Abstract
A plasmonic modulator is a device that controls the amplitude or phase of propagating plasmons. In a pure plasmonic modulator, the presence or absence of a plasmonic pump wave controls the amplitude of a plasmonic probe wave through a channel. This control has to be mediated by an interaction between disparate plasmonic waves, typically requiring the integration of a nonlinear material. In this work, we demonstrate a 2D semiconductor nonlinear plasmonic modulator based on a WSe_{2} monolayer integrated on top of a lithographically defined metallic waveguide. We utilize the strong interaction between the surface plasmon polaritons (SPPs) and excitons in the WSe_{2} to give a 73 % change in transmission through the device. We demonstrate control of the propagating SPPs using both optical and SPP pumps, realizing a 2D semiconductor nonlinear plasmonic modulator, with an ultrafast response time of 290 fs.
Introduction
Plasmonic modulators have been highly sought after for approaches to optical frequency information processing devices^{1,2,3,4,5}. Optical frequency plasmonic devices offer potential advantages over electronic devices due to the high carrier frequency of optical waves, as well as the potential to use ultrafast solidstate nonlinearities for subpicosecond switching times. Furthermore, by using plasmonic structures, optical frequency waves can be confined to subfreespace wavelength waveguides allowing for miniaturization of onchip optical devices^{1}. Early plasmonic modulators demonstrated modulation using quantum dots^{3}, photochromic molecules^{6} as integrated nonlinear materials, but were limited by slow (>40 ns and 10 s) switching times^{3,6}. Ultrafast (~200 fs) plasmonic modulation was demonstrated with a modulation depth of 7.5% (~0.3 dB) by direct optical pumping of bare metallic plasmonic waveguides^{5}, but required the use of high ~90 nJ pump pulse energy. The current stateoftheart plasmonic modulators based on traditional bulk nonlinear materials and nanoplasmonic resonator/interferometer structures typically can achieve modulation depths on order of 1–10 dB μm^{−1} with response times >2 ps and require ~3–20 pJ of pulse energy to operate^{7,8,9}. Recently, graphenebased alloptical^{10} and plasmonic^{11,12} modulators have been studied, and compared favorably to previous modulators in terms of switching speed and energy^{11}. In 2018, a graphenebased plasmonic modulator achieved 0.2 dB μm^{−1} modulation depth with a switching energy of 155 fJ and a response time of 2.2 ps using a deep subwavelength plasmonic waveguide^{12}. This progress motivates the investigation of other atomically thin materials in plasmonic modulator structures, that have the potential to achieve faster response times, lower switching energies and larger modulation depths.
In free space optical measurements, monolayer WSe_{2} and other semiconducting TMDs are known to exhibit large lightmatter interactions and large thirdorder nonlinear optical susceptibilities near their exciton resonance^{13,14,15,16,17,18,19}. Recently, there has been significant interest in using monolayer TMDs for plasmonic applications including the demonstration of SPPs coupling to dark excitons in monolayer WSe_{2}^{20,21}, increasing the nonlinear response using localized plasmonic effects^{22,23,24}, and enhancement of single quantum emitter emission rates^{25,26}
In this work, we investigate the 2D semiconductorplasmonic structure as depicted in Fig. 1a in order to understand the fundamental excitonSPP interactions and to demonstrate their promise for active plasmonic devices. Our results rely on the atomically thin nature of the TMD and the surface confined SPP mode to realize an attractive geometry where the active layer is near the maximum amplitude of the SPP mode. Furthermore, we develop a novel, selfconsistent theory of excitonSPP (ESPP) coupling that is unique to the 2D layer geometry and includes a complete ESPP dispersion relation for arbitrary distances between the metal surface and the TMD layer. We show that our ESPP model is highly predictive for both the linear (transmission) and nonlinear (differential transmission) response. We take advantage of the fast nonlinear optical response of 2D semiconductor excitons to realize an ultralow switching energy plasmonic modulator with a modulation depth of at least 4.1% in continuous wave (CW) measurements, limited by the pump power used in the measurement. Our timedomain measurements reveal a fast (slow) component of the nonlinear response with a response time of 290 fs (13.7 ps).
Results
Fabrication of ESPP device and linear response
Monolayer WSe_{2} was integrated on top of the metallic waveguide structures to serve as a nonlinear active layer. Monolayer WSe_{2} was isolated through mechanical exfoliation from high quality bulk crystals. The WSe_{2} thickness was confirmed by photoluminescence. In order to electrically isolate the WSe_{2} from the metallic waveguide (to avoid quenching of excitons), it was encapsulated with hBN. The hBNWSe_{2}hBN heterostructures were fabricated and transferred onto the waveguides using a polymer based dry transfer technique (polycarbonate film on polydimethylsiloxane, PDMS, stamp)^{27}. The transfer was performed under a microscope based probe station to allow for alignment of the 2D heterostructure and waveguide. All of the CW measurements in the main text were performed on the same sample with 5 nm top and 2 nm bottom hBN thickness. Timedomain measurements were performed on another sample with 9 nm and 3 nm hBN thickness. An optical microscope image of a hybrid 2D material plasmonic structure is shown in Fig. 1b.
The hybrid hBNWSe_{2}hBN/plasmonic structures were measured at 4.5 K (CW measurements) and 11 K (timedomain measurements) in a closedcycle optical cryostat to reduce thermal broadening effects. The transmission spectra and CW nonlinear measurements were measured using two tunable Ti:sapphire continuous wave lasers (M Squared SolsTiS). The laser was focused to a diffraction limited spot on the input grating coupler. Light scattered from the output grating coupler was isolated using a spatial filter and measured with a silicon photodiode. In the linear transmission measurements, the probe laser was modulated for lockin detection. In the nonlinear spectroscopy measurements, pump and probe beams were amplitude modulated at different frequencies near 500 kHz to allow for lockin detection at the modulation difference frequency. The timedomain pumpprobe measurements were performed with a tunable modelocked Ti:sapphire laser with a repetition rate of 76 MHz and pulse width of ~120 fs.
The SPP transmission spectrum is shown in Fig. 1c for 60 µW input power. The black data show the transmission spectrum for the hybrid hBNWSe_{2}hBN/plasmonic structure (with a ~4µmlong WSe_{2} layer), and the red data show a reference bare waveguide. At the exciton resonance (1.737 eV, 713.6 nm), the transmission is reduced by ~73% due to the presence of the WSe_{2} layer, indicating a large interaction between SPPs and WSe_{2} excitons. By comparing these transmission data to the photoluminescence spectrum (Fig. 1c inset), we can identify the dip in the SPP transmission as originating from the WSe_{2} neutral exciton (X^{0})^{14}. We note that the center energy of the PL and SPP absorption response are aligned to within 1 meV, consistent with previous optical measurements on monolayer WSe_{2}^{14}.
Theory of ESPP
In order to understand the coupling between SPPs and excitons, we use an extension of the wellknown SPP dispersion (k_{x}(ω)) that relates the wave vector component k_{x}, where the axis x is shown in Fig. 1a, of a mode propagating along the surface to its energy (\(\hbar \omega\)) where ω is the SPP’s angular frequency. Our approach complements other theories such as coupled oscillator (plexciton)^{28,29}, scattering^{30}, and gainassisted SPP theories^{4,31,32}. It is formulated for arbitrary distances between the metal surface and the TMD layer, and reduces to an expression calculated previously^{33,34} in the limit of vanishing distance. Using the dielectric function of the metal ε_{m}(ω) and the optical susceptibility χ(ω) of the TMD layer, we obtain their coupling directly by solving the dispersion relation, which is free of any fitting parameters. We use subscripts 1, 2, and 3 to denote the region above the TMD layer, between the metal surface and the TMD layer, and inside the metal, respectively (Supplementary Fig. 1).
The dispersion relation of the coupled exciton surface plasmon polariton is obtained in a way that is analogous to deriving that of an SPP, i.e., looking for nontrivial solutions of Maxwell’s equations that satisfy the continuity relations at the surface and decay away from it. The difference is the presence of the TMD layer, which requires additional continuity relations to be fulfilled, and there is no exponential decay in the region between the metal surface and the TMD layer. The coupling strength between the surface plasmon and the exciton in the TMD layer is governed by the factor \(e^{  {\mathrm{Im}} k_{2z}z_\ell }\) where k_{2z} is the wave vector component normal to the surface in region 2, and \(z_\ell\). As expected, the coupling is strong only if the layer is within the region of the evanescent surface mode. In the limit \(z_\ell \to 0\), we obtain k_{2z}(ε_{m}k_{2z} − k_{3z}) + gk_{3z} = 0 where \(k_{iz} = \pm \sqrt {\omega ^2\varepsilon _i/c^2  k_x^2}\) is the wave vector component perpendicular to the surface, the dielectric functions are ε_{1} = ε_{2} = 1 for the vacuum regions and ε_{3} = ε_{m}, and \(g = 4\pi i\left( {\omega ^2/c^2  k_x^2} \right)\chi (\omega )\) provides the coupling, in agreement with previous works^{33,34}. The more general form where the distance is an arbitrary input parameter is given (Supplementary Note 1). We use a Drude model for the metal and a Lorentz model for the TMD exciton. This results in an ESPP resonance at the exciton energy (1.737 eV) with the real and imaginary parts of k_{x}(ω) shown in (gray and blue curves, Fig. 2a). The ESPP group velocity is plotted (Supplementary Fig. 2). The peak value for \({\mathrm{Im k}}_{\mathrm{{x}}}\) of 0.07 µm^{−1} corresponds to an absorption length of 7.1 µm. Figure 2b shows the measured transmission as a function of the effective WSe_{2} sample length for the three different structures we investigated (Supplementary Fig. 3a–f). The effective WSe_{2} sample lengths were estimated from the optical microscope images by calculating an average length over the central 3 µm of the waveguide corresponding the fullwidth halfmax of the SPP spatial mode. An exponential fit to these data yields an effective decay length of 4.8 ± 0.6 µm, which is in good agreement (within a factor of two) of our theoretical model.
Nonlinear ESPP interactions
The transmission of the plasmonic device can be controlled by optically pumping the WSe_{2} excitons, partially saturating the absorption. Figure 3a depicts the experimental configuration where SPPs propagating through the plasmonic structure serve as the probe, and a free space laser focused on the hBNWSe_{2}hBN structure serves as an optical pump. Here, the focused optical pump beam diameter was chosen so that it illuminated nearly the entire WSe_{2} region with an intensity of 8.5 × 10^{6} Wm^{−}^{2}. Figure 3b shows the DT/T spectrum as a function of probe wavelength, i.e., the pumpinduced differential transmission (DT) normalized by the probe transmission (T). DT/T spectra for three different pump energies of 1.717 eV (red), 1.739 eV (black), and 1.746 (blue) are shown. When the pump laser is near resonance with the WSe_{2} X^{0}, the DT/T signal is maximized giving a peak value of DT/T = 4.1 × 10^{−3}. Figure 3c shows the pump power dependence of the DT signal near the center of the exciton peak (1.739 eV pump, 1.743 nm probe). The DT signal is linear with pump power indicating that the DT response arises from the thirdorder nonlinear susceptibility.
In order to demonstrate plasmonic modulation, we performed nonlinear measurements where both pump and probe lasers were coupled into the input grating, launching pump and probe SPPs (depicted in Fig. 4a). Figure 4b shows the CW DT/T spectra for three different pumpSPP energies 1.715 eV (red), 1.739 eV (black), and 1.771 eV (blue). We again observe a strong nonlinear response at the X^{0} resonance, corresponding to a maximum DT/T = 4.1 × 10^{−2}. For this case, we see the DT/T amplitude increases by a factor of 10 over the optically pumped signal. The SPP pump power (of the SPP) dependence is also linear (Fig. 4c), consistent with a thirdorder nonlinear response. From the finite difference timedomain (FDTD) model, we find that the SPP pump intensity is 4.6 × 10^{6} Wm^{−2}, ~2 times smaller than the optical pump case.
In order to quantify the response time of the system, we carried out resonant timedomain pumpprobe measurements. We used a single (~120 fs) pulsed laser tuned to resonance (1.736 eV, 714 nm) split into pump and probe, and a mechanical delay line to vary the pumpprobe temporal separation. The time dependent DT/T response is shown in Fig. 4d. A biexponential is fit to the positive time signal resulting in fast 290 ± 20 fs and slower 13.7 ± 0.6 ps components to the decay time. We note that these decay times are 5–10 times faster than previously reported for monolayer WSe_{2} on SiO_{2}^{35,36} which is not surprising due to the coupling to the SPP mode. Figure 4e shows the DT response as a function of pump pulse energy (of the SPP). We note that the required pump pulse energy to achieve a DT/T ≈1% is 650 fJ. We also note that in SPP pumpSPP probe measurements both pump and probe lasers were detected simultaneously, which both contribute to the DT signal. To account for this, the transmission used to calculate DT/T is the sum of both pump and probe beams combined.
To understand this plasmonic modulation effect and to estimate the orderofmagnitude of the thirdorder nonlinearity, we extended our linear analysis (Fig. 2a) to the thirdorder nonlinear response with perturbation theory. Since we only observe significant signal near 1.737 eV, we limit our model to inplane dipoles associated with the X^{0} excitons. This reduces the susceptibility tensor to the single thirdorder component χ^{(3)} (Supplementary Note 1). We assume that the pumpinduced change in the susceptibility (Δχ) is proportional to the average pump intensity (I_{p}), i.e. \({\mathrm{\Delta }}\chi (\omega ,I_{\mathrm{p}}) \approx \frac{{4\pi }}{c}I_{\mathrm{p}}\chi ^{(3)}(\omega )\). We can then use the linear dispersion relation with the replacement χ(ω) → χ(ω, I_{p}) = χ(ω) + Δχ(ω, I_{p}) which yields a pumpinduced change in the dispersion, Δk_{x}, and thus a measure of the pumpinduced differential transmission DT/T. We deduce a value for Imχ^{(3)} at the peak of the ESPP resonance by using the experimental value for DT/T and the estimated average intensity. For both, optical pump/SPP probe and SPP pump/SPP probe we find the order of magnitude of Imχ^{(3)} to be −10^{−20}m^{3}V^{−2}, in agreement with previously reported alloptical experiments^{16,35}. We note this value is a 2D thirdorder susceptibility. To compare this value to a hypothetical 3D susceptibility, one must divide it by the monolayer thickness.
Discussion
In this work, we have investigated both the linear and nonlinear response of excitons interacting with propagating SPPs in metallic waveguide structures. We show that the linear absorption of SPPs can be very large, exceeding 73%. The large absorption and nonlinear response might be surprising considering that the outofplane spatial extent of an SPP (~400 nm) is much larger than the TMD thickness (0.7 nm). However, our theoretical analysis is consistent with the measurements yielding an absorption coefficient on the order of 0.2 µm^{−1}. The key to the large linear absorption is the nanometerscale proximity of the TMD layer to the metal surface, which allows for the active layer to be located near the maximum of the SPP mode. By performing both optical pump and SPP pump DT measurements, we demonstrate control of SPP propagation with a DT/T response exceeding 4%. The modulation depth per unit length achieved in our modulator (0.04 dB µm^{−1}) is within an order of magnitude of other stateoftheart plasmonic modulators based on monolayer graphene^{12}. We note that in both optical and SPP pumped measurements, the maximum pump powers we used were conservatively chosen to avoid sample damage. Since the DT signals are linear in pump intensity up to the highest pump powers used (Figs. 3c and 4c), the reported modulation depths should be taken as lower bounds on the achievable modulation depth.
In principle, the modulation depth could be further enhanced by using longer TMD layers, stacking several TMD layers separated by hBN, or by decreasing the SPP mode size by depositing a high dielectric constant material on top of the structure. The modulation depth can also be increased by utilizing an interferometric or slot waveguide modulator structure^{11,12}. Furthermore, our theory predicts that the modulation depth increases with decreasing detuning between the exciton and the SPP resonance. This plasmonic enhancement follows from the equation \({\mathrm{\Delta }}k_x = h_{{\mathrm{enh}}}(\omega ){\mathrm{\Delta }}\chi (\omega )\), where the nonlinear change in the complexvalued propagation vector Δk_{x}, which governs directly measurable quantities such as DT/T \(\left(\propto {\mathrm{Im}} {\mathrm{\Delta}} {\mathrm{k}}_{\mathrm{x}} \right)\) is related to the change in the susceptibility Δχ(ω). The plasmonic enhancement factor h_{enh}(ω) is shown (Supplementary Fig. 4). Our model shows that increasing the exciton energy to 2.8 eV (with all other parameters unchanged) would increase Δk_{x} by more than 2 orders of magnitude.
To further quantify the performance of our modulator relative to previous works, we consider the response time and minimum energy needed to switch the modulator. Indeed the fast component of our response (290 fs) is comparable to the fastest previously reported plasmonic modulators^{5}, but we achieve a similar modulation depth with a ~10^{5} times lower pump pulse energy. Compared to other stateoftheart plasmonic modulators which typically require ~3–20 pJ of pulse energy to operate, with response times >2 ps^{7,8,9}, our demonstration of a 290fs response time with 650 fJ pump pulse energy compares favorably. We note that assuming a Gaussian pulse, this response time corresponds to a modulation bandwidth ~1.5 THz. We believe that future 2D semiconductorplasmonic structures based on our reported nonlinear excitonSPP plasmonic modulation effect could pave the way towards ultrafast plasmonic amplifiers and transistors with ultralow switching energies.
Methods
Fabrication
The gold waveguide was fabricated on 285 nm SiO_{2}/Si substrates by a twostep electron beam lithography process using an electron beam lithography system (100 kV Ellionix) and a spin coated poly(methyl methacrylate), PMMA, resist. In the first step, 200 nm gold was (electron beam) evaporated onto the substrate using 10 nm titanium sticking layer. In the second lithography step, PMMA was respun and the grating pattern was written and developed. We used an Ar^{+} milling process to etch the grating couplers into the waveguide. The waveguides are 5 µm × 13 µm. The grating couplers are composed of five grooves that are 40 nm deep with a width of 110 nm and period of 570 nm. The bare waveguides were characterized using atomic force microscopy (Supplementary Fig. 5a–d) and optical spectroscopy (Fig. 1c). The waveguide and grating coupler designs were optimized using an FDTD model. Simulations of the bare metallic structure show a maximum transmission of ~4% at the exciton resonance (Supplementary Fig. 6). We integrate a hexagonal boron nitride (hBN) encapsulated monolayer transition metal dichalcogenide (TMD) semiconductor, WSe_{2}, on top of the waveguide (see Fig. 1a), where the interaction between SPPs and excitons in the WSe_{2} provides the nonlinear response needed for modulation.
Data availability
The data that support the findings of this study are available from the corresponding author upon reasonable request.
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Acknowledgements
We acknowledge useful discussions with Javier García de Abajo, Robert Norwood, Josh Hendrickson, and Ricky Gibson. We thank Ty NewhouseIllige and Weigang Wang for performing the Ar^{+} milling process. We thank Fateme Mahdikhanysarvejahany for assistance in performing the timedomain measurements. This work is mainly supported by the AFOSRYIP award No. FA95501710215. M.R.K. and D.G.M. acknowledge support from the Gordon and Betty Moore Foundation’s EPiQS Initiative through grant GBMF4416. K.W. and T.T. acknowledge support from the Elemental Strategy Initiative conducted by the MEXT, Japan and the CREST (JPMJCR15F3), JST. J.R.S. acknowledges support from The Science Foundation of Arizona, Bisgrove Scholars Program (Grant No. BSP 082117) and AFOSR (Grant No. FA95501810049). B.J.L. acknowledges support from the National Science Foundation under Grant No. EECS1607911. AFM images and data were collected in the W.M. Keck Center for NanoScale Imaging in the Department of Chemistry and Biochemistry at the University of Arizona using equipment supported by the National Science Foundation under Grant No. 1337371. We would also like to thank Park Systems for their long term loan of the NX20 AFM instrument.
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Contributions
J.R.S. conceived and supervised the project. M.K. and B.H.B. fabricated the devices and performed the experiments, assisted by A.A. and M.M.; M.K., B.H.B., and J.R.S. analyzed the data with input from B.J.L.; M.R.K. and D.G.M. provided and characterized the bulk WSe_{2} crystals. T.T. and K.W. provided hBN crystals. R.B. developed and evaluated the coupled excitonSPP (ESPP) theory. M.K., B.H.B., R.B., and J.R.S. wrote the paper. All authors discussed the results.
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Klein, M., Badada, B.H., Binder, R. et al. 2D semiconductor nonlinear plasmonic modulators. Nat Commun 10, 3264 (2019). https://doi.org/10.1038/s4146701911186w
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