Abstract
Emerging photonic functionalities are mostly governed by the fundamental principle of Lorentz reciprocity. Lifting the constraints imposed by this principle could circumvent deleterious effects that limit the performance of photonic systems. Most efforts to date have been limited to waveguide platforms. Here, we propose and experimentally demonstrate a spatiotemporally modulated metasurface capable of complete violation of Lorentz reciprocity by reflecting an incident beam into farfield radiation in forward scattering, but into nearfield surface waves in reverse scattering. These observations are shown both in nonreciprocal beam steering and nonreciprocal focusing. We also demonstrate nonreciprocal behavior of propagativeonly waves in the frequency and momentumdomains, and simultaneously in both. We develop a generalized BlochFloquet theory which offers physical insights into Lorentz nonreciprocity for arbitrary spatial phase gradients, and its predictions are in excellent agreement with experiments. Our work opens exciting opportunities in applications where freespace nonreciprocal wave propagation is desired.
Introduction
The electromagnetic Lorentz reciprocity theorem^{1,2,3,4} states that in a linear, timeindependent system with symmetric constitutive optical tensors, the ratio between received and transmitted fields are the same for forward and timereversed propagation directions. While most electromagnetic and photonic devices operate under this principle, there are circumstances in which reciprocity has undesirable effects, e.g., photovoltaic cells reemitting absorbed solar energy or antennas listening to their own echo. In order to break reciprocity, any of the conditions assumed by the Lorentz theorem must be violated. The use of magnetooptical media breaks timeinversion symmetry and results in an asymmetric scattering matrix, thereby accomplishing optical isolation^{5,6}; however, bulky magnets are required for external bias rendering this conventional approach infeasible for systems integration. Incorporating nonlinear materials and using the electric field selfbiasing effect can also result in optical isolation^{7,8,9}, but the degree of nonreciprocity is powerdependent and typically requires significant interaction lengths. Breakdown of Lorentz reciprocity has also been demonstrated using spatiotemporally modulated waveguides^{10,11,12} and leakywave antennas^{13,14}. The spacetime modulation approach can be particularly attractive when applied in metasurface platforms due to its advantages in reduced size, improved integrability, and attaining surfacewaveassisted nonreciprocal behavior.
The advent of metasurfaces^{15,16,17,18,19,20} has allowed enhanced lightmatter interactions within ultrathin structures, enabling tailored scattering amplitude, phase, and polarization, as well as facilitating the integration of functional materials to accomplish active control^{21,22,23,24,25}. Spatially varying phase profiles in judiciously designed static gradient metasurfaces have provided a powerful means to manipulate the momentum harmonic contents of scattered light, ushering in a novel class of flat optics. In addition, active metasurfaces have been shown to be capable of either switching wavefront profiles whenever needed^{26,27,28}, or modulating in time the amplitude and phase of scattered light^{29,30}. However, a fully tailored electromagnetic response requires metasurfaces that can continuously alter their scattering properties simultaneously in time and space. These functionalities can be achieved in spatiotemporally modulated metasurfaces^{31} (STMMs), which have the potential to revolutionize fundamental and applied photonics, including nonreciprocity^{32,33}, through ondemand control of frequency and momentum harmonic contents of scattered light. For example, an STMM can focus a collimated beam (Fig. 1a), but the timereversed process is not allowed (Fig. 1b). At microwave frequencies, STMMs can be realized with subwavelength metasurface resonators embedded with active elements, such as positiveintrinsicnegative diodes or varactors, which are locally modulated through programmable spacetime voltage biases. This concept has been employed for frequencymultiplexed directional scattering within waveguide systems containing timevarying Huygens’ metadevices^{34}. For freespace waves, spatiotemporally modulated coding microwave metasurfaces^{35,36} have recently been exploited for nonreciprocal beam steering; however, nonreciprocity limited only to the frequencydomain was accomplished. Also, nearinfrared nonlinear Kerr metasurfaces^{37} have recently been reported for breakdown of the Lorentz theorem; the setup is limited to frequencydomain nonreciprocal beam steering achieved via a twobeam Bragg configuration, which is difficult to generalize to arbitrary spatiotemporal modulations. A truly multifunctional STMM that can achieve nonreciprocal propagation of arbitrary wavefronts, and that can even reach photontophoton conversion in forward scattering but photontosurface wave conversion in reverse scattering has not been experimentally demonstrated to date. In this sense, we call this an “extreme” breakdown of Lorentz reciprocity as the very nature of the photonic modes is modified in the scattering process, and would lead to giant optical isolation as no propagative modes are radiated in reverse scattering.
Here, we present a spatiotemporally modulated metasurface reflectarray capable of dynamically imprinting arbitrary wavefronts of freespace electromagnetic waves and demonstrate surfacewaveassisted maximum breakdown of the Lorentz theorem through nonreciprocal mode conversion. We exemplify the flexibility of our STMM platform by achieving dynamical beam steering in forward scattering and, when the forward reflection angle is above a certain threshold, we demonstrate nonreciprocity and complete freespace optical isolation by photontosurface wave conversion in reverse scattering. Even below threshold, using propagativeonly modes we measure nonreciprocal beam steering behavior both in the frequencydomain and momentumdomain, as well as simultaneously in both. In addition, our STMM platform can produce various other kinds of spatial phase distributions, including dynamical focusing. We show nonreciprocal focusing through coexistence of photontosurface wave and photontophoton excitations in reverse scattering, the former conversion processes overwhelming the latter ones. Importantly, the resulting optical isolation is quasioptimal and takes place without the need of surpassing any threshold in forward scattering. To model the experimental results, an analytical generalized BlochFloquet theory valid for arbitrary spatial phase distributions is developed, which successfully predicts various phenomena measured in the photontosurface waves reverse scattering regime. This work can potentially impact emerging technologies benefiting from freespace dynamical wavefront shaping and nonreciprocity, including adaptive optics, Dopplerlike frequency translation, echoimmune antennas, and isolated onchip communications enabled by robust oneway coupling to surface waves.
Results
Experimental design
A conceptual illustration of an STMM is shown in Fig. 1a, b, where each unit cell contains active elements that can be independently modulated to impart an arbitrary twodimensional (2D) phase profile in reflection. In this work, we consider STMMs working at microwave frequencies and varactors as the active elements. Each varactor at position r on the STMM is subjected to a timedependent harmonic voltage modulation \(V\left( {{\boldsymbol{r}},t} \right)\,=\,V_{{\mathrm{op}}} + \Delta _V\,{\mathrm{sin}}[\varphi ({\boldsymbol{r}})  {\mathrm{\Omega }}t]\), where V_{op} is the operating voltage (or offset bias), Δ_{V} is the voltage modulation amplitude, φ(r) is the spatial phase distribution, and Ω is the modulation frequency. The voltage modulation translates into a corresponding modulation of the capacitance \(C_{{\mathrm{var}}}\left( {{\boldsymbol{r}},t} \right)\,=\,C_{{\mathrm{op}}} + \Delta _C\,{\mathrm{sin}}[\varphi ({\boldsymbol{r}})  {\mathrm{\Omega }}t]\) as long as a linear relationship between C_{var} and V holds near V_{op}.
We design and fabricate an STMM on a commercially available double copper clad FR4 substrate (Fig. 1c, d). The resonators incorporate two varactor diodes and two capacitors in order to keep a small form factor of the unit cell while providing the required tunability. For simplicity, we restrict the modulation to one dimension by connecting resonators in each column, resulting in spatial modulation among different columns, i.e., along the xdirection, but invariant among rows, i.e., ydirection (phase delays along this direction can be ignored for Ω ≪ 2πc/L_{y}, where c is the speed of light in vacuum and L_{y} is the lateral size of the STMM along y). Each column is modulated with a desired voltage and phase using a programmable multioutput function generator. Relative phase shifts among channels can be induced by simultaneous triggering of the system, thereby generating arbitrary digitally constructed waveforms (see Methods and Supplementary Fig. 1).
The reflectivity of the unmodulated metasurface is characterized inside an anechoic chamber at a 10° incidence angle as a function of frequency for various static bias voltages uniformly applied to all varactors. Figure 2a shows measurements for ppolarized waves, with the magnetic field component along the ydirection. At the operating voltage V_{op }= 2 V a resonance appears around 6.6 GHz. The optimal working frequency for the modulated STMM, however, is not exclusively determined by the intrinsic resonances of the unmodulated metasurface, but results from an interplay between the unit cell design and the amplitude and phase of the modulation. Indeed, working away from the 6.6 GHz resonance increases the modulation efficiency (see Supplementary Fig. 3c) and thereby the conversion into frequency harmonics (see Supplementary Fig. 4); however, moving too far from the resonance degrades phase dispersion and breaks the linear C_{var} vs. V relationship (see Supplementary Fig. 3d). For our designed STMM and modulation protocol (Δ_{V}= 1 V, Ω = 2π × 50 kHz), we choose our operational frequency as ω_{in} = 2π × 6.9 GHz (λ_{in }= 4.3 cm), which is a good compromise between reflection efficiency, phase dispersion, and linearity.
To test the nonreciprocal functionalities of our spatiotemporally modulated metasurface, we first perform forward scattering measurements by dynamically imprinting appropriate phase delays φ(r) among the STMM columns. When applying a linear phase delay, we measure the steered beam as a function of scanning angle and frequency in the farfield, while for focusing we apply a parabolic phase profile for a selected frequency harmonic and map the resulting spatial distribution of the scattered power. Subsequently, the corresponding reverse scattering measurements are performed by effectively timereversing the output wavefronts of the forward processes, and measuring the farfield scattered power.
Theoretical formulation
We describe the response of the full array of subwavelength resonators with an effective 2D conductivity \(\sigma \left( {{\boldsymbol{r}},\omega ;t} \right) = \sigma _{{\mathrm{op}}}\left( \omega \right) + \Delta \sigma \left( \omega \right){\mathrm{sin}}\left[ {\varphi \left( {\boldsymbol{r}} \right)  {\mathrm{\Omega }}t} \right].\) Here, σ_{op}(ω) is the unmodulated complex conductivity at the operating voltage V_{op} and Δσ(ω) is the complex modulation amplitude. We extract σ_{op}(ω) and estimate Δσ(ω) from reflectivity measurements and standard Fresnel equations for multilayered systems (see Supplementary Fig. 3). When an incident plane wave \({\boldsymbol{E}}_\xi ^{{\mathrm{in}}}\left( {{\boldsymbol{r}},z,t} \right) = E^{{\mathrm{in}}} {\hat{\boldsymbol{e}}}_\xi ^  \left( {{\boldsymbol{k}}_{{\mathrm{in}}}} \right) e^{i({\boldsymbol{r}} \cdot {\boldsymbol{k}}_{{\mathrm{in}}}  z k_{z{\mathrm{v}},{\mathrm{in}}}  \omega _{{\mathrm{in}}}t)}\) with momentum \(({\boldsymbol{k}}_{{\mathrm{in}}},  k_{z{\mathrm{v}},{\mathrm{in}}}{\hat{\mathbf{z}}})\) impinges on the STMM, the reflected field for an arbitrary spatial phase distribution φ(r) on the STMM is given as
Here, \({\hat{\boldsymbol{e}}}_\xi ^ \pm \left( {\boldsymbol{k}} \right)\) are the \(\xi = s,p\) polarization unit vectors with ‘+’ and ‘−’ corresponding to waves propagating in the positive and negative z directions, respectively; \(\omega _n = \omega _{{\mathrm{in}}} + n{\mathrm{\Omega }}\) and k_{n} = k + n∇φ(r) are frequency and momentum harmonics, and \(k_{z{\mathrm{v}},n} = \sqrt {(\omega _n/c)^2  {\boldsymbol{k}}_n^2}\). To compute the reflected field, we develop an analytic BlochFloquet approach based on a local derivative expansion of φ(r), valid for smooth but otherwise general spatial phase distributions. The field amplitude \(\tilde {\cal{E}}_{\xi ,n}\) is a functional of both φ(r) and its gradient ∇φ(r),
Here, \(R_{\xi ,n}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right)\) is the reflection coefficient corresponding to the scattering process \(({\boldsymbol{k}},\omega _{{\mathrm{in}}}) \to \left( {{\boldsymbol{k}}_n,\omega _n} \right)\) at position r, the 2D Fourier transform \({\mathrm{FT}}[e^{i{\mathrm{sg}}(n)\varphi ({\boldsymbol{r}})}]\) is evaluated at \({\boldsymbol{k}}  {\boldsymbol{k}}_{{\mathrm{in}}} + {\mathrm{sg}}(n)\nabla \varphi ({\boldsymbol{r}})\), and \({\mathrm{\Lambda }}_{\xi ,n}\) is defined in the Methods section (see also Supplementary Notes 1–3 for a derivation of the forward scattered fields and the reflection coefficients). Finally, we mention that when the modulation takes place only over a finitesized region of the metasurface, the reflected field is still given by Eq. (1) after the Fourier transform in Eq. (2) is replaced by \({\mathrm{FT}}[ {\tilde \theta \left( {\boldsymbol{r}} \right)e^{i{\mathrm{sg}}\left( n \right)\varphi \left( {\boldsymbol{r}} \right)}} ]\), where \(\tilde \theta \left( {\boldsymbol{r}} \right) = 1\) if r belongs to the modulated region and is zero otherwise (see Supplementary Note 4 for the generalization of our theory to finitesized STMMs).
Dynamical wavefront shaping
In the simplest case of a linear phase distribution \(\varphi ^{{\mathrm{steer}}}\left( {\boldsymbol{r}} \right) = {\mathbf{\upbeta }} \cdot {\boldsymbol{r}}\) required for beam steering, the amplitude is \(\tilde {\cal{E}}_{\xi ,n}^{{\mathrm{steer}}} = \left( {2\pi } \right)^2R_{\xi ,n}^{{\mathrm{steer}}}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};0} \right)\delta \left( {{\boldsymbol{k}}  {\boldsymbol{k}}_{{\mathrm{in}}}} \right)\). In this case the derivative expansion is exact, and the reflected field is given by a single sum over discrete frequency and momentum harmonics for the scattering processes \(({\boldsymbol{k}}_{{\mathrm{in}}},\omega _{{\mathrm{in}}}) \to ({\boldsymbol{k}}_{{\mathrm{in}}} + n{\mathbf{\upbeta }},\omega _{{\mathrm{in}}} + n{\mathrm{\Omega }})\). The azimuthal and polar steering angles are, respectively, given by \(\cos \phi _n = {\boldsymbol{k}}_{{\mathrm{in}}} \cdot ({\boldsymbol{k}}_{{\mathrm{in}}} + n{\mathbf{\upbeta }})/\left[ {\left {{\boldsymbol{k}}_{{\mathrm{in}}}} \right\left {{\boldsymbol{k}}_{{\mathrm{in}}} + n{\mathbf{\upbeta }}} \right} \right]\) and \(\sin \theta _n = \left {{\boldsymbol{k}}_{{\mathrm{in}}} + n{\mathbf{\upbeta }}} \rightc/\omega _n.\) For large enough momentum “kicks” nβ, \(\sin \theta _n\) can become larger than 1 (\(k_{z{\mathrm{v}},n}\) purely imaginary) resulting in surface waves, which we later utilize to achieve photontosurface waves conversion in reverse scattering. We first demonstrate the multifunctional beam manipulation capability of our STMM by imprinting arbitrary beam steering phase distributions (Fig. 2b). We vary the phase gradient β along the xdirection and show beam steering of the +1 harmonic from +40° to −40°. We observe high quality beam steering with low sidebands and consistent amplitude for a wide range of angles.
To test the flexibility of our STMM for imprinting arbitrary reflection phases, we demonstrate dynamical focusing, a functionality that is relevant, e.g., in compact satellite technologies. The required phase distribution to focus a specific frequency harmonic \(\bar n\, \ne\, 0\) at an arbitrary focal point R_{f} = (x_{f}, y_{f}, z_{f}) is
All other harmonics \(n \,\ne\, \bar n\) do not result in perfect focusing, and the case n = 0 always undergoes specular reflection in STMMs. In contrast to the steering case, the momentum kicks \(n\nabla \varphi _{\bar n}^{{\mathrm{focus}}}\) vary as a function of position and the amplitude \(\tilde {\cal{E}}_{\xi ,n}^{{\mathrm{focus}}}\) is not proportional to a delta function. These properties hold for any nonlinear phase distribution φ_{NL}(r). Importantly, the phase of the reflected field in Eq. (1) arises from an intricate interplay among the phases of each planewave component in the momentum integral. Only for the \(n = \bar n\) frequency harmonic does the resulting reflection phase turn out to be precisely given by the focusing distribution Eq. (3) (see Supplementary Note 3 for a discussion of the phase of the total reflection coefficient for the different harmonics). Using our theoretical approach, we first model an infinitesized STMM subjected to our focusing modulation protocol, that produces a 1D focal line along the ydirection, and compute the field distribution for the \(n = \bar n = + 1\) harmonic (Fig. 2c).
In Fig. 2d, f we show the experimental results demonstrating the dynamical focusing capability of our STMM (see Methods). Unlike beam steering, which is largely aperture agnostic, focusing requires consideration of the metasurface’s overall dimensions. With a surface in the electric field direction measuring L_{x} = 19 cm (≈ 4.4 λ_{in}), a short focal length is necessary for measurable gain, otherwise weak focusing effects are indistinguishable from the usual plane wave like character of the harmonics. For the onaxis focusing case, it is apparent that focusing has been achieved by examination of the increased power and rapid falloff of the signal. At distances \(\ell < 12\,{\mathrm{cm}}\) (measured from the STMM center along the focal axis) we observe interference due to nearfield coupling between the scanning monopole and the STMM, evident in Fig. 2d. For the offaxis experiment, we measure a much tighter focus due to minimized interference and shadowing effects. To evaluate the quality of the focusing we estimate the gain along the focal axis. We define gain as the ratio between the power of the focused beam at frequency ω_{+1} and that of a beam steered at the same frequency ω_{+1} into the direction of the focal axis. Figure 2e compares the experimental gain for the offaxis case with the theoretical predictions using the extension of our theory approach to finitesized STMMs. The experimental data and the theory display the same shape along the focal axis, showing strong agreement. For x_{f} = 6 cm and z_{f} = 15 cm, the expected focal length is \(\ell _f = 16\,{\mathrm{cm}}\). However, due to the finite size of our metasurface, the gain peaks around \(\ell = 13\,{\mathrm{cm}}\), both in experiment and theory (Fig. 2e). At this point, theory predicts a gain of 5.24 dB while the measured value is (5.8 ± 0.6) dB.
Breakdown of Lorentz reciprocity via nearfield surfacewaves
We turn our attention to nonreciprocal excitation of surface waves both in beam steering and focusing. In Fig. 3a we report the n = +1 beam steered to \(\theta _{ + 1} \approx + 18^\circ\) (β_{x} = 44 m^{−1}) from a normally incident plane wave (k_{in }= 0). In the reverse experiment we send the timereversed n = +1 beam (−β, ω_{in }+ Ω) onto the STMM (see Methods). A frequency downconversion and a momentum upconversion must take place in order for the scattering process to be reciprocal. However, this is not permitted due to the travelingwave nature of the modulation. There exist three dominant reverse reflection pathways: (i) a frequency downconversion leading to (−β, ω_{in }+ Ω) → (−2β, ω_{in}), clearly breaking reciprocity in the momentumdomain. The measured reverse reflection is shown in Fig. 3b, with a reflection angle ≈ −36° (in contrast to the 0° reciprocal case) in excellent agreement with the theory prediction of −37.5°; (ii) a frequency upconversion (−β, ω_{in }+ Ω) → (0, ω_{in }+ 2Ω), resulting in nonreciprocity in the frequencydomain (Fig. 3c); and iii) a specular process (−β, ω_{in}+Ω) → (−β, ω_{in }+ Ω), violating reciprocity both in the frequencydomain and momentumdomain (Fig. 3d), with measured reflection angle ≈ −18°. Finally, we mention that the input wave (k_{in}, ω_{in}) can also undergo frequencyconserving specular reflection in the forward experiment, and that in general the backwards specularly reflected field (−k_{in}, ω_{in}) satisfies reciprocity. However, under a specific set of parameters it is still possible to attain nonreciprocity in amplitude (not shown). When the magnitude of the phase gradient surpasses a certain threshold (\(\left {\mathbf{\upbeta }} \right > \omega _{{\mathrm{in}}}/2c = 72.31\,{\mathrm{m}}^{  1}\) for k_{in }= 0, corresponding to a forward reflection angle of +30°), the reverse scattered beam at frequency ω_{in} does not reflect off the STMM at all. Instead, surface waves are launched on the metasurface as \(k_{z{\mathrm{v}},  1}^{{\mathrm{REV}},{\mathrm{steer}}} = i\left[ {4{\mathbf{\upbeta }}^2  (\omega _{{\mathrm{in}}}/c)^2} \right]^{1/2}\) is purely imaginary, resulting in photontosurface wave conversion, i.e., complete freespace optical isolation. In Fig. 3e, g we present nonreciprocity measurements for β_{x} = 96 m^{−1} (\(\theta _{ + 1} \approx + 43^\circ\)), and in Fig. 3f, h the corresponding theory calculations. By scattering an incident beam into farfield collimated radiation in the forward process but into nearfield evanescent modes in the reverse case, we demonstrate extreme breakdown of Lorentz reciprocity.
We now report optical isolation in dynamical focusing. In the forward process a plane wave (0, ω_{in}) can focus at frequency ω_{+1} using the \(\varphi _{\bar n = + 1}^{{\mathrm{focus}}}\left( {0,\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right)\) phase profile. Figure 4a shows the measured power profile of the forward reflected offaxis focused beam as a function of \(\ell\) and the angle α between the surface normal and the detector. We investigate the scattered field at ω_{in} after the focused beam at ω_{+1} is timereversed in order to probe nonreciprocity in the momentumdomain. To grasp some physical insight, we show in Fig. 4b a snapshot of the electric field distribution for the particular scattering process \((  \nabla \varphi _{\bar n = + 1}^{{\mathrm{focus}}},\omega _{{\mathrm{in}}} + {\mathrm{\Omega }}) \to (  2\nabla \varphi _{\bar n = + 1}^{{\mathrm{focus}}},\omega _{{\mathrm{in}}})\) for the infinitesized STMM, similarly to what is done above for nonreciprocal beam steering (see Methods). Also shown is the corresponding timeaveraged Poynting vector. The reverse scattered field does not collimate back into the direction of the original input beam, but instead shows a “ribbonlike” region (centered at x_{f} and of width \(2z_f/\sqrt 3\) for the chosen process) containing propagative modes (\(k_{z{\mathrm{v}},  1}^{{\mathrm{REV}},{\mathrm{focus}}} = \left[ {(\omega _{{\mathrm{in}}}/c)^2  4\nabla \varphi _{\bar n = + 1}^{{\mathrm{focus}}}^2} \right]^{1/2}\) is real) that radiate away from the metasurface, and is flanked by a region of surface waves with purely imaginary \(k_{z{\mathrm{v}},  1}^{{\mathrm{REV}},{\mathrm{focus}}}\) (these latter modes move along the STMM and weakly manifest in Fig. 4b due to their strong decay). Other choices of scattering processes also present the same nonreciprocal characteristics. The total reverse scattered field is the sum of all those possible scattering processes and results in maximum breakdown of Lorentz reciprocity (see Supplementary Notes 5 and 6 for further details of Lorentz nonreciprocity for infinitesized STMM with arbitrary nonlinear spatial phase distributions, including focusing).
For a finitesized STMM our calculations indicate that a similar physics takes place, the most important difference being that the propagative modes are asymmetrically radiated from the STMM for the offaxis focusing configuration (see Methods and Supplementary Note 7 for a discussion of the Poynting vector in reverse scattering). In Fig. 4c, d we experimentally validate these theoretical predictions by exciting the metasurface with a monopole antenna located at the focal point and emitting at frequency ω_{+1}, and detect the farfield scattered radiation from the STMM at frequency ω_{in}. The measured power map bears little resemblance to the original input plane wave. It shows a concave wedgeshaped region with low radiated power at the center, two peaks at asymmetric angular locations, and an outer region of negligible radiated power (displaying similarities to the Poynting vector depicted in Fig. 4b). All these properties of the reverse scattered field are in stark contrast to the input Gaussian profile for the forward process and in excellent agreement with the theory calculations for finitesized STMMs. In particular, the differences in the measured angular positions of the peaks and in their strengths are due to the inherent asymmetry of offaxis focusing in finitesized STMMs (see Supplementary Note 7 for a discussion of photontohybrid modes (surface waves and photons) conversion in reverse scattering for finitesized STMMs for focusing). For positive scanning angles, there is a main peak located at \(\alpha _ + ^{{\mathrm{exp}}} = \left( { + 54 \pm 1} \right)^\circ\), while for negative scanning angles there is a much weaker peak at \(\alpha _  ^{{\mathrm{exp}}} = (  26 \pm 1)^\circ\).
An extensive discussion of how the STMM emits radiation in reverse scattering can be found in the Supplementary Note 7, where we consider the analytical aspects for the radiative power spectrum in reverse scattering for the focusing functionality. Here, we briefly describe the main results. The structures observed in Fig. 4c, d result from the superposition of emitted radiation from every point on the metasurface. For example, the rightedge at x = L_{x}/2 emits radiation mainly in the direction shown in Fig. 4c with a predicted angle \(\alpha _{\mathrm{R}}^{{\mathrm{th}}} = + 53.27^\circ\), in very close agreement with the measurement. Points on the metasurface between x_{f} and L_{x}/2 also contribute to that same peak, resulting in the observed broadening. The second peak seen on the right side of Fig. 4c at a measured position \(\alpha _{{\mathrm{ER}}2}^{{\mathrm{exp}}} = ( + 36 \pm 1)^\circ\) arises from secondary emissions from points in the range [x_{f}, L_{x}/2] on the STMM. For example, the rightedge of the structure has a secondary emission direction forming a predicted angle \(\alpha _{{\mathrm{ER}}2}^{{\mathrm{th}}} = + 34.66^{\mathrm{o}}\), again in very close agreement with observations. On the other hand, the leftedge of the STMM at x = −L_{x}/2 emits radiation mainly in the direction shown in Fig. 4c with a predicted angle \(\alpha _{\mathrm{L}}^{{\mathrm{th}}} =  20.36^\circ\), which is slightly off from the measured position of the peak on the left side of Fig. 4c. The reason for this discrepancy is that all points between −L_{x}/2 and x_{f} contribute to the peak and its broadening, and there is a given point on the metasurface in the [−L_{x}/2, x_{f}] range that emits precisely in the direction of the peak. Also, in the Supplementary Note 7 we depict the structure of the Poynting vector in reverse scattering, showing a complex coexistence of propagative and evanescent features. In contrast to nonreciprocal beam steering, there is no threshold to launch surface waves in nonreciprocal focusing and evanescent modes overwhelm propagative ones. Just as in nonreciprocal steering, this represents a large violation of the Lorentz reciprocity theorem since in forward scattering there is a photontophoton conversion but in reverse scattering there is a photontophoton/surface wave hybrid conversion. The measurements reported in Fig. 4c, d constitute the first experimental demonstration of extreme nonreciprocal focusing functionality using STMMs.
In contrast to the case of STMMs modulated with a linear phase φ_{L}(r) = β · r, for which surface waves in reverse scattering are launched only when its gradient surpasses a certain threshold, no such constraint exists on any nonlinear phase φ_{NL}(r) dynamically imprinted on the metasurface. In this sense, extreme breakdown of Lorentz reciprocity and giant optical isolation are robust properties occurring in spacetime metasurfaces under arbitrary nonlinear spatial modulations (see Supplementary Note 8 for a discussion of nonreciprocity in arbitrary nonlinear phase distributions).
Discussion
In summary, we have introduced an STMM platform for complete violation of Lorentz reciprocity by photontophoton conversion in forward scattering, but photontosurface wave conversion in reverse scattering. This represents an extreme breakdown of Lorentz reciprocity as the very nature of the photonic modes is modified in the scattering process, leading to giant optical isolation as no propagative modes are radiated in reverse scattering. We also showed that our STMM allows beamsteering nonreciprocity in the frequencydomain, momentumdomain, and simultaneously in both. Our approach enables dynamical arbitrary wavefront shaping by offering substantial flexibility in the manipulation of frequencymomentum harmonic contents of freespace electromagnetic waves when compared to standard phasegradient and nonlinear optical systems. We have also developed an analytical method to model STMMs with arbitrary spatial phase distributions and its predictions are in excellent agreement with experiment, shedding light on the underlying physics of STMMs with complex phase distributions without resorting to fullwave numerical simulations.
Our goal in this paper is to demonstrate complete breakdown of Lorentz reciprocity via modeconversion, in the sense explained above. As such, we did not attempt to optimize our structure to achieve either large reflectivity or high efficiency for harmonics conversion. As is clear from Figs. 2 and 3, most of the impinging power gets absorbed by the structure, the reflectivity of the fundamental harmonic is about 4%, and the conversion efficiency into the n = +1 harmonic is ~ 0.1%. All these features are a direct consequence of the need to achieve a broad phase dispersion in our designed STMM, which forces us to work close to the nearzero reflection dip (Fig. 2a). Despite the low reflectivity and conversion efficiencies in the forward processes, our nonreciprocal beam steering experiment shows that, beyond a certain threshold, the timereversed propagative output signal in forward scattering gets completely transformed into evanescent surface waves on the STMM in reverse scattering, thereby achieving extreme nonreciprocity in the direction of propagation and changing the very nature of the photonic modes involved. Similarly, our nonreciprocal focusing measurements show a complete violation of the Lorentz theorem. Tailored metasurfaces with high reflectivity while maintaining a broad phase dispersion can be designed and fabricated for practical applications, as the ones discussed below. However, this by itself does not solve the challenge of substantially enhancing conversion efficiencies into upconverted or downconverted frequency harmonics, as most of the reflected power will still reside in the fundamental harmonic. These limitations can be addressed by using nonharmonic asymmetric timemodulation protocols and higher modulation frequencies, opening opportunities for efficiency improvement, momentumfrequency harmonic mode selectivity, and advanced wavefront manipulation. Using these more general modulation protocols one can in principle attain conversion efficiencies larger than 80%, provided that the complex modulations can be implemented by the electronic controller.
Maximum breakdown of Lorentz reciprocity can occur for any kind of linear or nonlinear spatial phase distributions dynamically imprinted on the metasurface, highlighting that extreme nonreciprocity is a generic property of STMMs. Furthermore, by independently addressing each individual resonator, our platform can be extended to achieve fully threedimensional dynamical wavefront shaping. STMMs based on our proofofconcept demonstration with improved designs and complex timemodulation protocols will enable a new architecture for compact and flat multifunctional optical components with builtin isolators, reducing stringent size, weight, and power requirements for wireless communications and remote sensing. In addition, such a spatiotemporally modulated platform can be used to compensate for Doppler shifts induced by relative motion in intersatellite and Earthtosatellite communications. Extension of STMMs to the THz and IR frequency range is possible by use of alternative materials and active elements, including backgate modulated graphenebased resonators, and electrooptic and photoacoustic media. Finally, our demonstration of maximum violation of Lorentz reciprocity for arbitrary wavefronts supports emerging technologies benefiting from freespace optical isolation, such as nonreciprocal wireless information transmission.
Methods
Device fabrication
The metasurface of dimensions L_{x} = L_{y} = 19 cm was fabricated using 12″ × 12″ double sided FR4 circuit boards, with a thickness h = 1.6 mm and 1 oz copper. The top side of the board was milled yielding an array of unit cells on one side, and a continuous ground plane separated by the FR4 spacer. After milling, the varactors (SMV1405) and capacitors (SMD 0.6 pF) were added by reflow soldering and electrical connections were made to the columns for external control. The voltage signals being fed into each column of the STMM were sourced from a highdensity signal generator that is installed on a National Instruments PCI eXtensions for Instrumentation (PXIe) chassis. Each waveform was digitally constructed and uploaded to the onboard buffer of the control system. Both the PXIe chassis and the signal generators have synchronized sample clocks, thus preventing relative phase drift in time and enabling the triggering of all channels to within 10 ns. See Supplementary Fig. 1a for a photograph of the fabricated sample with control lines.
Measurements
The fabricated metasurface was characterized inside an anechoic chamber using a broadband horn antenna (SAS571) and a quarter wave monopole antenna (see Supplementary Fig. 1b, d for a schematic of the experimental setups for dynamical steering and focusing, and Supplementary Fig. 1c, e for nonreciprocal steering and focusing). A vector network analyzer (VNAAgilent N5230A) was used for data collection. First, the reflectivity of the unmodulated metasurface was measured at a 10° incidence angle with ppolarized light with all varactors uniformly biased (Supplementary Fig. 2). These measurements were carried out with broadband antennas as the source and receiver, and the VNA was used for a conventional S21 measurement with the source and receiver swept across the band of interest (5.5–8 GHz). We then characterized the spatiotemporally modulated metasurface. For these measurements the source (6.3 mW input power) is in continuous wave (CW) operation at 6.9 GHz with a 100 Hz resolution, and the detector was swept in frequency with corresponding 100 Hz resolution to measure the generated frequency harmonics. For beam steering measurements both the source and the detector were broadband horn antennas; however, for the focusing experiments a monopole antenna was used instead of one of the horn antennas. In the forward experiments the source (CW at ω_{in}) was placed onaxis with the metasurface normal \((x = 0,y = 0,z = 1.3)\) m, and the receiver was placed on a computercontrolled gimbal which scanned the reflected power in the x−z plane. In the beam steering case this yielded radiation patterns of the harmonics scanned along a constant radius (Supplementary Fig. 1b); for focusing experiments a large portion of the x−z plane was scanned yielding a 2D map of forward radiated power in the harmonics (Supplementary Fig. 1d). For the reverse nonreciprocity experiments the detector and source are swapped, and the new source operates in continuous wave at ω_{+1} (Supplementary Fig. 1c, e). The detector measures a frequency sweep as explained above, centered this time at ω_{in}, capturing harmonics generated around this frequency. The receiver is again scanned in angle as in the forward experiment to measure reflected power over the area of interest.
Theory
The reflected field by the STMM is described by means of a generalized BlochFloquet approach based on a derivative expansion of the spatial phase distributions. It is given by Eq. (1), where \(\tilde {\cal{E}}_{\xi ,n}\) is defined in Eq. (2) with \({\mathrm{\Lambda }}_{\xi ,n} = [ {R_{\xi ,n  {\mathrm{sg}}\left( n \right)}\left( {{\boldsymbol{k}}_{{\mathrm{in}}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right) \pm \delta _{\left n \right,1}} ]/[R_{\xi ,n  {\mathrm{sg}}\left( n \right)}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right) \pm \delta _{\left n \right,1}]\). Here, the ‘+’ and ‘−’ signs correspond to ξ = s and ξ = p polarizations, respectively. The reflection coefficients \(R_{\xi ,n}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right)\) are obtained by using the local derivative expansion in Maxwell equations and solving numerically (or via continued fractions) an infinite set of coupled equations \(\eta _{\xi ,n  1}^ + {\cal{R}}_{\xi ,n  1} + A_{\xi ,n}{\cal{R}}_{\xi ,n} + \eta _{\xi ,n + 1}^  {\cal{R}}_{\xi ,n + 1} = 2B_{\xi ,n}\delta _{n,0}.\) For ppolarization, \({\cal{R}}_{p,n}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right) = R_{p,n}\left( {{\boldsymbol{k}},\omega _{{\mathrm{in}}};{\boldsymbol{r}}} \right)  \delta _{n,0}\), \(\eta _{p,n}^ \pm = \mp i(Z_{\mathrm{s}}/2)(k_{z{\mathrm{v}},n}/k_{{\mathrm{v}},n})\Delta \sigma \left( {\omega _n} \right)e^{ \pm i[\varphi \left( {\boldsymbol{r}} \right)  {\boldsymbol{r}} \cdot \nabla \varphi \left( {\boldsymbol{r}} \right)]}\), \(A_{p,n} = Z_{\mathrm{s}}\sigma _{{\mathrm{op}}}\left( {\omega _n} \right)(k_{z{\mathrm{v}},n}/k_{{\mathrm{v}},n}) + i(k_{z{\mathrm{v}},n}k_{{\mathrm{s}},n}/k_{{\mathrm{v}},n}k_{z{\mathrm{s}},n})\cot ( {hk_{z{\mathrm{s}},n}} ) + Z_{\mathrm{s}}/Z_{\mathrm{v}},\) and \(B_{p,n} =  Z_{\mathrm{s}}/Z_{\mathrm{v}}\). In these expressions, Z_{s} is the spacer impedance, h is the thickness of the spacer, \(k_{{\mathrm{v}},n} = \omega _n/c\) and \(k_{z{\mathrm{v}},n} = \sqrt {k_{{\mathrm{v}},n}^2  {\boldsymbol{k}}_n^2}\) are the magnitudes of the wavevector and its zcomponent in vacuum for the nth harmonic, and similarly \(k_{{\mathrm{s}},n} = k_{{\mathrm{v}},n}/Z_{\mathrm{s}}\) and \(k_{z{\mathrm{s}},n} = \sqrt {k_{{\mathrm{s}},n}^2  {\boldsymbol{k}}_n^2}\) are the corresponding quantities in the spacer. The reverse scattered field is given by a double summation over incoming and outgoing frequency harmonics, and a double integral over the respective incoming and outgoing planewave components: \({\boldsymbol{E}}_\xi ^{{\mathrm{scatt}},{\mathrm{REV}}}\left( {{\boldsymbol{r}},z,t} \right) = E^{{\mathrm{in}}}{\sum}_{n^{\prime} ,n =  \infty }^\infty {{\int} {d^2} } {\boldsymbol{k}}\prime {\int} {d^2} {\boldsymbol{k}}\left( {2\pi } \right)^{  4}\left[ {{\hat{\boldsymbol{e}}}_\xi ^ + \left( {{\boldsymbol{k}}_{n\prime }^\prime } \right) \odot {\hat{\boldsymbol{e}}}_\xi ^  \left( {  {\boldsymbol{k}}_n} \right)} \right] \times \) \(\tilde {\cal{E}}_{\xi ,n\prime }[  {\boldsymbol{k}}_n,{\boldsymbol{k}}_{n\prime }^\prime ,\omega _{n + n\prime };{\boldsymbol{r}}]\tilde {\cal{E}}_{\xi ,n}[{\boldsymbol{k}}_{{\mathrm{in}}},{\boldsymbol{k}}_n,\omega _n;{\boldsymbol{r}}]e^{i[{\boldsymbol{r}} \cdot {\boldsymbol{k}}_{n\prime }^\prime + zk_{z{\mathrm{v}},n\prime }^\prime  \omega _{n + n\prime }t]}\) (the ⊙ product gives a vector whose components are the product of the Cartesian components of the two polarization unit vectors). For our nonreciprocal beam steering and focusing experiments of Fig. 3b, g and Fig. 4c, d, only the n = +1 and n′ = −1 terms should be considered, rendering the output frequency equal to ω_{in}. For Fig. 3c, n = n′ = +1, and for Fig. 3d, n = +1 and n′ = 0. The calculated scanning angles \(\alpha _{{\mathrm{R}},{\mathrm{L}}}^{{\mathrm{th}}} = {\mathrm{arcos}}\left\{ {\frac{{  \left( {L_x/2d} \right){\mathrm{tan}}\left( {g_ \pm ^{{\mathrm{th}}}} \right) + \sqrt {{\mathrm{tan}}^2\left( {g_ \pm ^{{\mathrm{th}}}} \right) + \left[ {1  \left( {L_x/2d} \right)^2} \right]{\mathrm{tan}}^4\left( {g_ \pm ^{{\mathrm{th}}}} \right)} }}{{1 + {\mathrm{tan}}^2\left( {g_ \pm ^{{\mathrm{th}}}} \right)}}} \right\}\) in Fig. 4c are the angles formed between STMM vertical and the crossings of the main directions of emission from the right and left edges of the STMM with the measurement arc. Here, the “+” (“−”) sign corresponds to \(\alpha _{\mathrm{R}}^{{\mathrm{th}}}\) \(\left( {\alpha _{\mathrm{L}}^{{\mathrm{th}}}} \right)\), \(g_ \pm ^{{\mathrm{th}}} = {\mathrm{arccos}}[1 \pm (\omega _{{\mathrm{in}}}/c)^{  1}(d/dx)\varphi _{\bar n = + 1}^{{\mathrm{focus}}}(\!\pm L_x/2)],\) L_{x} is the size of the STMM along the xdirection, and d is the distance between the detector and the center of the STMM.
Data availability
The data that support the plots within this paper and other findings of this study are available from the corresponding authors upon reasonable request.
Code availability
The codes are available from the corresponding authors upon reasonable request.
References
Lorentz, H. A. The theorem of Poynting concerning the energy in the electromagnetic field and two general propositions concerning the propagation of light. Versl. K. Akad. W. Amsterdam 4, 1–11 (1896).
Potton, R. J. Reciprocity in optics. Rep. Prog. Phys. 67, 717–754 (2004).
Sounas, D. L. & Alù, A. Nonreciprocal photonics based on time modulation. Nat. Photonics 1, 774–783 (2017).
Caloz, C. et al. Electromagnetic nonreciprocity. Phys. Rev. Appl. 10, 047001 (2018).
Tamagnone, M. et al. Near optimal graphene terahertz nonreciprocal isolator. Nat. Commun. 7, 11216 (2016).
Lin, S., Silva, S., Zhou, J. & Talbayev, D. A oneway mirror: highperformance terahertz optical isolator based on magnetoplasmonics. Adv. Opt. Mater. 6, 1800572 (2018).
Mahmoud, A. M., Davoyan, A. R. & Engheta, N. Allpassive nonreciprocal metastructure. Nat. Commun. 6, 8359 (2015).
Shi, Y., Yu, Z. & Fan, S. Limitations of nonlinear optical isolators due to dynamic reciprocity. Nat. Photonics 9, 388–392 (2015).
Lawrence, M., Barton, D. R. III & Dionne, J. A. Nonreciprocal flat optics with silicon metasurfaces. Nano Lett. 18, 1104–1109 (2018).
Yu, Z. & Fan, S. Complete optical isolation created by indirect interband photonic transitions. Nat. Photonics 3, 91–94 (2009).
Lira, H., Yu, Z., Fan, S. & Lipson, M. Electrically driven nonreciprocity induced by interband photonic transition on a silicon chip. Phys. Rev. Lett. 109, 033901 (2012).
Sounas, D. L., Caloz, C. & Alù, A. Giant nonreciprocity at the subwavelength scale using angular momentumbiased metamaterials. Nat. Commun. 4, 2407 (2013).
Hadad, Y., Soric, J. C. & Alù, A. Breaking temporal symmetries for emission and absorption. Proc. Natl Acad. Sci. 113, 3471–3475 (2016).
Taravati, S. & Caloz, C. Mixerduplexer antenna leakywave system based on periodic spacetime modulation. IEEE Trans. Antennas Propag. 65, 442–452 (2017).
Yu, N. F. et al. Light propagation with phase discontinuities: generalized laws of reflection and refraction. Science 334, 333–337 (2011).
Grady, N. K. et al. Terahertz metamaterials for linear polarization conversion and anomalous refraction. Science 340, 1304–1307 (2013).
Lin, D., Fan, P., Hasman, E. & Brongersma, M. L. Dielectric gradient metasurface optical elements. Science 345, 298–302 (2014).
Arbabi, A., Horie, Y., Bagheri, M. & Faraon, A. Dielectric metasurfaces for complete control of phase and polarization with subwavelength spatial resolution and high transmission. Nat. Nanotechnol. 10, 937–943 (2015).
Kildishev, A. V., Boltasseva, A. & Shalaev, V. M. Planar photonics with metasurfaces. Science 339, 1232009 (2013).
Chen, H. T., Taylor, A. J. & Yu, N. A review of metasurfaces: physics and applications. Rep. Prog. Phys. 79, 076401 (2016).
Chen, H.T. et al. Active terahertz metamaterial devices. Nature 444, 597–600 (2006).
Driscoll, T. et al. Memory metamaterials. Science 325, 1518–1521 (2009).
Hess, O. et al. Active nanoplasmonic metamaterials. Nat. Mater. 11, 573–584 (2012).
Lee, S. H. et al. Switching terahertz waves with gatecontrolled active graphene metamaterials. Nat. Mater. 11, 936–941 (2012).
Sleasman, T., Mohammadreza, F. I., Gollub, J. N. & Smith, D. R. Microwave imaging using a disordered cavity with a dynamically tunable impedance surface. Phys. Rev. Appl. 6, 054019 (2016).
Cui, T. J., Qi, M. Q., Wan, X., Zhao, J. & Cheng, Q. Coding metamaterials, digital metamaterials and programmable metamaterials. Light Sci. Appl. 3, e218 (2014).
Li, L. et al. Electromagnetic reprogrammable codingmetasurface holograms. Nat. Commun. 8, 197 (2017).
Wu., P. C. et al. Dynamic beam steering with alldielectric electrooptic IIIV multiplequantumwell metasurfaces. Nat. Commun. 10, 3654 (2019).
Chen, H. T. et al. A metamaterial solidstate terahertz phase modulator. Nat. Photonics 3, 148 (2009).
Zeng, B. et al. Hybrid graphene metasurfaces for highspeed midinfrared light modulation and singlepixel imaging. Light Sci. Appl. 7, 51 (2018).
Shaltout, A. M., Shalaev, V. M. & Brongersma, M. L. Spatiotemporal light control with active metasurfaces. Science 364, 648 (2019).
Hadad, Y., Sounas, D. L. & Alù, A. Spacetime gradient metasurfaces. Phys. Rev. B 92, 100304 (2015).
Zang, J. W. et al. Nonreciprocal wavefront engineering with timemodulated gradient metasurfaces. Phys. Rev. Appl. 11, 054054 (2019).
Liu, M., Powell, D. A., Zarate, Y. & Shadrivov, I. V. Huygens’ metadevices for parametric waves. Phys. Rev. X 8, 031077 (2018).
Zhang, L. et al. Spacetimecoding digital metasurfaces. Nat. Commun. 9, 4334 (2018).
Zhang, L. et al. Breaking reciprocity with space‐time‐coding digital metasurfaces. Adv. Mater. 31, 1904069 (2019).
Guo, X., Ding, Y., Duan, Y. & Ni, X. Nonreciprocal metasurface with spacetime phase modulation. Light Sci. Appl. 8, 123 (2019).
Acknowledgements
We are grateful to the ISR FabLab at LANL for mounting the varactors on the metasurface. D.D. thanks Lukasz Cincio for computational assistance. Research presented in this paper was supported by the Laboratory Directed Research and Development program of Los Alamos National Laboratory under project number 20180062DR. Part of this work was performed at the Center for Integrated Nanotechnologies, a U.S. Department of Energy, Office of Basic Energy Sciences user facility. LANL is operated by Triad National Security, LLC, for the National Nuclear Security Administration of the U.S. Department of Energy (Contract No. 89233218CNA000001).
Author information
Authors and Affiliations
Contributions
A.A., H.T.C., D.D. and W.K.K. conceived the idea of this work. A.A. and A.C. designed the experiments. A.C. and S.S. fabricated samples and performed the measurements. S.V. designed the electronic control system. D.D. and W.K.K. developed the theory and conducted numerical simulations. A.A., A.C., H.T.C., D.D., W.K.K., W.P., A.S. and A.T. contributed to the writing of the paper. A.A. and D.D. supervised the entire study.
Corresponding authors
Ethics declarations
Competing interests
The authors declare no competing interests.
Additional information
Peer review information Nature Communications thanks the anonymous reviewer(s) for their contribution to the peer review of this work.
Publisher’s note Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Supplementary information
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Cardin, A.E., Silva, S.R., Vardeny, S.R. et al. Surfacewaveassisted nonreciprocity in spatiotemporally modulated metasurfaces. Nat Commun 11, 1469 (2020). https://doi.org/10.1038/s41467020152731
Received:
Accepted:
Published:
DOI: https://doi.org/10.1038/s41467020152731
This article is cited by

A selfbiased nonreciprocal magnetic metasurface for bidirectional phase modulation
Nature Electronics (2023)

Intelligent metasurfaces: control, communication and computing
eLight (2022)

Sidebandfree space–timecoding metasurface antennas
Nature Electronics (2022)

Fullduplex reflective beamsteering metasurface featuring magnetless nonreciprocal amplification
Nature Communications (2021)

Frequency selective wave beaming in nonreciprocal acoustic phased arrays
Scientific Reports (2020)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.