_{\lambda \mu \nu}\) have mass dimension zero and the coefficients \(a_{\mu}\), \(b_{\mu}\), \(H_{\mu \nu}\) have mass dimension one. By convention, the units for SME coefficients of nonzero mass dimension are chosen to be powers of GeV. Additional technical details are provided in Appendix C.1.
Extractions of Lorentzviolating signals from atomicclock tests have been performed with both nonrelativistic and relativistic methods. The starting point in either case is constructing the relativistic Hamiltonian stemming from Eq. (28). For especially light systems, e.g. H, \(\overline{\text{H}}\), He, Li, the nonrelativistic approach based on the Foldy–Wouthuysen sequence is expected to capture the dominant physics, where the relativisticinorigin SME coefficients are treated as small corrections amenable to standard techniques of perturbation theory [211, 212]. Carrying out this procedure results in the full Lorentzviolating perturbation \(\delta h_{\text{LV}}\) detailed in Appendix C.1 [207]. Of these renormalizable effects, the electronsector ctype coefficients first introduced in Eq. (27) represent a prime example of sensitive perturbations to atomicclock transitions.^{Footnote 6} The relevant perturbing Hamiltonian for a bound electron of momentum p⃗ reads [203, 213, 214]
where \(C_{0}^{(0)}\), \(C_{q}^{(2)}\) are linear combinations of \(c_{\mu \nu}\) matrix elements, \(T_{q}^{(2)}\) are spherical tensor operators, U is the Newtonian gravitational potential and c the speed of light. The shifted spectra are obtained by calculating the matrix elements of \(\delta h_{\text{LV}}\) between the unperturbed atomic states of interest. In most applications the total atomic angular momentum F and its spin projection \(m_{F}\) are conserved and may be used to label the states. The projection quantum number \(m_{F}\) typically defines the laboratory z axis and is identified with the direction of a uniformly applied external magnetic field. In this scenario, the conventional energy levels are shifted by
The shifted laboratory frequencies are simply proportional to the difference between the relevant energy shifts. Note that in general, and especially for systems based on heavy atoms or ions where relativistic corrections can be large, intrinsically relativistic methods, starting from solving the Dirac–Hartree–Fock equations, are used to obtain the electronic wave functions used in Eq. (31) to accurately capture the effects of the ctype coefficients [213, 215–220]. Relativistic analogues of the momentumspace matrix elements, e.g. \(\langle \vec{p}^{2} \rangle \rightarrow \langle c\gamma ^{0}\gamma ^{j} p_{j} \rangle \) have also been calculated, though the differences thus far considered were found to be negligible [215, 219]. Additional studies have recently extended some of these approaches into the nonrenormalizable \(d\geq 5\) sector [209, 210].
A variety of clockcomparison experiments have produced leading constraints on fermionsector SME coefficients. As detailed in Sect. 3 and Appendix A, the established standards of QSNET are based on a Cs fountain clock and Sr and Yb^{+} optical clocks. Systems based on a subset of these types of clocks currently hold leading constraints on minimal Lorentz violation affecting electrons and nucleons. Caesium parityviolation experiments have constrained the timelike component of the electronsector btype coefficient \(b_{0} < 2\times 10^{14}\text{ GeV}\) [221, 222]. In the nucleon sector, similar techniques have placed constraints \(b_{0} \lesssim 10^{8}\text{}10^{7}\text{ GeV}\) [221–223], in addition to the timelike dtype coefficient \(d_{00} \lesssim 10^{8}\text{}10^{7}\) [222, 223]. In the proton sector, fountainbased Cs clocks have stringently constrained linear combinations of all components of the ctype coefficients at levels \(\lesssim 10^{25}\text{}10^{16}\) [224–226]. Optical clocks based on ytterbium have also produced the current best limits \({\lesssim} 10^{21}\text{}10^{16}\) on the electron sector ctype coefficients [227]. Several other competitive constraints have been placed on minimal SME coefficients using a wide variety of clockcomparison experiments [213, 214, 218, 219, 223, 226, 228–252]. In addition, the first constraints in the nonminimal \(5 \leq d \leq 8\) electron and nucleon sectors were recently placed using H masers and the 1S2S transition [253] and H, \(\overline{\text{H}}\) spectroscopy [209].
The Yb^{+} E3 clock has the highest sensitivity to Lorentz violation among all presently operating clocks, with the reduced matrix element of the \(T^{(2)} \) operator \(\langle J\ T^{(2)}\ J\rangle =145\) a.u. (atomic units) for the upper clock state [217]. Cf^{15+} and Cf^{17+} have similar sensitivities, with respective matrix elements of 112 a.u. and 144 a.u. for ions in the ground state [217]. There are two types of measurements that the QSNET network can perform to search for Lorentz invariance violation in the electronphoton sector. First, one can follow an approach of the PTB Yb^{+} Lorentzviolation experiment, comparing frequencies of two colocated Yb^{+} clocks with different magnetic field orientations [90]. One has to investigate if such a scheme can be adapted for two different clocks. Such a method has the advantage of using usual clockcomparison metrological protocols. One can use clockcomparison data obtained for the dark matter searches, for example. However, the limits set by PTB already used a clock comparison at the 10^{−18} level, and higher accuracy will be required for an improvement of \(c_{IJ}\) and \(c_{TJ}\) coefficients (indices T, I, J denote Suncentred frame indices—see Appendix C.2). The \(c_{TT}\) coefficient was not considered in [90] and significant improvement is possible. In addition, one can constrain nonminimal coefficients in such experiments. In the second class of experiments, one uses a dynamic decoupling proposal of [217] to monitor the splitting between different Zeeman substates as Earth rotates around its axis and around the Sun placing a bound on \(C_{0}^{(2)}\). This method would use Zeeman multiplets of either upper Yb^{+} clock states or ground states of Cf highly charged ion clocks. We note that this method does require operating a Cf HCI clock (no need for a clock laser) but only the ability to carry out the dynamic decoupling sequence for the ground state, which does not involve optical transitions. This method can drastically, by orders of magnitude, improve Lorentzviolation tests for all \(c_{\mu \nu}\) coefficients for electrons.
Atomicclock experiments have demonstrated exceptional sensitivity to electron and protonsector Lorentz violation. As described in Appendix C.2, the SME coefficients depend on the choice of observer frame. This implies that every experiment is sensitive to a unique linear combination of SME coefficients and that dedicated studies investigating the performance of QSNET relative to existing experiments must ultimately be performed. As discussed in Sect. 2, since spacetime variations of α have been associated with violations of Lorentz and CPT invariance [65–67], it is conceivable that increased constraints on α variations from QSNET could be translated into new constraints on Lorentz violation. To summarise, given the existing capabilities and projected limits of QSNET described in Sect. 3.4, it is reasonable to suggest new, competitive and potentially leading constraints on violations of fundamental symmetries are within reach.
4.5 Tests of unification and quantum gravity
4.5.1 Tests of unification
A discovery of a time variation of μ or α could be used to probe very high energy theories such as models of grand unification [254, 255]. Grand unified theories are a natural extension of the Standard Model. The idea that all the forces of nature can be unified in one fundamental force is very attractive to theoretical physicists, as such models have the potential to reduce the number of fundamental constants in the model.
To define a grand unified theory, we need to decide which unification group to consider. Well studied examples of gauge groups are, e.g., SU(5), SO(10) or E_{6}, but other groups are possible. The minimal requirement for such a group is that the Standard Model gauge groups SU(3) × SU(2) × U(1) can be embedded in the grand unified theory group. The coupling constants of the gauge groups of the standard model, \(\alpha _{1}\) for U(1), \(\alpha _{2}\) for SU(2), and \(\alpha _{3}\) for SU(3), are assumed to all reach the same value \(\alpha _{u}\) (the unified coupling constant) at some unification scale \(\Lambda _{u}\). At energies larger than \(\Lambda _{u}\), the gauge symmetries of the unification group are manifest, while those of the Standard Model are manifest at energies below \(\Lambda _{u}\). Besides the gauge group, one must decide which Higgs field and fermion representations to introduce in the model and how to couple the Higgs fields to fermions or themselves. This generically introduces Higgs boson masses and Yukawa couplings and thus a number of fundamental constants.
Measurements of variations of μ can be used to probe grand unified theories [53–64]. Ignoring possible cosmological time variations of Yukawa couplings and of Higgs boson masses [256], and working at the one loop level, we only have two parameters: the unification scale \(\Lambda _{u}\) and the unified coupling constant \(\alpha _{u}\). As the proton mass is mainly determined by the QCD scale, quark masses can be neglected. We focus on the QCD scale \(\Lambda _{\mathrm{QCD}}\) and extract its value from the Landau pole of the renormalization group equation for the QCD coupling constant:
where the parameter \(b^{\mathrm{SM}}_{3}=7\) in the Standard Model and \(\mu _{R}\) is the renormalization scale. The QCD scale, i.e., the energy scale below which the SU(3) interactions are strong is defined by
The time variation of \(\Lambda _{\mathrm{QCD}}\) is then determined by
and one can see that a time variation of the QCD scale could be due to either a time variation of the unification scale or of the unified coupling constant. For constant quark and electron masses this equation determines the ratio:
The running of the three coupling constants \(\alpha _{i}\) of the Standard Model are given by
where \(b_{i} =(b^{{\mathrm{SM}}}_{1}, b^{{\mathrm{SM}}}_{2}, b^{{\mathrm{SM}}}_{3})=(41/10, 19/6, 7)\) are the coefficients of the renormalization group equations for the Standard Model. This leads to the following relation for the fine structure constant [53–55]
In the supersymmetric extension of the Standard Model, the coefficients \(b_{i}\) in Eqs. (36) need to be replaced by \(b^{{S}}_{i}=(b^{{S}}_{1}, b^{{S}}_{2}, b^{{S}}_{3})=(33/5, 1, 3)\) which are the coefficients of the renormalization group equations in the \({\mathcal{N}}=1\) supersymmetric case.
SU(5) grand unification models require us to introduce supersymmetry between the weak scale and the unification scale to obtain a numerical unification of the gauge couplings of the Standard Model at the unification scale.
One may consider different scenarios. First, we keep \(\Lambda _{u}\) invariant and consider the case where \(\alpha _{u} =\alpha _{u} (t)\) is time dependent. One then gets [53]
If we calculate \(\dot{\Lambda}_{\mathrm{QCD}}/\Lambda _{\mathrm{QCD}}\) using the relation above in the case of 6 quark flavors, neglecting the masses of the quarks, we find \(R \approx 46\). There are large theoretical uncertainties in R. Taking thresholds into account one gets \(R=37.7\pm 2.3\) [53]. The uncertainty in R is given, according to \(\Lambda _{\mathrm{QCD}} = 213^{+38}_{35} {\mathrm{MeV}}\), by the uncertainty in the ratio \(\alpha /\alpha _{s}\), which is dominated by the uncertainty in \(\alpha _{s}\).
We could alternatively consider the case where \(\alpha _{u}\) is invariant but \(\Lambda _{u}=\Lambda _{u} (t)\) is timedependent. One gets [54]
It is interesting to note that the effects of a time variation of the unified coupling constant or of a time variation of the grand unified scale are going in opposite directions. Clearly those are two extreme cases and a time variation of both parameters is conceivable. This could lead to cancellations between the different effects.
It should be clear that our results are strongly modeldependent. For example, in SO(10) without supersymmetry, where a unification of the gauge couplings is possible due to threshold corrections, varying the grand unification scale, one finds [257]:
We thus see that simultaneous measurements of \(\dot{\mu}/\mu \) and \(\dot{\alpha}/\alpha \) would enable us to discriminate between grand unified theories with very low energy experiments.
The model dependence in grand unification theories is what makes the detection of a possible time variation of the fundamental parameters so interesting. Indeed, QSNET could test grand unified theories without actually detecting any particle from a grand unified model. This is because QSNET will be sensitive to both variation of α and μ, and if a variation is detected for either or both constants, it will be possible to discriminate between grand unified models.
4.5.2 Test of quantum gravity
Quantum gravity will generate interactions between the Standard Model particles and any new particles of a hidden sector, e.g. dark matter particles [44–46, 258–260]. It is easy to convince oneself that only nonperturbative quantum gravitational effects have the potential to be large enough to be relevant for clocks as perturbative effects are generically very much smaller than nonperturbative ones [44, 45].
For a scalar field, quantum gravity will generate interactions of the type
where \(\kappa =\sqrt{4 \pi G_{N}}\) whether gauge interactions between the Standard Model and the hidden sector exist or not. The cases \(n=1\) and \(n=2\) correspond respectively to the linear and quadratic couplings discussed earlier. One expects \(d^{(n)}_{i}\sim 1\) on very generic grounds [44, 45] as these operators are normalised to the reduced Planck scale \(M_{P}=1/\sqrt{8 \pi G_{N}}=2.4\times 10^{18}\text{ GeV}\) which is the scale of quantum gravity. As these operators are generated via nonperturbative effects such as gravitational instantons, wormholes, or quantum black holes [261–263], there is no further suppression to be expected such as factors of \((16 \pi ^{2})^{k}\) due to kloop factors. If the scale suppressing the operators is properly normalised, the Wilson coefficients \(d^{(n)}_{i}\) must be of order one.
This reasoning leads quite generically to a bound on the mass of singlet scalar fields [44, 45]. Using data from the Eöt–Wash experiment, we find \(m<10^{2}\text{ eV}\) for a coupling \(d^{(1)}\sim 1\). It follows that QSNET has the potential to probe quantum gravity: if a very light singlet scalar field was detected with \(d^{(1)}\ll 1\), QSNET would have demonstrated that the linear operators discussed above are not generated by quantum gravity.
5 Summary and conclusions
Despite the fact that our understanding of physics strongly hinges on them, we know very little about the origin and the behaviour of fundamental constants. In particular, we do not know if they are true constants or rather feebly vary through space and time. The measurement of even the slightest variation would provide us with a clear research direction beyond the theories we have so far, which famously fail to explain the vast majority of the energy content of the universe. Indeed, we have shown that variations of fundamental constants could be linked to dark matter, dark energy, violations of fundamental symmetries of nature or could be evidence that the laws of physics undergo cosmological evolution. We have argued that a network of clocks provides us with a powerful opportunity to measure with unprecedented sensitivity and a high level of confidence variations of two fundamental constants: the fine structure constant, α, and the electrontoproton mass ratio, μ.
In this work we have introduced the QSNET project, which aims at realising such a network. We have described its first stage, that will include a range of atomic and molecular clocks in the UK with different sensitivities to variations of α and μ. We have evaluated the performance that can be obtained by QSNET. As illustrated with a few examples, such performance will enable us to explore large uncharted territories of the dark sector, potentially discovering new physics and/or imposing new constraints over many models and theories, widening our understanding of the physics that governs the universe. More specifically, QSNET will be sensitive to

Drifts of α and μ, with relevance for dark energy models and models that predict cosmological evolution of fundamental constants.

Oscillations of α and μ, that can be linked for example to virialised dark matter scalar fields.

Transient events due to kinks or topological defects in darksector fields.
Additionally, QSNET will allow us to perform tests of quantum gravity, violations of fundamental symmetries and grand unification theories.
In its next stages, the QSNET network will be extended, ideally across the globe and with some nodes in space, including more clocks and allowing for novel and improved capabilities of detection of variations of fundamental constants. Also, as happened in the last five decades, the ongoing progress of clock technology will allow us to improve stability and accuracy at each node of the network, further pushing our abilities to explore the unknown 95% of the universe.
Availability of data and materials
Not applicable.
Notes
From a detailed analysis of the molecular structure we found that the exact value is 0.49 [98].
For Cs \(T_{p}\) has been chosen to match the current stateoftheart experiments, for CaF \(T_{p}\) is limited by the natural linewidth of the transition.
Note that the situation in the case of an oscillating darkmatter scalar field of the type discussed in Sect. 4.1 is different, since \(\phi _{0}\) can be many orders of magnitude larger in that case.
The phrase ‘clockcomparison experiment’ originated in Ref. [207] and describes a broad class of experiments with atoms and ions. Experiments based on atomic clocks are a particular type of clockcomparison experiment.
Note that this class of fermion coefficients cannot be separated from the minimal CPTeven photon coefficients, as explained in Appendix C.1.
References
Zyla PA et al.. Review of particle physics. Prog Theor Exp Phys. 2020;2020(8):083C01. https://doi.org/10.1093/ptep/ptaa104.
Khoury J, Weltman A. Chameleon cosmology. Phys Rev D. 2004;69:044026. https://doi.org/10.1103/PhysRevD.69.044026.
Avelino PP, Martins CJAP, Nunes NJ, Olive KA. Reconstructing the dark energy equation of state with varying couplings. Phys Rev D. 2006;74:083508. https://doi.org/10.1103/PhysRevD.74.083508.
Dvali G, Zaldarriaga M. Changing α with time: implications for fifthforcetype experiments and quintessence. Phys Rev Lett. 2002;88:091303. https://doi.org/10.1103/PhysRevLett.88.091303.
Banks T, Dine M, Douglas M. Timevarying α and particle physics. Phys Rev Lett. 2002;88:131301. https://doi.org/10.1103/PhysRevLett.88.131301.
Taylor TR, Veneziano G. Dilaton couplings at large distances. Phys Lett B. 1988;213(4):450–4. https://doi.org/10.1016/03702693(88)912907.
Gambini R, Pullin J. Discrete quantum gravity: a mechanism for selecting the value of fundamental constants. Int J Mod Phys D. 2003;12(09):1775–81. https://doi.org/10.1142/S0218271803004018.
Taveras V, Yunes N. Barbero–Immirzi parameter as a scalar field: Kinflation from loop quantum gravity? Phys Rev D. 2008;78:064070. https://doi.org/10.1103/PhysRevD.78.064070.
Uzan JP. The stability of fundamental constants. C R Phys. 2015;16(5):576–85. https://doi.org/10.1016/j.crhy.2015.03.007. The measurement of time / La mesure du temps.
Arvanitaki A, Huang J, Van Tilburg K. Searching for dilaton dark matter with atomic clocks. Phys Rev D. 2015;91:015015. https://doi.org/10.1103/PhysRevD.91.015015.
Stadnik YV, Flambaum VV. Searching for dark matter and variation of fundamental constants with laser and maser interferometry. Phys Rev Lett. 2015;114:161301. https://doi.org/10.1103/PhysRevLett.114.161301.
Stadnik YV, Flambaum VV. Can dark matter induce cosmological evolution of the fundamental constants of nature? Phys Rev Lett. 2015;115:201301. https://doi.org/10.1103/PhysRevLett.115.201301.
Arvanitaki A, Dimopoulos S, Van Tilburg K. Sound of dark matter: searching for light scalars with resonantmass detectors. Phys Rev Lett. 2016;116:031102. https://doi.org/10.1103/PhysRevLett.116.031102.
Hees A, Minazzoli O, Savalle E, Stadnik YV, Wolf P. Violation of the equivalence principle from light scalar dark matter. Phys Rev D. 2018;98:064051. https://doi.org/10.1103/PhysRevD.98.064051.
Safronova MS, Budker D, DeMille D, Kimball DFJ, Derevianko A, Clark CW. Search for new physics with atoms and molecules. Rev Mod Phys. 2018;90:025008. https://doi.org/10.1103/RevModPhys.90.025008.
Brewer SM, Chen JS, Hankin AM, Clements ER, Chou CW, Wineland DJ, Hume DB, Leibrandt DR. \({}^{27}{\mathrm{Al}}^{+}\) quantumlogic clock with a systematic uncertainty below 10^{−18}. Phys Rev Lett. 2019;123:033201. https://doi.org/10.1103/PhysRevLett.123.033201.
Oelker E, Hutson RB, Kennedy CJ, Sonderhouse L, Bothwell T, Goban A, Kedar D, Sanner C, Robinson JM, Marti GE, Matei DG, Legero T, Giunta M, Holzwarth R, Riehle F, Sterr U, Ye J. Demonstration of \(4.8 \times 10^{17}\) stability at 1 s for two independent optical clocks. Nat Photonics. 2019;13(10):714–9. https://doi.org/10.1038/s4156601904934.
Godun RM, NisbetJones PBR, Jones JM, King SA, Johnson LAM, Margolis HS, Szymaniec K, Lea SN, Bongs K, Gill P. Frequency ratio of two optical clock transitions in ^{171}Yb^{+} and constraints on the time variation of fundamental constants. Phys Rev Lett. 2014;113:210801. https://doi.org/10.1103/PhysRevLett.113.210801.
Huntemann N, Lipphardt B, Tamm C, Gerginov V, Weyers S, Peik E. Improved limit on a temporal variation of \({m}_{p}/{m}_{e}\) from comparisons of Yb^{+} and Cs atomic clocks. Phys Rev Lett. 2014;113:210802. https://doi.org/10.1103/PhysRevLett.113.210802.
Lange R, Huntemann N, Rahm JM, Sanner C, Shao H, Lipphardt B, Tamm C, Weyers S, Peik E. Improved limits for violations of local position invariance from atomic clock comparisons. Phys Rev Lett. 2021;126:011102. https://doi.org/10.1103/PhysRevLett.126.011102.
BACON collaboration. Frequency ratio measurements at 18digit accuracy using an optical clock network. Nature. 2021;591(7851):564–9.
Derevianko A, Pospelov M. Hunting for topological dark matter with atomic clocks. Nat Phys. 2014;10(12):933–6.
Derevianko A. Detecting darkmatter waves with a network of precisionmeasurement tools. Phys Rev A. 2018;97:042506. https://doi.org/10.1103/PhysRevA.97.042506.
Roberts BM, Blewitt G, Dailey C et al.. Search for domain wall dark matter with atomic clocks on board global positioning system satellites. Nat Commun. 2017;8:1195. https://doi.org/10.1038/s41467017014404.
Wcisło P, Ablewski P, Beloy K, Bilicki S, Bober M, Brown R, Fasano R, Ciuryło R, Hachisu H, Ido T, Lodewyck J, Ludlow A, McGrew W, Morzyński P, Nicolodi D, Schioppo M, Sekido M, Le Targat R, Wolf P, Zhang X, Zjawin B, Zawada M. New bounds on dark matter coupling from a global network of optical atomic clocks. Sci Adv. 2018;4(12):eaau4869. https://doi.org/10.1126/sciadv.aau4869.
Roberts BM, Delva P, AlMasoudi A, AmyKlein A, Bærentsen C, Baynham CFA, Benkler E, Bilicki S, Bize S, Bowden W, Calvert J, Cambier V, Cantin E, Curtis EA, Dörscher S, Favier M, Frank F, Gill P, Godun RM, Grosche G, Guo C, Hees A, Hill IR, Hobson R, Huntemann N, Kronjäger J, Koke S, Kuhl A, Lange R, Legero T, Lipphardt B, Lisdat C, Lodewyck J, Lopez O, Margolis HS, ÁlvarezMartínez H, Meynadier F, Ozimek F, Peik E, Pottie PE, Quintin N, Sanner C, Sarlo LD, Schioppo M, Schwarz R, Silva A, Sterr U, Tamm C, Targat RL, Tuckey P, Vallet G, Waterholter T, Xu D, Wolf P. Search for transient variations of the fine structure constant and dark matter using fiberlinked optical atomic clocks. New J Phys. 2020;22(9):093010. https://doi.org/10.1088/13672630/abaace.
Stadnik YV. New bounds on macroscopic scalarfield topological defects from nontransient signatures due to environmental dependence and spatial variations of the fundamental constants. Phys Rev D. 2020;102:115016. https://doi.org/10.1103/PhysRevD.102.115016.
Barontini G, Boyer V, Calmet X, Fitch NJ, Forgan EM, Godun RM, Goldwin J, Guarrera V, Hill IR, Jeong M, Keller M, Kuipers F, Margolis HS, Newman P, Prokhorov L, Rodewald J, Sauer BE, Schioppo M, Sherrill N, Tarbutt MR, Vecchio A, Worm S. QSNET, a network of clock for measuring the stability of fundamental constants. In: SPIE quantum technology: driving commercialisation of an enabling science II. vol. 11881. 2021. p. 63–6. https://doi.org/10.1117/12.2600493.
Flambaum VV, Dzuba VA. Search for variation of the fundamental constants in atomic, molecular, and nuclear spectra. Can J Phys. 2009;87(1):25–33. https://doi.org/10.1139/p08072.0805.0462v2.
Porsev SG, Safronova UI, Safronova MS, Schmidt PO, Bondarev AI, Kozlov MG, Tupitsyn II, Cheung C. Optical clocks based on the Cf^{15+} and Cf^{17+} ions. Phys Rev A. 2020;102:012802. https://doi.org/10.1103/PhysRevA.102.012802.
Dirac PAM. The cosmological constants. Nature. 1937;139:323. https://doi.org/10.1038/139323a0.
Dirac PAM. New basis for cosmology. Proc R Soc Lond A. 1938;165:199–208. https://doi.org/10.1098/rspa.1938.0053.
Milne EA. Kinematics, dynamics, and the scale of time. Proc R Soc A. 1937;158:324–48. https://www.jstor.org/stable/96821.
Jordan P. G has to be a field. Naturwissenschaften. 1937;25:513–7. https://doi.org/10.1007/BF01498368.
Jordan P. Über die kosmologische Konstanz der Feinstrukturkonstanten. Z Phys. 1939;113:660–2. https://doi.org/10.1007/BF01340095.
Uzan JP. Varying constants, gravitation and cosmology. Living Rev Relativ. 2011;14:2. https://doi.org/10.12942/lrr20112. arXiv:1009.5514.
Webb JK, Murphy MT, Flambaum VV, Dzuba VA, Barrow JD, Churchill CW, Prochaska JX, Wolfe AM. Further evidence for cosmological evolution of the fine structure constant. Phys Rev Lett. 2001;87:091301. https://doi.org/10.1103/PhysRevLett.87.091301. arXiv:astroph/0012539.
Chand H, Srianand R, Petitjean P, Aracil B. Probing the cosmological variation of the fine—structure constant: results based on VLT—UVES sample. Astron Astrophys. 2004;417:853. https://doi.org/10.1051/00046361:20035701. arXiv:astroph/0401094.
’t Hooft G. A class of elementary particle models without any adjustable real parameters. Found Phys. 2011;41:1829–56. https://doi.org/10.1007/s1070101195868. arXiv:1104.4543.
Connes A. Noncommutative geometry. 1994.
Polchinski J. String theory. Vol. 1: an introduction to the bosonic string. Cambridge monographs on mathematical physics. Cambridge: Cambridge University Press; 2007. https://doi.org/10.1017/CBO9780511816079.
Polchinski J. String theory. Vol. 2: superstring theory and beyond. Cambridge monographs on mathematical physics. Cambridge: Cambridge University Press; 2007. https://doi.org/10.1017/CBO9780511618123.
Marciano WJ. Time variation of the fundamental ‘constants’ and Kaluza–Klein theories. Phys Rev Lett. 1984;52:489. https://doi.org/10.1103/PhysRevLett.52.489.
Calmet X. Hidden sector and gravity. Phys Lett B. 2020;801:135152. https://doi.org/10.1016/j.physletb.2019.135152. arXiv:1912.04147.
Calmet X. On searches for gravitational dark matter with quantum sensors. Eur Phys J Plus. 2019;134(10):503. https://doi.org/10.1140/epjp/i2019128855. arXiv:1907.05680.
Calmet X, Kuipers F. Bounds on very weakly interacting ultra light scalar and pseudoscalar dark matter from quantum gravity. Eur Phys J C. 2020;80(8):781. https://doi.org/10.1140/epjc/s1005202083507. arXiv:2008.06243.
Calmet X, Kuipers F. Theoretical bounds on dark matter masses. Phys Lett B. 2021;814:136068. https://doi.org/10.1016/j.physletb.2021.136068. arXiv:2009.11575.
Calmet X, Kuipers F. Implications of Quantum Gravity for Dark Matter. Int J Mod Phys D. 2021;30(14):2142004.
Kapner DJ, Cook TS, Adelberger EG, Gundlach JH, Heckel BR, Hoyle CD, Swanson HE. Tests of the gravitational inversesquare law below the darkenergy length scale. Phys Rev Lett. 2007;98:021101. https://doi.org/10.1103/PhysRevLett.98.021101. arXiv:hepph/0611184.
Hoyle CD, Kapner DJ, Heckel BR, Adelberger EG, Gundlach JH, Schmidt U, Swanson HE. Submillimeter tests of the gravitational inversesquare law. Phys Rev D. 2004;70:042004. https://doi.org/10.1103/PhysRevD.70.042004. arXiv:hepph/0405262.
Adelberger EG, Heckel BR, Hoedl SA, Hoyle CD, Kapner DJ, Upadhye A. Particle physics implications of a recent test of the gravitational inverse square law. Phys Rev Lett. 2007;98:131104. https://doi.org/10.1103/PhysRevLett.98.131104. arXiv:hepph/0611223.
Lee JG, Adelberger EG, Cook TS, Fleischer SM, Heckel BR. New test of the gravitational \(1/r^{2}\) law at separations down to 52 μm. Phys Rev Lett. 2020;124(10):101101. https://doi.org/10.1103/PhysRevLett.124.101101. arXiv:2002.11761.
Calmet X, Fritzsch H. The cosmological evolution of the nucleon mass and the electroweak coupling constants. Eur Phys J C. 2002;24:639–42. https://doi.org/10.1007/s1005200209760. arXiv:hepph/0112110.
Calmet X, Fritzsch H. Symmetry breaking and time variation of gauge couplings. Phys Lett B. 2002;540:173–8. https://doi.org/10.1016/S03702693(02)021470. arXiv:hepph/0204258.
Calmet X, Fritzsch H. Grand unification and time variation of the gauge couplings. In: 10th international conference on supersymmetry and unification of fundamental interactions (SUSY02). 2002. p. 1301–6. arXiv:hepph/0211421.
Langacker P, Segre G, Strassler MJ. Implications of gauge unification for time variation of the fine structure constant. Phys Lett B. 2002;528:121–8. https://doi.org/10.1016/S03702693(02)011899. arXiv:hepph/0112233.
Campbell BA, Olive KA. Nucleosynthesis and the time dependence of fundamental couplings. Phys Lett B. 1995;345:429–34. https://doi.org/10.1016/03702693(94)01652S. arXiv:hepph/9411272.
Olive KA, Pospelov M, Qian YZ, Coc A, Casse M, VangioniFlam E. Constraints on the variations of the fundamental couplings. Phys Rev D. 2002;66:045022. https://doi.org/10.1103/PhysRevD.66.045022. arXiv:hepph/0205269.
Dent T, Fairbairn M. Time varying coupling strengths, nuclear forces and unification. Nucl Phys B. 2003;653:256–78. https://doi.org/10.1016/S05503213(03)000439. arXiv:hepph/0112279.
Dent T. Varying alpha, thresholds and extra dimensions. Nucl Phys B. 2004;677:471–84. https://doi.org/10.1016/j.nuclphysb.2003.10.047. arXiv:hepph/0305026.
Landau SJ, Vucetich H. Testing theories that predict time variation of fundamental constants. Astrophys J. 2002;570:463–9. https://doi.org/10.1086/339775. arXiv:astroph/0005316.
Wetterich C. Crossover quintessence and cosmological history of fundamental ‘constants’. Phys Lett B. 2003;561:10–6. https://doi.org/10.1016/S03702693(03)003836. arXiv:hepph/0301261.
Flambaum VV, Tedesco AF. Dependence of nuclear magnetic moments on quark masses and limits on temporal variation of fundamental constants from atomic clock experiments. Phys Rev C. 2006;73:055501. https://doi.org/10.1103/PhysRevC.73.055501. arXiv:nuclth/0601050.
Calmet X, Keller M. Cosmological evolution of fundamental constants: from theory to experiment. Mod Phys Lett A. 2015;30(22):1540028. https://doi.org/10.1142/S0217732315400283. arXiv:1410.2765.
Kostelecky VA, Lehnert R, Perry MJ. Spacetime—varying couplings and Lorentz violation. Phys Rev D. 2003;68:123511. https://doi.org/10.1103/PhysRevD.68.123511. arXiv:astroph/0212003.
Bertolami O, Lehnert R, Potting R, Ribeiro A. Cosmological acceleration, varying couplings, and Lorentz breaking. Phys Rev D. 2004;69:083513. https://doi.org/10.1103/PhysRevD.69.083513. arXiv:astroph/0310344.
Ferrero A, Altschul B. Radiatively induced Lorentz and gauge symmetry violation in electrodynamics with varying alpha. Phys Rev D. 2009;80:125010. https://doi.org/10.1103/PhysRevD.80.125010. arXiv:0910.5202.
Kostelecký VA, Russell N. Data tables for Lorentz and CPT violation. 2021 edition. arXiv:0801.0287v14.
Kostelecky A, Potting R. Lorentz symmetry in ghostfree massive gravity. 2021. arXiv:2108.04213.
Flambaum VV, Dzuba VA. Search for variation of the fundamental constants in atomic, molecular, and nuclear spectra. Can J Phys. 2009;87(1):25–33. https://doi.org/10.1139/p08072.
Dzuba VA, Flambaum VV. Highly charged ions for atomic clocks and search for variation of the fine structure constant. In: Wada M, Schury P, Ichikawa Y, editors. TCP 2014. Cham: Springer; 2017. p. 79–86. https://doi.org/10.1007/978331961588210.
Dzuba VA, Flambaum VV, Webb JK. Spacetime variation of physical constants and relativistic corrections in atoms. Phys Rev Lett. 1999;82:888–91. https://doi.org/10.1103/PhysRevLett.82.888.
Dzuba VA, Flambaum VV, Webb JK. Calculations of the relativistic effects in manyelectron atoms and spacetime variation of fundamental constants. Phys Rev A. 1999;59:230–7. https://doi.org/10.1103/PhysRevA.59.230.
Holliman CA, Fan M, Contractor A, Brewer SM, Jayich AM. Radium ion optical clock. Phys Rev Lett. 2022;128(3):033202. https://doi.org/10.1103/PhysRevLett.128.033202.
Schioppo M et al.. Comparing ultrastable lasers at \(7\times 10^{17}\) fractional frequency instability through a 2220 km optical fibre network. Nat Commun. 2022;13:212. https://doi.org/10.1038/s41467021278843.
Pustelny S, Jackson Kimball DF, Pankow C, Ledbetter MP, Wlodarczyk P, Wcislo P, Pospelov M, Smith JR, Read J, Gawlik W, Budker D. The global network of optical magnetometers for exotic physics (GNOME): a novel scheme to search for physics beyond the standard model. Ann Phys. 2013;525(8–9):659–70. https://doi.org/10.1002/andp.201300061.
Calmet X, Fritzsch H. The cosmological evolution of the nucleon mass and the electroweak coupling constants. Eur Phys J C, Part Fields. 2002;24:639–42. https://doi.org/10.1007/s1005200209760.
Calmet X, Fritzsch H. Symmetry breaking and time variation of gauge couplings. Phys Lett B. 2002;540(3):173–8. https://doi.org/10.1016/S03702693(02)021470.
Calmet X, Fritzsch H. A time variation of proton–electron mass ratio and grand unification. Europhys Lett. 2006;76(6):1064–7. https://doi.org/10.1209/epl/i2006103930.
Kómár P, Kessler EM, Bishof M, Jiang L, Sørensen AS, Ye J, Lukin MD. A quantum network of clocks. Nat Phys. 2014;10(8):582–7. https://doi.org/10.1038/nphys3000.
Baumgratz T, Datta A. Quantum enhanced estimation of a multidimensional field. Phys Rev Lett. 2016;116:030801. https://doi.org/10.1103/PhysRevLett.116.030801.
Kok P, Dunningham J, Ralph JF. Role of entanglement in calibrating optical quantum gyroscopes. Phys Rev A. 2017;95:012326. https://doi.org/10.1103/PhysRevA.95.012326.
Proctor TJ, Knott PA, Dunningham JA. Multiparameter estimation in networked quantum sensors. Phys Rev Lett. 2018;120:080501. https://doi.org/10.1103/PhysRevLett.120.080501.
Weyers S, Gerginov V, Kazda M, Rahm J, Lipphardt B, Dobrev G, Gibble K. Advances in the accuracy, stability, and reliability of the PTB primary fountain clocks. Metrologia. 2018;55(6):789–805. https://doi.org/10.1088/16817575/aae008.
Heavner TP, Donley EA, Levi F, Costanzo G, Parker TE, Shirley JH, Ashby N, Barlow S, Jefferts SR. First accuracy evaluation of NISTF2. Metrologia. 2014;51(3):174–82. https://doi.org/10.1088/00261394/51/3/174.
Guéna J, Abgrall M, Rovera D, Laurent P, Chupin B, Lours M, Santarelli G, Rosenbusch P, Tobar M, Ruoxin L, Gibble K, Clairon A, Bize S. Progress in atomic fountains at LNESYRTE. IEEE Trans Ultrason Ferroelectr Freq Control. 2012;59:391–410. https://doi.org/10.1109/TUFFC.2012.2208.
Szymaniec K, Lea SN, Gibble K, Park SE, Liu K, Głowacki P. NPL Cs fountain frequency standards and the quest for the ultimate accuracy. J Phys Conf Ser. 2016;723:012003. https://doi.org/10.1088/17426596/723/1/012003.
Levi F, Calonico D, Calosso CE, Godone A, Micalizio S, Costanzo GA. Accuracy evaluation of ITCsF2: a nitrogen cooled caesium fountain. Metrologia. 2014;51(3):270–84. https://doi.org/10.1088/00261394/51/3/270.
Bothwell T, Kedar D, Oelker E, Robinson JM, Bromley SL, Tew WL, Ye J, Kennedy CJ. JILA SrI optical lattice clock with uncertainty of \(2.0\times 10^{18}\). Metrologia. 2019;56(6):065004. https://doi.org/10.1088/16817575/ab4089.
Sanner C, Huntemann N, Lange R, Tamm C, Peik E, Safronova MS, Porsev SG. Optical clock comparison for Lorentz symmetry testing. Nature. 2019;567(7747):204–8.
Kajita M. Precise measurement of transition frequencies of optically trapped \({}^{40}\text{Ca}^{19}\text{F}\) molecules. J Phys Soc Jpn. 2018;87:104301. https://doi.org/10.7566/JPSJ.87.104301.
Truppe S, Williams HJ, Fitch NJ, Hambach M, Wall TE, Hinds EA, Sauer BE, Tarbutt MR. An intense, cold, velocitycontrolled molecular beam by frequencychirped laser slowing. New J Phys. 2017;19:022001. https://doi.org/10.1088/13672630/aa5ca2.
Truppe S, Williams HJ, Hambach M, Caldwell L, Fitch NJ, Hinds EA, Sauer BE, Tarbutt MR. Molecules cooled below the Doppler limit. Nat Phys. 2017;13:1173–6. https://doi.org/10.1038/nphys4241.
Williams HJ, Truppe S, Hambach M, Caldwell L, Fitch NJ, Hinds EA, Sauer BE, Tarbutt MR. Characteristics of a magnetooptical trap of molecules. New J Phys. 2017;19:113035. https://doi.org/10.1088/13672630/aa8e52.
Williams HJ, Caldwell L, Fitch NJ, Truppe S, Rodewald J, Hinds EA, Sauer BE, Tarbutt MR. Magnetic trapping and coherent control of lasercooled molecules. Phys Rev Lett. 2018;120:163201. https://doi.org/10.1103/PhysRevLett.120.163201.
Caldwell L, Devlin JA, Williams HJ, Fitch NJ, Hinds EA, Sauer BE, Tarbutt MR. Deep laser cooling and efficient magnetic compression of molecules. Phys Rev Lett. 2019;123:033202. https://doi.org/10.1103/PhysRevLett.123.033202.
Anderegg L, Augenbraun BL, Bao Y, Burchesky S, Cheuk LW, Ketterle W, Doyle JM. Laser cooling of optically trapped molecules. Nat Phys. 2018;14:890–3. https://doi.org/10.1038/s415670180191z.
Kajita M, Gopakumar G, Abe M, Hada M, Keller M. Test of \({m}_{p}/{m}_{e}\) changes using vibrational transitions in \({\text{N}_{2}}^{+}\). Phys Rev A. 2014;89:032509. https://doi.org/10.1103/PhysRevA.89.032509.
Germann M, Tong X, Willitsch S. Observation of electricdipoleforbidden infrared transitions in cold molecular ions. Nat Phys. 2014;10(11):820–4. https://doi.org/10.1038/NPHYS3085.
Peik E, Tamm C. Nuclear laser spectroscopy of the 3.5 eV transition in Th229. Europhys Lett. 2003;61(2):181–6. https://doi.org/10.1209/epl/i200300210x.
Flambaum VV. Enhanced effect of temporal variation of the fine structure constant and the strong interaction in ^{229}Th. Phys Rev Lett. 2006;97:092502. https://doi.org/10.1103/PhysRevLett.97.092502.
Berengut JC, Dzuba VA, Flambaum VV. Enhanced laboratory sensitivity to variation of the finestructure constant using highly charged ions. Phys Rev Lett. 2010;105:120801. https://doi.org/10.1103/PhysRevLett.105.120801.
Derevianko A, Dzuba VA, Flambaum VV. Highly charged ions as a basis of optical atomic clockwork of exceptional accuracy. Phys Rev Lett. 2012;109:180801. https://doi.org/10.1103/PhysRevLett.109.180801.
Kozlov MG, Safronova MS, Crespo LópezUrrutia JR, Schmidt PO. Highly charged ions: optical clocks and applications in fundamental physics. Rev Mod Phys. 2018;90:045005. https://doi.org/10.1103/RevModPhys.90.045005.
Schmöger L, Versolato OO, Schwarz M, Kohnen M, Windberger A, Piest B, Feuchtenbeiner S, PedregosaGutierrez J, Leopold T, Micke P, Hansen AK, Baumann TM, Drewsen M, Ullrich J, Schmidt PO, LópezUrrutia JRC. Coulomb crystallization of highly charged ions. Science. 2015;347(6227):1233–6. https://doi.org/10.1126/science.aaa2960.
Schmoeger L, Schwarz M, Baumann TM, Versolato OO, Piest B, Pfeifer T, Ullrich J, Schmidt PO, Crespo LopezUrrutia JR. Deceleration, precooling, and multipass stopping of highly charged ions in Be^{+} Coulomb crystals. Rev Sci Instrum. 2015;86(10):103111. https://doi.org/10.1063/1.4934245.
Micke P, Leopold T, King SA, Benkler E, Spiess LJ, Schmoeger L, Schwarz M, LopezUrrutia JRC, Schmidt PO. Coherent laser spectroscopy of highly charged ions using quantum logic. Nature. 2020;578:60. https://doi.org/10.1038/s4158602019598.
Ludlow AD, Boyd MM, Ye J, Peik E, Schmidt PO. Optical atomic clocks. Rev Mod Phys. 2015;87:637–701. https://doi.org/10.1103/RevModPhys.87.637.
Voigt C, Denker H, Timmen L. Timevariable gravity potential components for optical clock comparisons and the definition of international time scales. Metrologia. 2016;53(6):1365–83. https://doi.org/10.1088/00261394/53/6/1365.
Baudis L. Dark matter searches. Ann Phys. 2016;528(1–2):74–83. https://doi.org/10.1002/andp.201500114.
Jaeckel J, Ringwald A. The lowenergy frontier of particle physics. Annu Rev Nucl Part Sci. 2010;60(1):405–37. https://doi.org/10.1146/annurev.nucl.012809.104433.
Irastorza IG, Redondo J. New experimental approaches in the search for axionlike particles. Prog Part Nucl Phys. 2018;102:89–159. https://doi.org/10.1016/j.ppnp.2018.05.003.
Agrawal P, Bauer M, Beacham J, Berlin A, Boyarsky A, Cebrian S, CidVidal X, d’Enterria D, De Roeck A, Drewes M et al.. FeeblyInteracting Particles: FIPs 2020 Workshop Report. Eur Phys J C. 2021;81:1015.
Peccei RD, Quinn HR. CP conservation in the presence of instantons. Phys Rev Lett. 1977;38:1440–3. https://doi.org/10.1103/PhysRevLett.38.1440.
Peccei RD, Quinn HR. Constraints imposed by CP conservation in the presence of instantons. Phys Rev D. 1977;16:1791–7. https://doi.org/10.1103/PhysRevD.16.1791.
Weinberg S. A new light boson? Phys Rev Lett. 1978;40:223–6. https://doi.org/10.1103/PhysRevLett.40.223.
Wilczek F. Problem of strong P and T invariance in the presence of instantons. Phys Rev Lett. 1978;40:279–82. https://doi.org/10.1103/PhysRevLett.40.279.
Kim JE. Weak interaction singlet and strong CP invariance. Phys Rev Lett. 1979;43:103. https://doi.org/10.1103/PhysRevLett.43.103.
Shifman MA, Vainshtein AI, Zakharov VI. Can confinement ensure natural CP invariance of strong interactions? Nucl Phys B. 1980;166:493–506. https://doi.org/10.1016/05503213(80)902096.
Zhitnitsky AR. On possible suppression of the axion hadron interactions (in Russian). Sov J Nucl Phys. 1980;31:260.
Dine M, Fischler W, Srednicki M. A simple solution to the strong CP problem with a harmless axion. Phys Lett B. 1981;104:199–202. https://doi.org/10.1016/03702693(81)905906.
Preskill J, Wise MB, Wilczek F. Cosmology of the invisible axion. Phys Lett B. 1983;120:127–32. https://doi.org/10.1016/03702693(83)906378.
Abbott LF, Sikivie P. A cosmological bound on the invisible axion. Phys Lett B. 1983;120:133–6. https://doi.org/10.1016/03702693(83)90638X.
Dine M, Fischler W. The not so harmless axion. Phys Lett B. 1983;120:137–41. https://doi.org/10.1016/03702693(83)906391.
Foster JW, Rodd NL, Safdi BR. Revealing the dark matter halo with axion direct detection. Phys Rev D. 2018;97:123006. https://doi.org/10.1103/PhysRevD.97.123006.
Khmelnitsky A, Rubakov V. Pulsar timing signal from ultralight scalar dark matter. J Cosmol Astropart Phys. 2014;2014(02):019. https://doi.org/10.1088/14757516/2014/02/019.
Porayko NK, Zhu X, Levin Y, Hui L, Hobbs G, Grudskaya A, Postnov K, Bailes M, Bhat NDR, Coles W, Dai S, Dempsey J, Keith MJ, Kerr M, Kramer M, Lasky PD, Manchester RN, Osłowski S, Parthasarathy A, Ravi V, Reardon DJ, Rosado PA, Russell CJ, Shannon RM, Spiewak R, van Straten W, Toomey L, Wang J, Wen L, You X. Parkes pulsar timing array constraints on ultralight scalarfield dark matter. Phys Rev D. 2018;98:102002. https://doi.org/10.1103/PhysRevD.98.102002.
Van Tilburg K, Leefer N, Bougas L, Budker D. Search for ultralight scalar dark matter with atomic spectroscopy. Phys Rev Lett. 2015;115:011802. https://doi.org/10.1103/PhysRevLett.115.011802.
Hees A, Guéna J, Abgrall M, Bize S, Wolf P. Searching for an oscillating massive scalar field as a dark matter candidate using atomic hyperfine frequency comparisons. Phys Rev Lett. 2016;117:061301. https://doi.org/10.1103/PhysRevLett.117.061301.
Stadnik YV, Flambaum VV. Improved limits on interactions of lowmass spin0 dark matter from atomic clock spectroscopy. Phys Rev A. 2016;94:022111. https://doi.org/10.1103/PhysRevA.94.022111.
Stadnik YV, Flambaum VV. Enhanced effects of variation of the fundamental constants in laser interferometers and application to darkmatter detection. Phys Rev A. 2016;93:063630. https://doi.org/10.1103/PhysRevA.93.063630.
Kennedy CJ, Oelker E, Robinson JM, Bothwell T, Kedar D, Milner WR, Marti GE, Derevianko A, Ye J. Precision metrology meets cosmology: improved constraints on ultralight dark matter from atomcavity frequency comparisons. Phys Rev Lett. 2020;125:201302. https://doi.org/10.1103/PhysRevLett.125.201302.
Vermeulen SM, Relton P, Grote H, Raymond V, Affeldt C, Bergamin F, Bisht A, Brinkmann M, Danzmann K, Doravari S, Kringel V, Lough J, Lück H, Mehmet M, Mukund N, Nadji S, Schreiber E, Sorazu B, Strain KA, Vahlbruch H, Weinert M, Willke B. Direct limits for scalar field dark matter from a gravitationalwave detector. Nature. 2021;600:424–8.
Branca A, Bonaldi M, Cerdonio M, Conti L, Falferi P, Marin F, Mezzena R, Ortolan A, Prodi GA, Taffarello L, Vedovato G, Vinante A, Vitale S, Zendri JP. Search for an ultralight scalar dark matter candidate with the AURIGA detector. Phys Rev Lett. 2017;118:021302. https://doi.org/10.1103/PhysRevLett.118.021302.
Smith GL, Hoyle CD, Gundlach JH, Adelberger EG, Heckel BR, Swanson HE. Shortrange tests of the equivalence principle. Phys Rev D. 1999;61:022001. https://doi.org/10.1103/PhysRevD.61.022001.
Schlamminger S, Choi KY, Wagner TA, Gundlach JH, Adelberger EG. Test of the equivalence principle using a rotating torsion balance. Phys Rev Lett. 2008;100:041101. https://doi.org/10.1103/PhysRevLett.100.041101.
Touboul P, Métris G, Rodrigues M, André Y, Baghi Q, Bergé J, Boulanger D, Bremer S, Carle P, Chhun R, Christophe B, Cipolla V, Damour T, Danto P, Dittus H, Fayet P, Foulon B, Gageant C, Guidotti PY, Hagedorn D, Hardy E, Huynh PA, Inchauspe H, Kayser P, Lala S, Lämmerzahl C, Lebat V, Leseur P, Liorzou F, List M, Löffler F, Panet I, Pouilloux B, Prieur P, Rebray A, Reynaud S, Rievers B, Robert A, Selig H, Serron L, Sumner T, Tanguy N, Visser P. MICROSCOPE mission: first results of a space test of the equivalence principle. Phys Rev Lett. 2017;119:231101. https://doi.org/10.1103/PhysRevLett.119.231101.
Bergé J, Brax P, Métris G, PernotBorràs M, Touboul P, Uzan JP. MICROSCOPE mission: first constraints on the violation of the weak equivalence principle by a light scalar dilaton. Phys Rev Lett. 2018;120:141101. https://doi.org/10.1103/PhysRevLett.120.141101.
Centers GP, Blanchard JW, Conrad J, Figueroa NL, Garcon A, Gramolin AV, Kimball DFJ, Lawson M, Pelssers B, Smiga JA, Sushkov AO, Wickenbrock A, Budker D, Derevianko A. Stochastic fluctuations of bosonic dark matter. Nat Commun. 2021;12:7321.
Martin J. Quintessence: a minireview. Mod Phys Lett A. 2008;23:1252–65. https://doi.org/10.1142/S0217732308027631. arXiv:0803.4076.
Wetterich C. An asymptotically vanishing timedependent cosmological “constant”. Astron Astrophys. 1995;301:321. arXiv:hepth/9408025.
Amendola L. Scaling solutions in general nonminimal coupling theories. Phys Rev D. 1999;60:043501. https://doi.org/10.1103/PhysRevD.60.043501.
Amendola L. Coupled quintessence. Phys Rev D. 2000;62:043511. https://doi.org/10.1103/PhysRevD.62.043511.
Dvali G, Zaldarriaga M. Changing α with time: implications for fifthforcetype experiments and quintessence. Phys Rev Lett. 2002;88:091303. https://doi.org/10.1103/PhysRevLett.88.091303.
Chiba T, Kohri K. Quintessence cosmology and varying α. Prog Theor Phys. 2002;107(3):631–6. https://doi.org/10.1143/PTP.107.631. https://academic.oup.com/ptp/articlepdf/107/3/631/5121258/1073631.pdf.
Damour T, Piazza F, Veneziano G. Runaway dilaton and equivalence principle violations. Phys Rev Lett. 2002;89:081601. https://doi.org/10.1103/PhysRevLett.89.081601.
Damour T, Piazza F, Veneziano G. Violations of the equivalence principle in a dilatonrunaway scenario. Phys Rev D. 2002;66:046007. https://doi.org/10.1103/PhysRevD.66.046007.
Wetterich C. Crossover quintessence and cosmological history of fundamental “constants”. Phys Lett B. 2003;561(1):10–6. https://doi.org/10.1016/S03702693(03)003836.
Anchordoqui L, Goldberg H. Time variation of the fine structure constant driven by quintessence. Phys Rev D. 2003;68:083513. https://doi.org/10.1103/PhysRevD.68.083513.
Copeland EJ, Nunes NJ, Pospelov M. Models of quintessence coupled to the electromagnetic field and the cosmological evolution of alpha. Phys Rev D. 2004;69:023501. https://doi.org/10.1103/PhysRevD.69.023501.
Lee S, Olive KA, Pospelov M. Quintessence models and the cosmological evolution of α. Phys Rev D. 2004;70:083503. https://doi.org/10.1103/PhysRevD.70.083503.
Marra V, Rosati F. Cosmological evolution of alpha driven by a general coupling with quintessence. J Cosmol Astropart Phys. 2005;2005(05):011. https://doi.org/10.1088/14757516/2005/05/011.
Lee S. Time variation of fine structure constant and proton–electron mass ratio with quintessence. Mod Phys Lett A. 2007;22(25n28):2003–11. https://doi.org/10.1142/S0217732307025236.
Shlyakhter A. Direct test of the constancy of fundamental nuclear constants. Nature. 1976;264(5584):340.
Damour T, Dyson F. The Oklo bound on the time variation of the finestructure constant revisited. Nucl Phys B. 1996;480(1):37–54. https://doi.org/10.1016/S05503213(96)004671.
Fujii Y, Iwamoto A, Fukahori T, Ohnuki T, Nakagawa M, Hidaka H, Oura Y, Möller P. The nuclear interaction at Oklo 2 billion years ago. Nucl Phys B. 2000;573(1):377–401. https://doi.org/10.1016/S05503213(00)000389.
Petrov YV, Nazarov AI, Onegin MS, Petrov VY, Sakhnovsky EG. Natural nuclear reactor at Oklo and variation of fundamental constants: computation of neutronics of a fresh core. Phys Rev C. 2006;74:064610. https://doi.org/10.1103/PhysRevC.74.064610.
Olive KA, Pospelov M, Qian YZ, Coc A, Cassé M, VangioniFlam E. Constraints on the variations of the fundamental couplings. Phys Rev D. 2002;66:045022. https://doi.org/10.1103/PhysRevD.66.045022.
Carroll SM. Quintessence and the rest of the world. Phys Rev Lett. 1998;81:3067–70. https://doi.org/10.1103/PhysRevLett.81.3067. arXiv:astroph/9806099.
Vilenkin A. Cosmic strings and domain walls. Phys Rep. 1985;121(5):263–315. https://doi.org/10.1016/03701573(85)90033X.
’t Hooft G. Magnetic monopoles in unified gauge theories. Nucl Phys B. 1974;79(2):276–84. https://doi.org/10.1016/05503213(74)904866.
Polyakov AM. Particle spectrum in quantum field theory. In: 30 years of the Landau institute—selected papers. Singapore: World Scientific; 1996. p. 540–1.
Abrikosov AA. On the magnetic properties of superconductors of the second group. Sov Phys JETP. 1957;5:1174–82.
Nielsen HB, Olesen P. Vortexline models for dual strings. Nucl Phys B. 1973;61:45–61. https://doi.org/10.1016/05503213(73)903507.
Zel’Dovich YB, Kobzarev IY, Okun LB. Cosmological consequences of a spontaneous breakdown of a discrete symmetry. Sov Phys JETP. 1975;40:1.
Press WH, Ryden BS, Spergel DN. Dynamical evolution of domain walls in an expanding universe. Astrophys J. 1989;347:590–604.
Urrestilla J, Bevis N, Hindmarsh M, Kunz M, Liddle AR. Cosmic microwave anisotropies from BPS semilocal strings. J Cosmol Astropart Phys. 2008;2008(07):010. https://doi.org/10.1088/14757516/2008/07/010.
Friedberg R, Lee TD, Sirlin A. Class of scalarfield soliton solutions in three space dimensions. Phys Rev D. 1976;13:2739–61. https://doi.org/10.1103/PhysRevD.13.2739.
Coleman S. Qballs. Nucl Phys B. 1985;262(2):263–83. https://doi.org/10.1016/05503213(85)90286X.
Wcisło P, Morzyński P, Bober M, Cygan A, Lisak D, Ciuryło R, Zawada M. Experimental constraint on dark matter detection with optical atomic clocks. Nat Astron. 2016;1(1):1–6.
Oliveira JCRE, Martins CJAP, Avelino PP. Cosmological evolution of domain wall networks. Phys Rev D. 2005;71:083509. https://doi.org/10.1103/PhysRevD.71.083509.
Avelino PP, Martins CJAP, Oliveira JCRE. Onescale model for domain wall network evolution. Phys Rev D. 2005;72:083506. https://doi.org/10.1103/PhysRevD.72.083506.
Planck Collaboration, Aghanim, N. Planck 2018 results—VI. Cosmological parameters. Astron Astrophys. 2020;641:6. https://doi.org/10.1051/00046361/201833910.
Kostelecky VA, Samuel S. Spontaneous breaking of Lorentz symmetry in string theory. Phys Rev D. 1989;39:683. https://doi.org/10.1103/PhysRevD.39.683.
Kostelecky VA, Potting R. CPT, strings, and meson factories. Phys Rev D. 1995;51:3923–35. https://doi.org/10.1103/PhysRevD.51.3923. arXiv:hepph/9501341.
Kostelecky VA, Potting R. CPT and strings. Nucl Phys B. 1991;359:545–70. https://doi.org/10.1016/05503213(91)900715.
Kostelecky VA, Potting R. Expectation values, Lorentz invariance, and CPT in the open bosonic string. Phys Lett B. 1996;381:89–96. https://doi.org/10.1016/03702693(96)005898. arXiv:hepth/9605088.
Ellis JR, Mavromatos NE, Nanopoulos DV. Derivation of a vacuum refractive index in a stringy spacetime foam model. Phys Lett B. 2008;665:412–7. https://doi.org/10.1016/j.physletb.2008.06.029. arXiv:0804.3566.
Gliozzi F. Dirac–Born–Infeld action from spontaneous breakdown of Lorentz symmetry in braneworld scenarios. Phys Rev D. 2011;84:027702. https://doi.org/10.1103/PhysRevD.84.027702. arXiv:1103.5377.
Hashimoto K, Murata M. A landscape in boundary string field theory: new class of solutions with massive state condensation. Prog Theor Exp Phys. 2013;2013:043B01. https://doi.org/10.1093/ptep/ptt010. arXiv:1211.5949.
Gambini R, Pullin J. Emergence of stringlike physics from Lorentz invariance in loop quantum gravity. Int J Mod Phys D. 2014;23(12):1442023. https://doi.org/10.1142/S0218271814420231. arXiv:1406.2610.
Rovelli C, Speziale S. Lorentz covariance of loop quantum gravity. Phys Rev D. 2011;83:104029. https://doi.org/10.1103/PhysRevD.83.104029. arXiv:1012.1739.
Carroll SM, Harvey JA, Kostelecky VA, Lane CD, Okamoto T. Noncommutative field theory and Lorentz violation. Phys Rev Lett. 2001;87:141601. https://doi.org/10.1103/PhysRevLett.87.141601. arXiv:hepth/0105082.
Carlson CE, Carone CD, Lebed RF. Bounding noncommutative QCD. Phys Lett B. 2001;518:201–6. https://doi.org/10.1016/S03702693(01)010450. arXiv:hepph/0107291.
Calmet X. Spacetime symmetries of noncommutative spaces. Phys Rev D. 2005;71:085012. https://doi.org/10.1103/PhysRevD.71.085012. arXiv:hepth/0411147.
Calmet X. What are the bounds on spacetime noncommutativity? Eur Phys J C. 2005;41:269–72. https://doi.org/10.1140/epjc/s2005022269. arXiv:hepph/0401097.
Bailey QG, Lane CD. Relating noncommutative \(\mathrm{SO}(2, 3)_{\bigstar}\) gravity to the Lorentzviolating standardmodel extension. Symmetry. 2018;10(10):480. https://doi.org/10.3390/sym10100480. arXiv:1810.05136.
Carroll SM, Field GB, Jackiw R. Limits on a Lorentz and parity violating modification of electrodynamics. Phys Rev D. 1990;41:1231. https://doi.org/10.1103/PhysRevD.41.1231.
Coleman SR, Glashow SL. Highenergy tests of Lorentz invariance. Phys Rev D. 1999;59:116008. https://doi.org/10.1103/PhysRevD.59.116008. arXiv:hepph/9812418.
Kostelecký VA, Li Z. Backgrounds in gravitational effective field theory. Phys Rev D. 2021;103(2):024059. https://doi.org/10.1103/PhysRevD.103.024059. arXiv:2008.12206.
Kostelecký VA, Li Z. Searches for beyondRiemann gravity. Phys Rev D. 2021;104(4):044054. https://doi.org/10.1103/PhysRevD.104.044054. arXiv:2106.11293.
de Rham C. Massive gravity. Living Rev Relativ. 2014;17:7. https://doi.org/10.12942/lrr20147. arXiv:1401.4173.
Horava P. Quantum gravity at a Lifshitz point. Phys Rev D. 2009;79:084008. https://doi.org/10.1103/PhysRevD.79.084008. arXiv:0901.3775.
Bluhm R, Kostelecky VA. Spontaneous Lorentz violation, Nambu–Goldstone modes, and gravity. Phys Rev D. 2005;71:065008. https://doi.org/10.1103/PhysRevD.71.065008. arXiv:hepth/0412320.
Bluhm R, Fung SH, Kostelecky VA. Spontaneous Lorentz and diffeomorphism violation, massive modes, and gravity. Phys Rev D. 2008;77:065020. https://doi.org/10.1103/PhysRevD.77.065020. arXiv:0712.4119.
Bluhm R. Explicit versus spontaneous diffeomorphism breaking in gravity. Phys Rev D. 2015;91(6):065034. https://doi.org/10.1103/PhysRevD.91.065034. arXiv:1401.4515.
Weinberg S. Effective field theory, past and future. In: 6th international workshop on chiral dynamics (CD09). PoS. 2009. https://doi.org/10.22323/1.086.0001. 0908.1964.
Colladay D, Kostelecky VA. CPT violation and the standard model. Phys Rev D. 1997;55:6760–74. https://doi.org/10.1103/PhysRevD.55.6760. arXiv:hepph/9703464.
Colladay D, Kostelecky VA. Lorentz violating extension of the standard model. Phys Rev D. 1998;58:116002. https://doi.org/10.1103/PhysRevD.58.116002. arXiv:hepph/9809521.
Kostelecky VA. Gravity, Lorentz violation, and the standard model. Phys Rev D. 2004;69:105009. https://doi.org/10.1103/PhysRevD.69.105009. arXiv:hepth/0312310.
Bluhm R. Overview of the SME: implications and phenomenology of Lorentz violation. Lect Notes Phys. 2006;702:191–226. https://doi.org/10.1007/354034523X_8. arXiv:hepph/0506054.
Tasson JD. What do we know about Lorentz invariance? Rep Prog Phys. 2014;77:062901. https://doi.org/10.1088/00344885/77/6/062901. arXiv:1403.7785.
Kostelecky AV, Tasson JD. Mattergravity couplings and Lorentz violation. Phys Rev D. 2011;83:016013. https://doi.org/10.1103/PhysRevD.83.016013. arXiv:1006.4106.
Mewes M. Nonminimal Lorentz violation in macroscopic matter. Symmetry. 2020;12(12):2026. https://doi.org/10.3390/sym12122026. arXiv:2012.08302.
Jackiw R, Kostelecky VA. Radiatively induced Lorentz and CPT violation in electrodynamics. Phys Rev Lett. 1999;82:3572–5. https://doi.org/10.1103/PhysRevLett.82.3572. arXiv:hepph/9901358.
Bluhm R, Kostelecky VA, Russell N. CPT and Lorentz tests in hydrogen and antihydrogen. Phys Rev Lett. 1999;82:2254–7. https://doi.org/10.1103/PhysRevLett.82.2254. arXiv:hepph/9810269.
Kostelecky VA, Lane CD. Constraints on Lorentz violation from clock comparison experiments. Phys Rev D. 1999;60:116010. https://doi.org/10.1103/PhysRevD.60.116010. arXiv:hepph/9908504.
Bluhm R, Kostelecky VA, Lane CD, Russell N. Clock comparison tests of Lorentz and CPT symmetry in space. Phys Rev Lett. 2002;88:090801. https://doi.org/10.1103/PhysRevLett.88.090801. arXiv:hepph/0111141.
Kostelecký VA, Vargas AJ. Lorentz and CPT tests with clockcomparison experiments. Phys Rev D. 2018;98(3):036003. https://doi.org/10.1103/PhysRevD.98.036003. arXiv:1805.04499.
Vargas AJ. Overview of the phenomenology of Lorentz and CPT violation in atomic systems. Symmetry. 2019;11(12):1433. https://doi.org/10.3390/sym11121433.
Foldy LL, Wouthuysen SA. On the Dirac theory of spin 1/2 particle and its nonrelativistic limit. Phys Rev. 1950;78:29–36. https://doi.org/10.1103/PhysRev.78.29.
Kostelecky VA, Lane CD. Nonrelativistic quantum Hamiltonian for Lorentz violation. J Math Phys. 1999;40:6245–53. https://doi.org/10.1063/1.533090. arXiv:hepph/9909542.
Hohensee MA, Leefer N, Budker D, Harabati C, Dzuba VA, Flambaum VV. Limits on violations of Lorentz symmetry and the Einstein equivalence principle using radiofrequency spectroscopy of atomic dysprosium. Phys Rev Lett. 2013;111:050401. https://doi.org/10.1103/PhysRevLett.111.050401. arXiv:1303.2747.
Hohensee MA, Chu S, Peters A, Muller H. Equivalence principle and gravitational redshift. Phys Rev Lett. 2011;106:151102. https://doi.org/10.1103/PhysRevLett.106.151102. arXiv:1102.4362.
Dzuba VA, Flambaum VV, Safronova MS, Porsev SG, Pruttivarasin T, Hohensee MA, Häffner H. Strongly enhanced effects of Lorentz symmetry violation in entangled Yb^{+} ions. 2015. arXiv:1507.06048.
Safronova MS, Johnson WR. Allorder methods for relativistic atomic structure calculations. In: Advances in atomic, molecular, and optical physics. vol. 55. San Diego: Academic Press; 2008. p. 191–233. https://doi.org/10.1016/S1049250X(07)550044. https://www.sciencedirect.com/science/article/pii/S1049250X07550044.
Shaniv R, Ozeri R, Safronova MS, Porsev SG, Dzuba VA, Flambaum VV, Häffner H. New methods for testing Lorentz invariance with atomic systems. Phys Rev Lett. 2018;120(10):103202. https://doi.org/10.1103/PhysRevLett.120.103202. arXiv:1712.09514.
Dzuba VA, Flambaum VV. Limits on gravitational Einstein equivalence principle violation from monitoring atomic clock frequencies during a year. Phys Rev D. 2017;95(1):015019. https://doi.org/10.1103/PhysRevD.95.015019. arXiv:1608.06050.
Pruttivarasin T, Ramm M, Porsev SG, Tupitsyn II, Safronova M, Hohensee MA, Haeffner H. A michelsonMorley test of Lorentz symmetry for electrons. Nature. 2015;517:592.