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# Anomalous diffraction of matter waves with minimal quantum metasurfaces

*EPJ Quantum Technology*
**volume 8**, Article number: 3 (2021)

## Abstract

In the last few years, there is a huge upsurge in the number of closed deals regarding quantum technologies for materials, computing, communication and instrumentation. Such a trend has inevitably affected the research funding market; thus, large state initiatives are taken that are directly expected to drive the formulation of novel research concepts and the development of quantum device prototypes from sensors and circuitry to quantum memory and repeaters. A fundamental operation behind all these applications is the effective steering of electrons, constituting matter waves, along specific directions and with certain magnitudes, due to development of various reflective and refractive orders. The objective of this study is to optimize the simplest structure that supports such anomalous diffraction, namely a quantum metasurface comprising cylindrical rods embedded in suitable crystalline matter. Several highly-performing designs from these minimal setups are proven to work exceptionally as multiport components, employable to a variety of quantum engineering implementations.

## Introduction

Quantum technologies are today developing at a rapid pace and providing novel concepts that address in a revolutionary manner multiple core scientific problems. Quite high on this list one may find quantum sensing that boosts dramatically the optical resolution of extremely close point-like sources [1] and sets new limits in spectroscopy and metrology via quantum interpolation [2]. Such evolutions have led to demonstration of quantum memory that enhances the interval over which phases are accumulated, beyond the coherence lifetime [3]. Moreover, quantum communication technologies based on solid-state devices enabling stogage of quantum entanglement have been proposed, paving the way for building multiplexed repeaters for long-distance quantum networks [4]. Importantly, whole classes of computational tasks have been found to be executed exponentially faster on a quantum processor than on a classical one, regardless of the employed algorithm, indicating a first realization of quantum supremacy [5, 6]. Even quantum network architectures have become feasible via interconnections that convert quantum states from one physical system to those of another in a reversible way [7].

All the aforementioned scientific breakthroughs leading to modules most of which are at an infant stage, have ignited large quantum research investments from industry titans and prioritized quantum information science in careful strategic plans [8, 9]. In particular, several workshops on the future of quantum engineering as an emerging branch [10] and brainstorming in roundtables on how the research competitiveness will be maintained in quantum computing [11], culminated in impressive initiatives [12]. Such huge bills are expected to further stimulate research on quantum technologies in the near future even though the funding interest is already high. Only the last few years, several Multi-University Research Initiatives (MURIs) have been approved from Army Research Office (ARO) on ab-initio characterization of quantum materials [13], from Air Force Office of Scientific Research (AFOSR) on certifying untrusted quantum devices [14] and from US Department of Defense (DoD) on quantum state control of molecular collision dynamics [15], all concerning the suitable pairing of matter waves with quantum texture.

A backbone operation behind all these fancy applications is the steering of quantum particle beams along specific routes and with certain intensities to be processed accordingly for computation, simulation or memory purposes. It is usually achieved by crafting sophisticated paths of specific material on a host base, along which the quantum signals are guided [16] or exploiting spin-orbit interaction into ring structures to make them work as splitters [17]. Similarly, quantum interference is used for spectral demultiplexing with help from directional couplers and add-drop filters, all these integrated on a single monolithic silicon chip [18]. The same on-chip philosophy is adopted by solid-state quantum sensors with applications in magnetometry, thermometry and chemical sensing [19]. Moreover, a superconducting quantum processor with multiple transmon qubits coupled via coplanar waveguide resonators has been proposed [20] while photonics quantum circuits enabling generation, manipulation, and analysis of multidimensional quantum systems have been experimentally tested [21].

One may accomplish efficient quantum signal steering alternative to opening guidance paths into a background matrix [22], by developing a structure that diffracts the incoming matter waves at controllable axes and pre-determined probabilities. Such an idea is borrowed from Photonics, where suitable phase discontinuities to reflective or refractive waves are imprinted through metasurfaces of optical resonators [23] to develop anomalous diffractive phenomena that, in turn, formulate multi-port networks with tailorable their overall response [24]. Anomalous effects, namely diffraction along counter-intuitive directions, has been investigated in Quantum Mechanics but only in the context of measuring the response for guessing the inhomogeneities size/shape into a host matrix; it aims at recovering non-destructively the composition of embedded nanostructures and makes a hard three-dimensional inverse problem [25, 26]. However, deliberately creating simply-shaped inclusions, like cylindrical posts, into a background medium is a relatively feasible task via several fabrication methods. In particular, one can engrave chemically nanowires [27] or epitaxially grow radially inhomogeneous elongated heterostructures [28], either following a bottom-up building [29] or top-down dipping [30] approach.

In this work, we investigate the simplest version of this realistically constructable class of quantum devices, namely a periodic metasurface comprising circular cylindrical cavities of specific texture and large length, being embedded into a background host [31]. The structure is obliquely illuminated by a beam of electrons and explicit expressions for the directions and the magnitudes of the developed diffraction waves are obtained. The analyzed effect is based on the interference of electron beams whose principles have been formulated many decades ago [32]. However, our work differs from studies of similar objectives that use multiple gratings but do not solve analytically the boundary value problems [33, 34] or employ isolated rods without collective operations [35]. Particular emphasis is placed on the first anomalous order and various combinations of inclusion materials and backgrounds are examined; for each of them, the incidence angle, the energy of the incoming beam and the cylinders size are selected so that the anomalous reflection or transmission is maximized. It is found that quantum well configurations give higher scores than their quantum barrier counterparts [36] while the operation of the device as a quantum multiport with several diffractive channels, is demonstrated. Therefore, this study gives numerous alternative minimal designs for splitting and steering components that may be utilized in various quantum setups from circuitry and memory elements to signal processing and repeaters.

## Mathematical formulation

### Configuration and assumptions

Let us consider a plane matter wave created by an electron beam whose particles move along a specific direction with equal probability of existence across the planes normal to it. The beam is traveling into a host medium whose macroscopic potential energy is denoted by \(V_{0}\) while the effective mass of an electron within equals \(m_{0}\); since the developed matter wave is propagating, the kinetic energy of its particles is larger (by *E*) than the local potential level \(V_{0}\). It should be declared that, in this model, the impurity of phonon scattering is not taken into account and, accordingly, the electron wave is regarded as coherent [37]; in other words, the particle beam can be represented by a specific wave vector. Therefore, the incoming beam is characterized by a single energy *E* which is feasible if passed through an energy-selective setup like tilted nanocavities [38] or planar layers [39]. The impinging quantum wave meets obliquely (under angle *θ*, as in Fig. 1) a grating with period 2*b* comprising cylindrical inclusions of radius \(a< b\) and filled with a different quantum material of energy \(V=V_{0}-\Delta V\) and effective mass *m*.

From fundamentals of Quantum Mechanics [40, pp. 11–15], we know that, the key quantity determining the interaction of any e-beam with its environment is the wave function \(\Psi (\mathbf{r})\) whose squared magnitude is proportional to the probability of finding the electron at a point with position vector **r**. The time-independent Schrödinger equation [41, p. 31] respected by the wave function of any e-beam is written as:

where *E* is the total energy of the beam, \(V(\mathbf{r})\) the local potential energy and \(m(\mathbf{r})\) the local effective mass; obviously *ħ* stands for the reduced Planck constant.

Note that in Fig. 1, we assign to each of the cylindrical inclusions an integer number *n* and we define infinite coordinate systems \((r_{n},\varphi _{n})\equiv (x_{n},y_{n})\) for \(n\in \mathbb{Z}\), each one centralized at one post. The global coordinate system \((r,\varphi )\equiv (x,y)\) is assumed the one with \(n=0\). The wave function describing the incoming matter wave, if the parallel wires were absent, takes the form \(\Psi _{\mathrm{back}}=e^{-i k_{0} x \cos \theta - i k_{0} y \sin \theta }\), where \(k_{0}=\sqrt{2m_{0}E}/\hbar \) is the wavenumber of the impinging beam into background medium. On the contrary, by adopting partial wave formalism [42, p. 596], the wave function into the central (\(n=0\)) post is written as: \(\Psi ^{(0)}_{\mathrm{int}}=\sum_{p=-\infty }^{+\infty }c_{p}J_{p}(kr)e^{ip \varphi }\), where \(c_{p}\) are complex determinable constants (\(p\in \mathbb{Z}\)), \(J_{p}\) the Bessel function of *p*th order and \(k=\sqrt{2m(E+\Delta V)}/\hbar \) corresponds to the wave vector norm into the cavity material. As far as the perturbation that \(\Psi _{\mathrm{back}}\) feels due to the central inclusion is concerned, it is given by: \(\Psi ^{(0)}_{\mathrm{scat}}=\sum_{p=-\infty }^{+\infty }s_{p}H_{p}(k_{0}r)e^{ip \varphi }\) where \(s_{p}\) are complex determinable coefficients (\(p\in \mathbb{Z}\)) while \(H_{p}\) is the Hankel function of second type and *p*th order.

Interestingly, due to the infinite front of the incident electron beam \(\Psi _{\mathrm{back}}\) and the infinite extent of the grating along *y* axis, the wave function into any other (\(n\ne 0\)) post and its contribution to the overall scattering effect are written via no additional coefficients than the ones of the central cylinder \(\{c_{p},s_{p}\}\). Indeed, the response of the *n*th cavity will be identical to that of the 0th one but expressed in its local coordinate system \((r_{n},\varphi _{n})\) and multiplied by the term \(\sigma _{n}=e^{- i k_{0} 2 b n \sin \theta }\) corresponding to the phase of the incident wave at the center of *n*th inclusion; namely: \(\Psi ^{(n)}_{\mathrm{int}}=\sigma _{n}\sum_{p=-\infty }^{+\infty }c_{p}J_{p}(kr_{n})e^{ip \varphi _{n}}\) and \(\Psi ^{(n)}_{\mathrm{scat}}=\sigma _{n}\sum_{p=-\infty }^{+\infty }s_{p}H_{p}(k_{0}r_{n})e^{ip \varphi _{n}}\).

### Near field and boundary conditions

If one employs the addition theorem for cylindrical coordinates [43, pp. 372–374], all scattering components can be expressed in terms of the central polar coordinate system \((r,\varphi )\). In particular:

where the first term corresponds to the central inclusion (\(n=0\)) and the second one to all the others. Indeed, the symbol \(K_{w}\) is used for the following slowly-convergent series:

By imposing the required boundary conditions only around the central cylinder \(r=a\) for continuity of the complex-valued wave function \(\Psi ^{(0)}_{\mathrm{int}}=\Psi _{\mathrm{back}}+\Psi _{\mathrm{scat}}\) and proportionality of its normal derivative \(\hat{\mathbf{r}}\cdot \nabla \Psi ^{(0)}_{\mathrm{int}}/m=\hat{\mathbf{r}} \cdot \nabla [\Psi _{\mathrm{back}}+\Psi _{\mathrm{scat}} ]/m_{0}\), the following linear system for the unknowns \(\{c_{p},s_{p}\}\) is formulated:

for \(p\in \mathbb{Z}\) while the prime denotes the derivative with respect to the entire argument. The only numerical issue that may emerge in solving (3), is the evaluation of the infinite sums \(K_{p-q}\) which possess oscillatory and slowly decaying general terms (as \(1/\sqrt{|n|}\)) with respect to *n* [44, p. 364]. To overcome such a computational snag, we exploit the analytical formula [45, p. 6]: \(\sum_{n=1}^{+\infty }e^{-2ik_{0}b(|n|+n\sin \theta )}/\sqrt{|n|}={ \mathrm{Li}}_{1/2} (e^{-2ik_{0}b(1+\sin \theta )} )\), where \(\mathrm{Li}_{1/2}\) is the polylogarithm function of order \(1/2\). To put it more clearly, we subtract the asymptotic general terms of Hankel-related functions from the corresponding series (2) and we simultaneously add the aforementioned equivalent analytical result. The remainder sum converges much faster since the higher order terms of the difference vanish rapidly [46].

### Far field and diffractive channels

Once the linear system (3) gets properly truncated with respect to *p*, the values of the angular spectral coefficients inside and outside the cylindrical inclusions \(\{c_{p},s_{p}\}\) are rigorously determined. Given the fact that the size 2*a* of the posts is small compared to the spatial wavelength \(2\pi /k_{0}\) of the impinging wave, it is reasonable to ignore the contribution from azimuthal terms \(e^{-ip\theta }\) of higher angular momentum *p*. Importantly, we are interested for the far field (\(r\rightarrow +\infty \)) and the infinite dimension of the structure, combined with its symmetry, renders the effect of the scattering orders with \(|p|>1\) on the final outcome, somehow less significant. More specifically, we keep the omni-directional (\(p=0\)) and the bipolar (\(p=\pm 1\)) variations in the scattering wave function. Let us consider the general term \(W_{p}(k_{0}a)= \vert J_{p}(k_{0}a)/H_{p}(k_{0}a) \vert \) corresponding to the solution of a single impenetrable cylinder of radius *a* embedded into a background where the impinging matter wave has wavenumber \(k_{0}\). The bipolar approximation is valid as long as \(W_{2}(k_{0}a)\ll \min \{ W_{0}(k_{0}a),W_{\pm 1}(k_{0}a) \} \), namely when \(k_{0}a<\pi /2\).

If one defines \(s_{1C}=s_{+1}-s_{-1}\) and \(s_{1S}=i(s_{+1}+s_{-1})\), the quantity in (1) is written in terms of the global Cartesian coordinates \((x,y)\) for the far field (\(x\rightarrow \pm \infty \)) as follows:

where \(G(x,y)=\sum_{n=-\infty }^{+\infty }\sigma _{n} H_{0} (k_{0}\sqrt{x^{2}+(y-2bn)^{2}} )\).

If one applies Poisson summation formula [47, p. 467] for the sum defining the function \(G(x,y)\) and uses the Fourier pair for Hankel function indicated by [47, p. 823]: \(H_{0} (k_{0}\sqrt{x^{2}+y^{2}} )=\frac{i}{\pi }\int _{- \infty }^{+\infty }\exp (-i\beta y-|x|\sqrt{\beta ^{2}-k_{0}^{2}})/ \sqrt{\beta ^{2}-k_{0}^{2}} \,d\beta \), the wave function of (4), is written as:

where \(\kappa _{u}=\sqrt{(u\pi +k_{0}b\sin \theta )^{2}-(k_{0}b)^{2}}\). For \(x<0\), we have reflective matter waves while for \(x>0\), we obtain transmissive ones with complex amplitudes:

respectively. The first term in (6) concerns the impinging wave function in the background and \(\delta _{u0}\) is the Kronecker’s delta which equals one only for \(u=0\), otherwise zero.

It should be stressed that the scattering component of the wave function comprises infinite diffraction terms each characterized by an integer order \(u\in \mathbb{Z}\). In Fig. 1, we schematically show three of them, every single of which corresponds to an independent refractive channel. Indeed, due to the infinite extent of the developed waves, they are linearly independent each other, namely \(\int _{-\infty }^{+\infty }\int _{-\infty }^{+\infty }e^{-i(k_{x}-k_{x}')}e^{-i(k_{y}-k^{ \prime }_{y})}\,dx\,dy=(2\pi )^{2} \delta (k_{x}-k_{x}')\delta (k_{y}-k_{y}')\), where *δ* is the Dirac’s delta function and thus they can work as channels of a quantum multiport networks where information is hidden in the magnitude or phase of the wave function. The condition for the diffraction order *u* to give a propagating mode reads:

for which \(\kappa _{u}\) is purely imaginary. Note that the quantity at the left-hand side of (7) is always negative and thus affects only the orders with \(u<0\), while the opposite happens for the right-hand side limit (concerns diffraction of \(u>0\)). The angle at which the waves of diffraction order *u* are traveling (either reflecting or refractive) is equal to: \(\theta _{u}=\arcsin (\frac{u\pi }{k_{0}b}+\sin \theta )\). In Fig. 2(a), we represent on the plane with horizontal axis the incoming beam angle *θ* and with vertical axis the period of the grating divided by the traveling wavelength \(k_{0}b\), the limits imposed by the inequality (7) for various positive and negative orders. These lines indicate the \(k_{0}b\) (at fixed angle *θ*) beyond which the diffracting channel of the related order carries a propagating wave. It is clear that responses of opposite orders *u* are generated together (at normal incidence \(\theta =0^{\circ}\)) and as the incoming beam gets more and more oblique, it becomes easier for an anomalous wave (smaller \(k_{0}b\) limit for \(u<0\)) to exist compared to an ordinary one (larger \(k_{0}b\) limit for \(u>0\)). The non-blank parametric region contains \((\theta ,k_{0}b)\) combinations supporting only the first anomalous order \(u=-1\), except of course the inevitable Snell’s response (\(u=0\)). Across this “curved parallelogram”, we represent the quantity \((\theta +\theta _{-1})\) describing what is the direction spread of the anomalous reflective wave compared to the incident ray. We notice that the difference in angle can belong to an extensive value range from an anomalous direction parallel to negative *y* axis at normal incidence (\(\theta =0^{\circ}\)) to a vanishing \(\theta _{u}\) at grazing ray incidence (\(\theta =90^{\circ}\)). Remarkably, the two angles are opposite (\(\theta _{-1}=- \theta \)) along the major diagonal of the colored domain defined by the limits of orders \(u=\pm 1\) and \(u=-2\); such a feature means that the electron beam is reflected back to the source that created it (\(x<0\)) and negatively refracted [48] from the other side (\(x>0\)) of the grating.

When it comes to the probabilities for the particle to travel along the reflective or transmissive direction defined via angle \(\theta _{u}\), they are given respectively by [49, p. 38]:

Indeed, the normalization condition stands only along the direction being normal (*x*) to the cluster of cylindrical cavities.

## Numerical results

### Optimization strategy

By inspection of (7), it is clear that the wave with \(u=0\) is always propagating since it is dictated by the Snell’s law [42, pp. 187–191] formed for electromagnetic fields. However, the response is quite trivial since it partially expresses the unhampered propagation of the incoming e-beam in the absence of the grating and partially the reflection achieved with a perfect mirror. On the contrary, when \(u\ne 0\), namely when the distance \(k_{0}b\) or the angle *θ* increases, we obtain modes steered at unconventional, counter-intuitive directions that can be directly exploitable to quantum circuits and quantum signal processors. If one keeps \(\theta >0\) without losing the generality since the layout is symmetric with respect to *x* axis, it is understood that the first diffraction wave that can be activated beyond ordinary Snell’s response (as \(k_{0}b\) or *θ* increases) is the one with order \(u=-1\); usually this correspond to negative diffraction direction (\(\theta _{-1}<0\)) and thus is called anomalous. Three characteristic cases for the transmissive channels are indicated in Fig. 1, where the Snell (\(\theta _{0}=\theta \)), an ordinary (\(\theta _{u}>0\)) and an anomalous (\(\theta _{u}<0\)) refraction are sketched.

To keep the objective of this study as simple as possible, we will confine ourselves to designs supporting only the ordinary Snell-like response (\(u=0\)) and the anomalous order \(u=-1\). In particular, we aim at finding gratings that suppress the conventional reflection and transmission \((\rho _{0}, \tau _{0})\) and inevitably boost the matter wave steering along the anomalous direction \((\rho _{-1}, \tau _{-1})\). Note that the condition for zero Snell’s response reads:

Our optimization scheme takes a long directory of *M* quantum media (with macroscopic potentials and effective masses) containing from isolated elements (germanium, silicon, carbon etc.) and semiconductors (arsenides, nitrides, tellurides etc.) to arbitrary alloys, mixtures and heterojunctions [50, pp. 229–245]. Sophisticated computational simulation models evaluating the effective parameters [51, pp. 75–80] that describe the transport of quantum particles into them have been developed [52], being additionally validated by high-fidelity measurements. It should be stressed that the effective masses of the materials are positive which means that the waves into them are either of purely propagating or purely evanescent nature. Note that masses can be different when the particle moves along different directions, namely the material is considered anisotropic, a property commony assumed for similar setups in Electrodynamics [53]. Every single of the \(M^{2}>1000\) combinations is tried by assigning to each material from the list, both the role of background host and the filling to the cylindrical cavities. Every single of the \(M^{2}\) designs is examined by carefully sweeping the angle of the incoming matter wave over an extensive range excluding very oblique beams: \(5^{\circ}<\theta <85^{\circ}\), the ratio between the inclusion radius over the half-period of the grating: \(0.1< a/b<0.4\) and the kinetic energy *E* of the incident particles by respecting (7) for single anomalous propagating diffraction order \(u=-1\). If one keeps the half-distance between the inclusions *b* fixed, the permissible value range for *E* at a specific *θ* is given by the pair of lines of the same color in Fig. 2(b), each of which corresponds to a different background medium with a different effective mass \(m_{0}\). Such an interval of energies giving only anomalous diffraction of \(u=-1\) (plus the Snell’s \(u=0\)), shrinks with the effective mass \(m_{0}\) (in the case of diamond, \(m_{0}\) is the highest) even though it is not apparent due to the logarithmic scale of energy axis. Note that, exactly as happens in Fig. 2(a), the vertical extent of the acceptable parametric domain initially increases with *θ* up to the breaking point that the generating loci of the two diffraction orders (\(u=-2\) and \(u=+1\)) cross each other, namely at \(\theta =\arcsin (1/3)\cong 19.5^{\circ}\). Beyond this point, the considered *E* range becomes smaller with *θ*.

By using a tight brute-force optimization scheme, our aim is to determine the cylinder size \(a/b\) (for constant *b*) that pairs better with the impinging beam of \(\{\theta , E\}\) leading to maximal anomalous reflection \(\rho _{-1}\) or transmission \(\tau _{-1}\) from (8), by approximately obeying the condition (9).

### Optimal designs response

From all the parameters defining the configuration of Fig. 1, once the pair of materials has been decided, the one changing less easily is the half-period of the grating *b*, since even the size *a* of the cavities is controllable during fabrication process, let alone the incidence angle *θ* and the impinging particles energy *E*. Indeed, regardless of the construction philosophy (bottom-up [29] or top-down [30]) or the assembly nature (physical [29] or chemical [27]), the grid at which the inclusions are planted is predetermined. Therefore, when we implementing our optimization strategy, we assume a fixed *b* throughout (\(2b=5\text{ nm}\) in Figs. 3(a) and 3(b), \(2b=10\text{ nm}\) in Figs. 3(c) and 3(d)), without varying it simultaneously. More specifically, the results of the proposed inverse process are shown in Fig. 3, where to each quantum material from our list (with \(M=32\) entries) has been assigned a serial number (s/n) in proportion to how big is its macroscopic potential energy (*V* or \(V_{0}\)). Along the horizontal axis, we show the serial number of the material filling the cylindrical nanocavities, while the vertical axis determines the texture of the background host. In this way, a square canvas of \(M^{2}=32^{2}=1024\) pixel is formed the lower right triangular part of which corresponds to quantum barrier configurations while the upper left one describes quantum well setups.

In Fig. 3(a), the represented quantity is the maximal anomalous reflection probability \(\rho _{-1}\) when the rest of parameters \(\{a/b,\theta ,E\}\) are swept as indicated above; poor results (\(\rho _{-1}<50\%\)) are omitted. We clearly observe that most of the successful designs appear at the upper left region of our materials plane, namely concern quantum well configurations giving quite high anomalous steering of the reflective wave (\(\rho _{-1}>70\%\)). However, the best score is achieved for quantum barriers configurations, namely when the background is the material of the lowest potential *V* (InSb); for certain inclusion media surpasses the limit of 90%. In Fig. 3(b), we show the results of the optimization when maximizing the transmissive probability \(\tau _{-1}\); one directly observes much higher performances compared to the case of \(\rho _{-1}\) in Fig. 3(a). Again the quantum well designs are much more efficient than the corresponding quantum barrier ones and in most examples the maximal performance reach the perfect outcome of 100%. Overall there are more combinations of materials that give significant anomalous transmission (\(\tau _{-1}>50\%\)) compared to them excelling at anomalous reflection (\(\rho _{-1}>50\%\)); however, the configurations hosted in InSb exhibit much less granted response. In Figs. 3(c) and 3(c) we consider a larger period of the cylinders grating (\(2b=10\text{ nm}\)) and repeat the maximization process described above. As far as the reflective probability is concerned, the average maximal score is lower than those in Fig. 3(a); nonetheless, there are more alternative texture pairs that deliver above the 50% threshold, most of which with low \(V_{0}\). Such a trend for more degrees of freedom when *b* is larger, has been verified by Fig. 3(d), where the maximal \(\tau _{-1}\) is shown; however, the performance remains as high as in Fig. 3(b) this time. Importantly, multiple material combinations corresponding to quantum barrier setups emerge and give acceptable anomalous transmission, while the best results are recorded for those hosts of relatively diminished potential energy.

In Fig. 4, we show the response along the anomalous direction of certain designs from Figs. 3(a), 3(b) for various incidence angles *θ* and variable impinging energies *E*; results are shown for those \((\theta , E)\) combinations that only \(u=0,-1\) diffraction orders are excited. In Fig. 4(a), we consider the anomalously reflecting design of InP posts embedded in BeTe (from Fig. 3(a)). The maximization of the represented quantity \(\rho _{-1}\) occurs in the middle of the map, while it vanishes close to the borders generating diffraction of \(u=+1\) or \(u=-2\); however, when one crosses parametrically such a boundary may experience huge increase in high-order response. In Fig. 4(b), we regard the highest-performing quantum grating, namely CdO cylinders into InSb (from Fig. 3(a)) with \(\rho _{-1}>90\%\). The operational range of energies *E* is much larger since the effective mass of InSb host \(m_{0}\) is tiny (see Fig. 2(b)); in addition, the resonance is substantially sharper than the one of Fig. 4(a) even though it occurs in a similar *E*-interval.

In Fig. 4(c), we move to maximally-\(\tau _{-1}\) setups and examine the optimal CdTe cavities in AlN background (from Fig. 3(b)). We notice that the peak is exhibited for \(\theta \cong \arcsin (1/3)\) and close to the maximal permissible energy. Furthermore, the represented quantity does not vanish when higher diffractive orders are developed while a secondary local maximum appears at lower *E* for \(\theta \cong 45^{\circ}\). Finally, in Fig. 4(d), we investigate the response of SiC rods into diamond (from Fig. 3(b)). The resonance emerges at even more significant energies, close to the point that the diffraction orders \(u=-2,+1\) are simultaneously activated and \(\tau _{-1}\) drops more rapidly far from it.

In Fig. 5, we investigate the influence of incident energy *E* sweep on all the reflective and transmissive probabilities for certain designs. Firstly, we consider the layout of Fig. 4(b) supporting substantial \(\rho _{-1}\) and, indeed, the corresponding term gets sharply maximized at \(E\cong 6.5\text{ eV}\). In Fig. 5(a), where the \(\rho _{u}=\rho _{u}(E)\) curves are represented, one can identify the energy thresholds at which each diffraction order *u* gets activated. Moreover, the rapid variation of \(\rho _{0}\) is complementary to that of \(\tau _{0}\) in Fig. 5(b) at low-*E* range, since the configuration is lossless and the matter waves are not channeled towards alternative (except for Snell’s) directions. By inspection of Figs. 5(a) and 5(b), one can understand that the proposed structure can work as a multichannel functional quantum metasurface being able to control incoming and outgoing matter waves in a number of propagation directions simultaneously. In this way, the concept of engineering multichannel reflectors [24] that can control incoming and outgoing waves in a number of propagation directions simultaneously, which has been elaborated and established in Photonics, is translated into quantum arena. In Figs. 5(c) and 5(d), we regard a design with substantial \(\tau _{-1}\) and, once again, the activation of more diffractive orders *u* for increasing *E*, is noticed. Furthermore, highly selective responses are observed for \(\{\rho _{0},\tau _{0}\}\) and at energy levels that new orders are generated, abrupt changes are exhibited. Finally, the maximum in \(\tau _{-1}\) is more wide-band compared to the corresponding one in \(\rho _{-1}\) of Fig. 4(a), which is also understood by comparing Fig. 3(b) with 3(c).

In Fig. 6(a), we examine an optimal layout from the ones reported in Fig. 3(c) (ZnTe cavities hosted by SiC), where the period of the grating is larger (\(b=5\text{ nm}\)). Similarly to Figs. 4(a) and 4(b), the maximum occurs in the middle of the curved rectangle and diminishes rapidly when one moves towards the point of activation of the two higher-order diffraction waves (\(u=+1,-2\)) at \(\theta =\arcsin (1/3)\). The huge decline pace for increasing energy *E* is potentially related to the fact that optimization gives an \(a/b=0.1\) corresponding to an extremum of the considered interval (\(0.1< a/b<0.4\)); the same happens in Fig. 4(b) where \(a/b=0.4\). In order to avoid reporting resonances appearing outside of the regarded parametric box, a refinement to the adopted optimization strategy should be performed as in similar photonic studies [54]. In Fig. 6(b), we observe the variations of reflective probabilities \(\rho _{u}\) for various orders *u* as functions of incoming particles energy *E* for the same design, while in Fig. 6(c), the corresponding transmissive probabilities \(\tau _{u}=\tau _{u}(E)\) are shown. The utility of the proposed configuration as a multi-port quantum network that steers the electron beams with controllable direction and intensity, is once again demonstrated; note also the large values recorded for the transmissive probability \(\tau _{u}\) for the orders with \(u=+1,-2\).

### Performance robustness

As briefly mentioned above, there are several alternative fabrication methods for the setup depicted in Fig. 1, namely growing multiple parallel nanowires into a specific host. Chemical approaches constitute a major construction category containing vapor-liquid-solid growth after injecting precursor gases leading to the nucleated development of cavities from catalytic particles [55] and fast modulation of nanowire composition during bottom-up engraving combined with wet-chemical etching [27]. In addition, a highly-efficient solution-based method for the direct growth of core/shell nanowire arrays on various conductive substrates is implemented [56] suitable for various applications in electrochemical energy storage and optical devices. Epitaxial techniques are also utilized for physical creation of core–multishell structures of radial heterostructure growth for the development of nanowire-based structures [28] or bottom-up syntheses of complex quantum devices with a special focus on nanowire networks with a predefined number of superconducting islands [29]. Furthermore, top-down practices have been applied for realizing diamond cavities in bulk hosts with use of inductively coupled plasma etching [30], while semiconductor processing techniques are implemented to give photonic crystal heterostructures and interfaces, namely the quantum analogue of metasurfaces [57]. Finally, self-assembling design rules are being developed for the generation of complex hierarchical nanostructured systems by exploiting the analogy of nanoparticles with molecules leading to robust and highly reproducible synthesis [58], while micromachined cavities are successfully employed for the construction of superconducting resonators in various quantum layouts [59].

However, all the aforementioned approaches are not flawless and thus the obtained designs contain several size imperfections; either the radius *a* of the rods is not exactly equal to the optimal one or (less frequently) the recommended half-period *b* is not properly respected. In both cases, the duty cycle \(a/b\) is different from that indicated by the optimization process; therefore, it is meaningful to examine the response of the device when the ratio \(a/b\) is perturbed around the proposed value. In Fig. 7, we consider maximally reflecting designs from Fig. 3(a) and show the trajectory on the reflection \((\rho _{0},\rho _{-1})\) and transmission \((\tau _{0},\tau _{-1})\) plane where the horizontal axis corresponds to the Snell’s diffraction and the vertical the anomalous quantity of order \(u=-1\). If further diffraction waves are propagated, they are evaluated by subtracting the values \(\{\rho _{0},\rho _{-1},\tau _{0},\tau _{-1}\}\) from unity indicated by the dashed diagonal lines. In Fig. 7(a), where the reflective channels are examined, one notices the remarkable robustness of the design with InP cavities into BeTe and the sharp change in the performance of BeTe cylinders into diamond; similar trends are recorded in Fig. 7(b), where the transmissivities are represented. As far as the most successful design is concerned (CdO rods in InSb), we observe a remarkable transition from a fully reflective regime (optimal operational point of Fig. 7(a)) to a fully matched one at the point that the red curve touches the dashed line in Fig. 7(b).

In Fig. 8, we show the same quantities as in Fig. 7 but for three maximally transmissive designs appearing in Fig. 3(b). The optimal operational regimes are almost fully transmissive and that is why the markers are located around the origin in Fig. 8(a) and around the upper left corner in Fig. 8(b). Similarly to Fig. 7, we notice the different robustness of the three picked designs and the asymmetry of the curves around the maximal anomalous transmission points; indeed, the response of the structure changes much more reluctantly when \(a/b\) is selected bigger than the recommended compared to the opposite way. It must be finally stressed that every single point on the curves corresponds to a distinct set of probability separations along specific directions of space and thus defines a distinct point of operation of the formed quantum multiport network.

Therefore, we are permitted to say that even when robustness of the design is not substantial, its utility gets not necessarily reduced: as long as the redistribution of probabilities is rigorously computed, any combination of parameters can lead to a useful response profile. In other words, not only the ratio \(a/b\) but even if the angle of incidence *θ* or the particle energy *E* is misselected, can give modules with interesting channel outline serving alternative needs into a quantum circuit. In Fig. 9, we consider the design of Fig. 4(c), namely CdTe cavities in AlN background, and show the spatial distribution of \(|\Psi (x,y)|^{2}\), with help from commercial software. In Fig. 9(a), the energy of the incoming particle is exactly equal to that achieving maximal anomalous refraction and such an effect is fully demonstrated by the abrupt turn of the propagation direction towards the same side that the metasurface is illuminated. In Fig. 9(b), we have selected a different energy for the incoming particle and we obtain multiple (4–5) refractive matter waves with different angles, waist widths and intensities; in this way, the operation of the quantum grating as multiport channel network with rich scattering matrix is shown. These “fringes”, namely the slightly “noisy” pattern of Fig. 9, are attributed to the fact that both the front of the incoming beam and the metasurface extent are finite.

A case of special interest in the normal incidence (\(\theta =0^{\circ}\)), which demands a specific level of energy \(E\gtrsim \frac{1}{2m_{0}}(\hbar \pi /b)^{2}\) for anomalous diffraction (this time both \(u=\pm 1\) orders are activated). In Fig. 10(a), we show the probability distribution \(|\Psi (x,y)|^{2}\) for a normally excited design which achieves an almost perfect splitting of the incoming beam along two symmetric directions corresponding to the two simultaneously (for \(\theta =0^{\circ}\)) generated diffraction orders with \(u=\pm 1\). In this way, the functionality of the regarded layout as wave matter splitter is fully demonstrated. Note that the intensity of the refractive beams is controllable via the texture and the rest of the parameters of the configuration. In Fig. 10(b), we show a scenario of splitting with reduced magnitude controlled by the mechanism of normal reflections \(\rho _{0}\).

## Conclusions

Diffraction of matter waves along various counter-intuitive directions with controllable intensity is an important and general process behind numerous quantum systems. Perhaps the simplest structure that such an anomalous effect may occur is a periodic metasurface comprising cylindrical posts embedded into a background host; thus, in this study its optimal working regimes for various combinations of quantum media are reported. The operation of the structure as a quantum multiport network, where each diffraction order plays the role of a channel of information, is demonstrated at an extensive range of incoming e-beam angles and energies while the effect of the inclusions size on the re-distribution of probabilities is examined.

The presented results are also useful to the interested experimentalist that aims at fabricating steering modules for quantum circuits and signal processors, where the spatial channeling of matter waves is required. In this way, multiple alternative materializations for a fundamental and generic subsystem vital for several quantum engineering applications are provided, ready to respect the availability and feasibility constraints. Interesting expansions of the present work may contain similar concepts already implemented in Electromagnetics like inhomogeneous cylinders [60], rods placed into a different host [61] or wires of unknown texture that can be guessed [62] via external measurements.

## Availability of data and materials

The datasets used and analyzed during the current study are available from the corresponding author upon reasonable request.

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## Acknowledgements

The author is grateful to Prof. Efthimios Kaxiras (Harvard University, Cambridge, MA, USA) for useful discussions regarding the quantum interactions between matter and electron beam.

## Funding

This work was partially supported by Nazarbayev University Faculty Development Competitive Research Grant 021220FD4051 entitled: “Optimal Design of Photonic and Quantum Metamaterials”.

## Author information

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### Contributions

CV as the sole author of the manuscript, conceived, designed and performed the analysis; he also wrote and reviewed the paper. The author read and approved the final manuscript.

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The author declares that they have no competing interests.

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### Cite this article

Valagiannopoulos, C. Anomalous diffraction of matter waves with minimal quantum metasurfaces.
*EPJ Quantum Technol.* **8, **3 (2021). https://doi.org/10.1140/epjqt/s40507-021-00092-0

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DOI: https://doi.org/10.1140/epjqt/s40507-021-00092-0

### Keywords

- Quantum metasurface
- Anomalous diffraction
- Matter waves