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# Ultra-high-Q resonances in plasmonic metasurfaces

## Abstract

Plasmonic nanostructures hold promise for the realization of ultra-thin sub-wavelength devices, reducing power operating thresholds and enabling nonlinear optical functionality in metasurfaces. However, this promise is substantially undercut by absorption introduced by resistive losses, causing the metasurface community to turn away from plasmonics in favour of alternative material platforms (e.g., dielectrics) that provide weaker field enhancement, but more tolerable losses. Here, we report a plasmonic metasurface with a quality-factor (Q-factor) of 2340 in the telecommunication C band by exploiting surface lattice resonances (SLRs), exceeding the record by an order of magnitude. Additionally, we show that SLRs retain many of the same benefits as localized plasmonic resonances, such as field enhancement and strong confinement of light along the metal surface. Our results demonstrate that SLRs provide an exciting and unexplored method to tailor incident light fields, and could pave the way to flexible wavelength-scale devices for any optical resonating application.

## Introduction

Metallic nanostructures are essential to many applications in photonics, including biosensing1, spectroscopy2,3, nanolasing4, all-optical switching5, nonlinear optical processes6, and metasurface technologies7,8,9. These plasmonic elements form flexible components with geometry-dependent responses and have many desirable properties, such as the possibility to confine light to sub-wavelength scales and large local-field enhancements9,10. Metals also possess intrinsic nonlinear optical constants that are many orders of magnitude larger than dielectric materials11.

When structured at the sub-wavelength scale8,9,12, individual nanostructures exhibit localized surface plasmon resonances (LSPRs), where electromagnetic fields couple to the free-electron plasma of a conductor at a metal–dielectric interface6,10. Depending on its shape, an individual nanoparticle may be polarized by an incident light beam, acting as a lossy dipole antenna13 and trapping light for a short period of time. In contrast to other photonic resonant devices such as whispering gallery mode resonators, microring resonators, or photonic crystals14,15,16, resonating dipoles in a metasurface can easily be accessed by a beam propagating in free space and require only a sub-wavelength propagation region for operation. Therefore, a plasmonic metasurface resonator enables a series of specialized optical responses, including phase-matching-free nonlinear optical effects6,17, strongly localized field enhancements9, multi-mode operation18, and a spatially localized optical response7. Such a metasurface with a large quality factor (Q-factor) could be used as a cavity for applications that need increased light–matter interactions, small mode volumes, large field enhancements, and large optical nonlinearities, such as an ultra-flat nano-laser with a large transverse mode size4,19 or frequency conversion applications (e.g., nonlinear harmonic generation20 or THz-wave generation21). One frequently cited limitation of LSPR-based metasurfaces are their low Q-factors (e.g., Q < 10) due to the intrinsic Ohmic losses present in metals at optical frequencies10,22,23,24. As the Q-factor is related to the light–matter interaction time as well as to enhancements to the electric field, it is typically desirable to maximize this quantity14. Low Q-factors therefore make many potential applications of plasmonics-based metasurface devices impractical, and new methods for obtaining large Q-factor resonances in a metasurface have long been sought after.

The optical response of coupled plasmonic nanoresonators has been a topic of intense study25. Notably, plasmonic metasurfaces of large periodically arranged nanostructures support collective resonances called surface lattice resonances (SLRs)26,27,28,29,30,31,32. Here the individual responses from the surface plasmons of many individual nanostructures form a collective response that couples to in-plane diffraction orders of the periodic array26,30. As a consequence, a relatively high-Q resonance can emerge at an optical wavelength λSLR ≈ nP, close to the product of the refractive index of the background medium n and the lattice period P26,32. Recent theoretical studies of this platform have predicted Q-factors on the order of 103 by properly engineering the dimensions of the individual nanostructures and the period of the lattice31,32,33, hinting at the possibility of combining the aforementioned benefits of metals with long interaction times provided by high Q-factors. However, to date, the highest experimentally observed Q-factor in an SLR-based metasurface is 43034. The disparity between theory and experiment has been attributed to a variety of reasons, including poor spatial coherence of light beams28,35, small array sizes30,31,36, fabrication imperfections30,31, and the addition of an adhesion layer37.

Inspired by this discrepancy, here we perform a detailed investigation to determine the dominant factors that most drastically affect the observed Q of an SLR-based metasurface: the nanostructure geometry, the array size, and the spatial coherence of the probing light source. Using the results of this study, we demonstrate a plasmonic metasurface capable of supporting ultra-high-Q SLRs.

## Results

The metasurface in consideration consists of a rectangular array of rectangular gold nanostructures embedded in a homogeneous silica glass (n ~ 1.45) environment (Fig. 1a). The lattice constant Py = 1060 nm was selected to place the SLR wavelength in the telecommunication window; Px = 500 nm was reduced from a square lattice, increasing the nanoparticle density and consequently increasing the extinction ratio of the resonance. The overcladding is carefully matched to the substrate material to ensure a symmetric cladding index, as it has been shown that the Q of an SLR may be affected by the homogeneity of the environment26,38,39. As shown by the numerical predictions in Fig. 1b, for an x-polarized beam, this metasurface is expected to support an LSPR at λLSPR = 830 nm and an SLR of the first type around λSLR = 1550 nm (See Supplementary Sec. S2: SLR type). The SLR linewidth is substantially narrower than that of the LSPR, corresponding to a much higher Q-factor. Incidentally, the inset field profiles in Fig. 1b also reveal that the SLR provides a more significant field enhancement, with $$| {E}_{\max }({\lambda }_{{\rm{SLR}}})| \sim 3| {E}_{\max }({\lambda }_{{\rm{LSPR}}})|$$. Figure 1c shows an image of the fabricated device with dimensions matching those of the simulations. The measured transmission spectra are presented in Fig. 1d, closely matching the predicted spectrum. Notably, the full width at half-maximum of the linewidth is only Δλ = 0.66 nm, corresponding to a Q-factor of Q = 2340. This value exceeds the record for plasmonic metasurfaces by an order of magnitude34,37,40 and is among the highest reported in a metasurface. It is roughly within a factor of two of semi-analytic calculations performed using the lattice sum approach (LSA), where Q ~ 5000 (see “Methods” for details). In order to observe this value for the Q-factor, both the metasurface and the measurement apparatus needed to be arranged with a few considerations in mind, which we describe in greater detail below.

### The role of nanoparticle polarizability

First, the individual structures need to be engineered to exhibit the appropriate response at λSLR. The optical response of a nanostructure can be approximated using the polarizability of a Lorentzian dipole,

$$\alpha (\omega )=\frac{{A}_{0}}{\omega -{\omega }_{0}+i\gamma },$$
(1)

where A0 is the oscillator strength, ω0 = 2πc/λLSPR corresponds to the nanoparticle resonance frequency, and γ is the damping term. These quantities all depend on the particle geometry12 (here the length Ly and width Lx of a rectangular bar). The contribution of the particle lattice to the polarizability can be introduced using the LSA39,41:

$${\alpha }^{* }(\omega )=\frac{\alpha (\omega )}{1-{\epsilon }_{0}\alpha (\omega )S(\omega )},$$
(2)

where α*(ω) is known as the effective polarizability of the entire metasurface and S(ω) corresponds to the lattice sum. This latter term depends only on the arrangement of the lattice. An SLR appears approximately where S(ω) exhibits a pole, at ωSLR = (2πc/λSLR). At this spectral location, the individual responses of all of the nanostructures contribute cooperatively41.

Equation (2) may be used to predict the optical response of the entire metasurface, including the behavior of its many resonances, as a function of the geometry of its nanostructures (see “Methods”): by changing the geometry of a nanostructure12,42, its individual resonance wavelength λLSPR, oscillator strength A0, and damping constant γ are all modified. In turn, adjusting these values changes the polarizability of the nanostructures throughout the spectrum, including at the SLR wavelength α(ωSLR), and therefore also the response of the entire metasurface at this wavelength α*(ωSLR). Here we adjust the above parameters by changing the dimensions of the nanostructures (see “Methods”), while the parameters could be alternatively modified by considering altogether different nanostructure shapes, such as nanorings, nanorods, or core–shell nanoparticles42. By contrast, the spectral location of the SLR wavelength is dictated mainly by the lattice period and the background index λSLR ≈ nP32,43,44. In other words, the lattice configuration governs the presence of the SLR, and the nanostructure geometry dictates its coupling efficiency to free space. Indeed, recent theoretical studies in this platform have shown Q-factors on the order of 103 by properly selecting the dimensions of the individual nanostructures31,33.

We reproduce this dependence in this platform explicitly by plotting the calculated transmission of a metasurface (see “Methods”) as a function of nanostructure resonance wavelength λLSPR (Fig. 2). (The dependence of the SLR behavior on particle dimensions, which is connected to the resonance wavelength, is also demonstrated using full-wave simulations in Supplementary Sec. S3: Dependence of SLR behavior on particle dimensions.) Here we hold the oscillator strength A0 and damping term γ constant and slowly increase the nanoparticle resonance wavelength λLSPR. Note that the resonance position differs slightly from the position of the dip due to the incorporation of a long-wavelength correction45. In Fig. 2b, c, the SLR wavelength does not change substantially from its location around λSLR = 1542 nm; however, the extinction ratio ΔT and the linewidth Δλ of the resonance change dramatically. In Fig. 2d, we plot the extracted Q-factors for these SLRs and for other values of A0, as well (see Supplementary Sec. S1: Q-factor extraction for the fits). Based on well-established relationships between nanoparticle geometry and polarizability10,46, this A0 range corresponds to a change in nanoparticle volume of roughly 20%. We find that, for every given value of A0, there is a corresponding λLSPR for which light couples optimally to the lattice resonance at λSLR and produces the highest Q-factor. The optimal conditions are therefore found in the balance between increasing α relative to Py (i.e., increasing coupling strength) and maintaining a large spectral gap between λLSPR and λSLR (i.e., limiting Ohmic losses associated with metallic nanoparticles). The trade-off between coupling and loss is a traditional one for optical resonators and is reproduced in the SLR-based metasurface platform47.

### Effect of array size

Next, we study the dependence of the Q-factor on the array size. For certain metasurfaces, it has already been predicted that larger array sizes lead to better device performance36,48. This dependence makes some intuitive sense—since high-Q operation requires low absorption losses, we are required to operate the device far from the LSPR. However, at a sufficiently far operating wavelength, the scattering cross-section is also small, resulting in each antenna scattering very weakly. Consequently, far from the LSPR, one requires a sufficiently large number of scatterers to build up the resonance. Equivalently, the standing wave mode in an SLR consists of counter-propagating surface waves; therefore, a larger array provides an expanded propagation length in the cavity to support these modes.

To examine the dependence of Q on the number of nanostructures explicitly, we fabricated and characterized a series of devices of increasing array size. Figure 3 shows the resulting transmission spectra, as well as their corresponding semi-analytic predictions. The observed Q-factors increase monotonically as a function of array size (Fig. 3b—see Supplementary Sec. S1: Q-factor extraction for the fits). In the smallest array (300 × 300 μm2), the SLR is almost imperceptible. This trend might help explain the relatively low Q values observed in previous studies9,30,31,36 where array sizes were typically no larger than 250 × 250 μm2, likely due to the relatively slow write-speed of the electron-beam lithography process necessary for fabrication26,37. By contrast, our devices have array sizes reaching up to 600 × 600 μm2 (see Supplementary Sec. S4: Image of the device).

### The role of spatial coherence

Finally, it is of critical importance to consider all aspects of the characterization system in order to get an accurate measurement of the Q-factor. In particular, we have found that the spatial coherence of the probe beam was critical to obtaining a clean measurement of the dip in transmission indicating a resonance. A spatially coherent beam, such as a laser, excites every region of the metasurface in phase, producing a resonance feature that is both deeper and narrower compared to using a spatially incoherent source. Additionally, the higher-order modes of the lattice are more sensitive to angular variance in the measurements, leading to broader peaks when using incoherent sources35. Furthermore, in our particular experiment, the transmitted signal from our coherent supercontinuum source was both brighter and could also be better collimated than our incoherent thermal source. Therefore, the light collected from the metasurface array could be isolated with a smaller pinhole in the image plane, selecting the signal coming from nanostructures at the center of the array with a more uniform collective response.

In Fig. 3, we compare the performance of the metasurface when illuminated using different light sources: a broadband supercontinuum laser (i.e., a well-collimated coherent source), and a tungsten-halogen lamp. The comparison between these measurements indicates that the Q increases with the coherence of the light source—using the thermal light source reduces the Q-factor by a factor of 2–5 when compared to the laser. Additionally, it decreases the resonance coupling strength, as is evident from the reduced extinction ratio of the SLRs. Figure 3b summarizes the Q-factors extracted from these measurements and compares them to numerical predictions. LSA calculations predict that Q-factors increase as a function of array size; this trend continues for both smaller and larger devices than those probed experimentally. Note that, even when using an incoherent source, the largest array still produces a very large Q-factor (Q ~ 1000). The observation of such a high Q using an incoherent source reinforces the validity of our aforementioned metasurface design criteria—that is, the importance of the choice of nanostructure geometry and of the array size.

In some of the measurements, the value for the normalized transmittance can be seen to exceed unity (i.e., T > 1). We speculate that this is because the nanostructures aid in coupling to the substrate, reducing the reflections from the first interface.

## Discussion

Despite promising results, Fig. 3b also highlights some discrepancies between the simulation and the experiment for the largest arrays, notably reducing the measured Q-factors. This disparity could be due to multiple reasons, which we enumerate below. First, the prediction produced by the LSA might be overestimating the Q by assuming that each nanoparticle is excited with a constant-valued local field. This assumption cannot be entirely correct for a Gaussian beam and a finite array, where particles closer to the boundaries of the array feel a weaker local field than the particles near the center. Second, the fabrication procedure produces stitching errors, which become more important for larger arrays. This added disorder might contribute to the reduction in Q. Lastly, the Q-factors might be limited due to additional measurement considerations, such as the finite coherence length of the light source or imperfections with the collimation.

In this work, we only looked into rectangular nanoparticles in rectangular lattices. Based on LSA calculations and the discrete-dipole approximation (DDA) used in previous work26,39,44,49,50, it is evident that any particle geometry (e.g., cylindrical, rectangular, or triangular) that can be approximated by dipoles with the same Lorentzian parameters A0, λLSPR, and γ will yield an identical SLR Q-factor. For nanoparticles that cannot be modeled by dipoles—regardless of the particle geometry—the SLR Q-factor will be the same provided that the polarizability at λSLR remains the same. Regarding different lattice configurations, the spectral responses of other lattice geometries such as hexagonal, orthorhombic, and kagome are likely to be different than the rectangular lattice design we have adopted. However, lattice sums can be computed for these regular lattices, and therefore they can also be treated using our method. Therefore, strategies presented in this work are largely blind to the specific lattice arrangements, and its conclusions will be helpful in obtaining resonances with large-Q factors in other geometries.

The Q-factors for the type of device presented here could be further increased, however, by considering larger arrays or by further optimizing the nanostructure dimensions—instead of rectangles, a more intricate nanostructure shape could tailor the Lorentzian dipole coefficients A0, λLSPR, and γ more independently to allow for optimal coupling and higher extinction ratios. These shapes include L-shaped antennas51, split-ring resonators52, and others that also exhibit higher-order moments53,54. Alternatively, a nanoparticle with a large aspect ratio could increase coupling to more neighboring particles using out-of-plane oscillations44. Finally, the metasurface shown here can be combined with other established methods to enable multiple simultaneous resonances39,50,55.

Table 1 contains a short survey of the literature on metasurface nanocavities. Other than the reported Q-factors, we have included, when available, information that is relevant to compare their work against ours, such as the operating wavelength, the material platform, the array size, and the type of light source used. Our work demonstrates the highest Q by an order of magnitude among metasurfaces with plasmonic components and is exceeded only by metasurfaces that incorporate a bound state in the continuum (BIC).

To summarize, we have fabricated and experimentally demonstrated a plasmonic metasurface nanoresonator with a high Q-factor, which is in excellent agreement with numerical predictions. Our work presents the experimental demonstration of a high-Q plasmonic metasurface nanoresonator with an order-of-magnitude improvement over prior art (see Table 1). We have found that the observed Q-factor obtained from an SLR may be limited by a poor choice of nanostructure dimensions, a small array size, or poor spatial coherence of the source illumination; we hypothesize that one or many of these factors may have been the cause for the low Q-factors reported in previous experiments featuring SLRs. Additionally, our device follows simple design principles that can be easily expanded upon to enable multiple resonances to fully tailor the transmission spectrum of a wavelength-scale surface. Our result highlights the potential of SLR-based metasurfaces and expands the capabilities of plasmonic nanoparticles for many optical applications.

## Methods

### Simulations

#### Finite-difference time domain (FDTD)

Full-wave simulations were performed using a commercial three-dimensional FDTD solver. A single unit cell was simulated using periodic boundary conditions in the in-plane dimensions and perfectly matched layers in the out-of-plane dimension. The structures were modeled using fully dispersive optical material properties for silica56 and for gold57. Minimal artificial absorption ($${\rm{Im}}(n)\ \sim \ 1{0}^{-4}$$) was added to the background medium to reduce numerical divergences.

#### Lattice sum approach

The LSA is a variant of the DDA method58. It is a semi-analytic calculation method that has been found to produce accurate results for plasmonic arrays39,41,44. The main assumption in LSA when compared to DDA is that the dipole moments of all interacting nanoparticles are assumed to be identical44. The main benefit of using LSA for our application compared to alternatives such as FDTD is its capability to model finite-sized arrays with an arbitrary number of nanostructures, by assuming that the overall response of the array closely follows the responses of the nanoparticles at the center of the array. By comparing simulations performed using the LSA against the DDA, this assumption has also been found to be quite accurate44. Its rapid simulation time makes it a useful tool for iterating many simulations to study trends and behaviors of entire metasurfaces, especially for finite array effects, such as the effect of array size on the Q-factor.

Using the LSA approach, the dipole moment p of any particle in the array is written as

$${\bf{p}}=\frac{{\epsilon }_{0}\alpha (\omega ){{\bf{E}}}_{{\rm{inc}}}}{1-{\epsilon }_{0}\alpha (\omega ){{S}}(\omega )}\equiv {\epsilon }_{0}{\alpha }^{* }(\omega ){{\bf{E}}}_{{\rm{inc}}},$$
(3)

where the effect of inter-particle coupling is incorporated in the lattice sum $${{S}}$$ and α* is the effective polarizability. This equation produces Eq. (2) in the main text. The calculations presented in this work also incorporate a modified long-wavelength correction45:

$$\alpha (\omega )\to \frac{{\alpha }_{{\rm{static}}}(\omega )}{1-\frac{2}{3}i{k}^{3}{\alpha }_{{\rm{static}}}(\omega )-\frac{{k}^{2}}{l}{\alpha }_{{\rm{static}}}(\omega )},$$
(4)

where k is the wavenumber in the background medium k = (2πn/λ) and l is the effective particle radius. Also here, minimal artificial absorption ($${\rm{Im}}(n)=6\times 1{0}^{-4}$$) was added to the refractive index n = 1.452 of the background medium to reduce numerical divergences associated with the approach when considering large arrays41. We set l = 180 nm for all calculations. The static polarizability of the nanoparticle is given by

$${\alpha }_{{\rm{static}}}(\omega )=\frac{{A}_{0}}{\omega -{\omega }_{0}-i\gamma },$$
(5)

where A0 is the oscillator strength, ω0 = 2πc/λLSPR corresponds to the nanoparticle resonance frequency, and γ is the damping term.

For a planar array of N dipoles, the lattice sum term $${{S}}$$ is

$${{S}}(\omega )=\mathop{\sum }\limits_{j=1}^{N}\frac{\exp ({\rm{i}}k{r}_{j})}{{\epsilon }_{0}{r}_{j}}\left[{k}^{2}+\frac{(1-{\rm{i}}k{r}_{j})(3{\cos }^{2}{\theta }_{j}-1)}{{r}_{j}^{2}}\right],$$
(6)

where rj is the distance to the jth dipole and θj is the angle between rj and the dipole moment p.

The optical transmission spectra can be obtained by using the optical theorem, $${\rm{Ext}}\propto k{\rm{Im}}({\alpha }^{* })$$59:

$$T(\omega )=1-\frac{4\pi k}{{P}_{x}{P}_{y}}{\rm{Im}}[{\alpha }^{* }(\omega )],$$
(7)

where Px and Py are the lattice constants along the x and y dimensions, respectively.

To produce the plots in Fig. 1d, we performed an LSA calculation using the following parameters for the single dipole: λLSPR = 780 nm; A0 = 3.46 × 10−7 m3/s, γ = 8.5 × 1013 s−1. LSA parameters were determined by matching to FDTD data. The lattice constants were Px = 500 nm and Py = 1067.5 nm. The total array size was 600 × 600 μm2, corresponding to Nx = 1200 × Ny = 562 nanostructures, respectively. The LSA calculations in Fig. 3 used these same parameters but varied the total number of nanostructures.

To calculate the figures in Fig. 2a, c, we performed a series of LSA calculation using the following parameters for the particle: A0 = 3.98 × 10−7 m3/s, γ = 1/[2π(2.1 fs)] ≈ 7.6 × 1013 s−1. The dipole resonance wavelengths λLSPR were 800, 833, 866, 900, 933, 966, and 1000 nm, respectively. Based on the performed FDTD simulations, these resonance wavelengths could correspond to rectangular gold nanostructures with widths of Lx = 110, 120, 130, 140, 150, 160, and 170 nm, respectively, if Ly = 190 nm, and t = 20 nm. (Note that, in the main text, Ly = 200 nm). See Supplementary Sec. S3: Dependence of SLR behavior on particle dimensions for the corresponding simulations. The lattice constants were Px = 500 nm and Py = 1060 nm, respectively. The total array size was 600 × 600 μm2, corresponding to Nx = 1200 × Ny = 567 nanostructures, respectively. To obtain Fig. 2d, a series of LSA calculations were performed for many values of λLSPR ranging from 800 to 1000 nm, and the Q-factors were extracted from the results using a fit to a Lorentzian. The curves in Fig. 2d come from repeating this procedure with oscillator strengths of A0 = 3.98 × 10−7, 4.38 × 10−7, and 4.77 × 10−7 m3/s.

### Device details

We fabricated different metasurface devices with array sizes of 300 × 300, 400 × 400, 500 × 500, and 600 × 600 μm2, with a corresponding number of participating nanostructures of 600 × 284, 800 × 378, 1000 × 472, and 1200 × 567, respectively. The lattice constants of the rectangular arrays are Px = 500 nm × Py = 1060 nm. The dimensions of the rectangular gold nanostructures are Lx = 130 nm × Ly = 200 nm, with a thickness of t = 20 nm. The lattice is embedded within a homogeneous background n ≈ 1.46.

### Fabrication

The metasurfaces are fabricated using a standard metal lift-off process. We start with a fused silica substrate. We deposit a silica undercladding layer using sputtering. We then define the pattern using electron-beam lithography in a positive tone resist bi-layer with the help of a commercial conductive polymer. The mask was designed using shape-correction proximity error correction60 to correct for corner rounding. Following development, a thin adhesion layer of chromium (0.2-nm thick) is deposited using e-beam evaporation, followed by a layer of gold deposited using thermal evaporation. Lift-off is performed, and a final protective silica cladding layer is deposited using sputtering. The initial and final silica layers are sputtered using the same tool under the same conditions to ensure that the environment surrounding the metasurface is completely homogeneous. Before characterization, the surface of the device is then covered in index-matching oil. The backside of the silica substrate is coated with an anti-reflective coating to minimize substrate-related etalon fringes.

### Characterization

See Supplementary Sec. S5: Experimental set-up for a schematic of the experimental set-up.

#### Coherent light measurements

To measure the transmission spectra, we flood-illuminated all of the arrays in the sample using a collimated light beam from a broadband supercontinuum laser source. The wavelength spectrum of the source ranges from λ = 470 to 2400 nm. The beam comes from normal incidence along the z-direction with light polarized in the x-direction. The incident polarization is controlled using a broadband linear polarizing filter. Light transmitted by the metasurface is then imaged by a f = 35 mm lens, and a 100-μm pinhole is placed in the image plane to select the desired array. The transmitted light is collected in a large core (400 μm) multimode fiber and analyzed using an optical spectrum analyzer and is normalized to a background trace of the substrate without gold nanostructures. The resolution of the spectrometer is set to 0.01 nm.

#### Incoherent light measurements

Here the experiment goes as above, but the samples are excited using a collimated tungsten-halogen light source (ranging from λ = 300 to 2600 nm) and a 400-μm pinhole.

## Data availability

The data that support the plots within this paper and other findings of this study are available from the corresponding author upon reasonable request.

## Code availability

The code used to analyze the data and the related simulation files are available from the corresponding author upon reasonable request.

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## Acknowledgements

Fabrication in this work was performed in part at the Centre for Research in Photonics at the University of Ottawa (CRPuO). The authors acknowledge support from the Canada Excellence Research Chairs (CERC) Program, the Canada Research Chairs (CRC) Program, and the Natural Sciences and Engineering Research Council of Canada (NSERC) Discovery funding program. M.S.B.-A. acknowledges the support of the Ontario Graduate Scholarship (OGS), the University of Ottawa Excellence Scholarship, and the University of Ottawa International Experience Scholarship. O.R. acknowledges the support of the Banting Postdoctoral Fellowship of the NSERC. Y.M. was supported by the Mitacs Globalink Research Award. M.J.H. acknowledges the support of the Academy of Finland (Grant No. 308596) and the Flagship of Photonics Research and Innovation (PREIN) funded by the Academy of Finland (Grant No. 320165).

## Author information

Authors

### Contributions

M.S.B.-A., O.R., and M.J.H. conceived the basic idea for this work. O.R. and M.S.B.-A. performed the FDTD simulations. M.J.H., M.S.B.-A., and O.R. performed the lattice sum calculations. O.R. and G.C. fabricated the device. M.Z.A. and M.J.H. designed the preliminary experimental set-up. M.S.B.-A. and Y.M. carried out the measurements. O.R., M.S.B.-A., and Y.M. analyzed the experimental results. J.U., B.T.S., J.-M.M., M.J.H., R.W.B., and K.D. supervised the research and the development of the manuscript. M.S.B.-A. and O.R. wrote the first draft of the manuscript. All co-authors subsequently took part in the revision process and approved the final copy of the manuscript. Portions of this work were presented at the 2020 SPIE Photonics West Conference in San Francisco, CA.

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### Competing interests

The authors declare no competing interests.

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Bin-Alam, M.S., Reshef, O., Mamchur, Y. et al. Ultra-high-Q resonances in plasmonic metasurfaces. Nat Commun 12, 974 (2021). https://doi.org/10.1038/s41467-021-21196-2

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• DOI: https://doi.org/10.1038/s41467-021-21196-2

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