Research Article | Open Access
Xuanmiao Hong, Guangwei Hu, Wenchao Zhao, Kai Wang, Shang Sun, Rui Zhu, Jing Wu, Weiwei Liu, Kian Ping Loh, Andrew Thye Shen Wee, Bing Wang, Andrea Alù, Cheng-Wei Qiu, Peixiang Lu, "Structuring Nonlinear Wavefront Emitted from Monolayer Transition-Metal Dichalcogenides", Research, vol. 2020, Article ID 9085782, 10 pages, 2020. https://doi.org/10.34133/2020/9085782
Structuring Nonlinear Wavefront Emitted from Monolayer Transition-Metal Dichalcogenides
The growing demand for tailored nonlinearity calls for a structure with unusual phase discontinuity that allows the realization of nonlinear optical chirality, holographic imaging, and nonlinear wavefront control. Transition-metal dichalcogenide (TMDC) monolayers offer giant optical nonlinearity within a few-angstrom thickness, but limitations in optical absorption and domain size impose restriction on wavefront control of nonlinear emissions using classical light sources. In contrast, noble metal-based plasmonic nanosieves support giant field enhancements and precise nonlinear phase control, with hundred-nanometer pixel-level resolution; however, they suffer from intrinsically weak nonlinear susceptibility. Here, we report a multifunctional nonlinear interface by integrating TMDC monolayers with plasmonic nanosieves, yielding drastically different nonlinear functionalities that cannot be accessed by either constituent. Such a hybrid nonlinear interface allows second-harmonic (SH) orbital angular momentum (OAM) generation, beam steering, versatile polarization control, and holograms, with an effective SH nonlinearity of ~25 nm/V. This designer platform synergizes the TMDC monolayer and plasmonic nanosieves to empower tunable geometric phases and large field enhancement, paving the way toward multifunctional and ultracompact nonlinear optical devices.
In the past decade, nonlinear signals (second- and third-harmonic generation, SHG and THG) from nanomaterials and artificially structured materials, namely, metamaterials and metasurfaces, have attracted extensive attention for their wavelength tunability, coherence, and ultrafast responses [1–6]. These materials show promising applications in nanoprobing , imaging [2, 3], and crystalline detection [4–6]. Compared with the control of linear optical signals with a metasurface [7–14], the wavefront engineering and control of generated nonlinear signals are the most challenging task to realizing integrated, ultrathin, and efficient nonlinear optical devices, ranging from nonlinear beam steering [15, 16], nonlinear metalenses [17, 18], nonlinear holography [19, 20], optical image encoding , and the generation of a nonlinear optical vortex beam [22–24]. There have been several pioneering works on nonlinear phase control based on plasmonic metasurfaces, most of which focus on SHG manipulation [17, 20–27]. However, their weak second-order effective susceptibility, due to the inherently weak nonlinear response [22, 28] of plasmonic materials that rely on surface symmetry breaking, poses an intrinsic challenge for broad applications. Although SHG can be boosted by orders of magnitude to the level of ~pm/V under resonance conditions, the samples may be easily damaged by thermal effects due to the strong absorption. Alternatively, nonlinear hybrid metasurfaces, such as Au/multiple quantum well (MQW), have been proposed as an alternative to traditional plasmonic metasurfaces [29–31]. Previous works report 2~3 orders of magnitude of enhancement following this route [32–35]. Nevertheless, demanding fabrication requirements make it difficult to design ultrathin and compact multifunctional nonlinear metasurfaces that are needed for the flexible wavefront control of nonlinear signals.
On the other hand, emerging 2D materials, such as transition-metal dichalcogenide (TMDC) monolayers, are well known for their strong light-matter interactions and valley-polarized optoelectronic properties [36–44]. Of particular interest is the large nonlinearity of monolayer TMDCs (with chemical composition , , W, Ta, and Nb and , Se, and Te). Their broken centrosymmetry enables a second-order susceptibility around 1~100 nm/V [45–48], which is much larger than the one of many plasmonic metasurfaces (see Section 3 in SI for details), and is even comparable to record values reported in Au/MQW hybrid metasurfaces (~54 nm/V) . However, the polycrystalline nature of most CVD-grown TMDC monolayers is only several tens of μm in size; it is quite challenging to spatially control the amplitude, polarization, phase, and even angular momentum of the emitted SH from monolayer TMDC. A paradigm-shift mechanism is needed to boost, manipulate, and control the SH photons of atomically thin materials.
Nature actually provides a hint towards such a mechanism. Epoxy is a type of strong glue made from two resins, with neither individually able to make the glue sticky. Putting those two resins together, a strong and powerful adhesive is obtained, because a chemical bond is produced. Inspired by the working principle of epoxy, we experimentally report a recipe for full control of SH photons via an integrated nonlinear optical interface composed of plasmonic nanosieves strongly coupled to a TMDC monolayer. As a proof-of-concept validation, TOC illustrates the schematic of bonding a WS2 monolayer with a plasmonic Au nanosieve; the bonded assembly behaves as a hybrid nonlinear optical interface for multifunctional SHG manipulation. SHG is in principle forbidden in Au nanosieves since they are made of centrosymmetric rectangular nanoholes, but the integrated hybrid optical interface offers highly efficient SHG emission, whose properties may be precisely controlled at a hundred-nanometer pixel-level resolution. SHG, originating from the WS2 monolayer, is enhanced by the strong local fields within each Au nanoholes, and simultaneously, the geometric phase determined by individual Au nanoholes can be locally engineered and imparted to the WS2 monolayer on top of the Au nanosieves. Our experimental results indicate that an effective SHG susceptibility of ~25 nm/V is achieved, 3 orders of magnitude larger than the one of conventional plasmonic metasurfaces . Based on these principles, we demonstrate in the following several multifunctional nonlinear optical devices for free-space transmissive nonlinear optical interfaces for beam steering, versatile polarization control, orbital angular momentum (OAM) generation, and holograms. This strategy readily leads to the realization of a plethora of designer functions, enabling a new platform, i.e., TMDC-metasurface nonlinear optical interfaces, to realize robust nonlinear applications (e.g., high-order harmonic generation, HHG) with high efficiency, ultracompactness, and flexible fabrication.
Figure 1(a) illustrates the fabrication processing of a monolayer Au-WS2 metasurface, which can be easily prepared by a material transferring method (see Methods for details). An atomic force microscope (AFM) image of the WS2 flake shown in Figure 1(b), whose height profile is measured to be ~0.7 nm, indicates a WS2 monolayer. An optical image of the WS2 monolayer on the Au nanosieve is shown in Figure 1(c), indicating that the Au nanosieve is fully covered by a triangular WS2 monolayer with an area of 100 μm2. Figure 1(d) presents a scanning electron microscope (SEM) image of the same sample, indicated by the square area in Figure 1(c), where the high-quality WS2 monolayer can be clearly observed. Figure 1(e) presents the two-photon induced photoluminescence (TPL) spectrum from a WS2 monolayer under the excitation at 810 nm, showing the peak wavelength at ~620 nm. Figure 1(f) shows the Raman spectrum of the WS2 monolayer excited at 532 nm. Two typical signatures located at 352.3 and 417.3 cm−1 can be observed, which are attributed to the and phonon modes from the WS2 monolayer, respectively. In general, the characterization results prove the high quality of the WS2 monolayer, and their intrinsic properties are not changed in the hybrid Au-WS2 interface.
Figure 2(a) shows the calculated transmission spectrum of a single Au rectangular nanohole under a circular polarized (CP) excitation by using the FDTD method. The inset shows the calculated electric-field distribution at 810 nm, which is in good agreement with the wavelength of the fundamental laser at 810 nm. Figure 2(b) presents the measured spectra of the emitted SH signals of the Au-WS2 interface (red curve), a bare WS2 monolayer (blue curve) and pure Au nanoholes (black curve). It can be clearly seen that both curves have sharp peaks at 405 nm, which is the SHG wavelength. Note that no SHG can be observed in the bare Au metasurface under the same excitation (black curve). As shown in Figure 2(c), the intensity of the emitted signal of the Au-WS2 interface is increased linearly as the square of incident power. Thus, it can be concluded that the emitted signal is ascribed to the SHG of the WS2 monolayer. More importantly, the measured SHG intensity from the Au-WS2 interface is 5 times stronger than the one from the pure WS2 monolayer under the same excitation condition, which is ascribed to the strong field confinement in Au nanoholes. The area ratio of the nanohole and the whole unit cell is around . Without considering the local-field enhancement effect, the SHG intensity of the Au-WS2 interface should be in comparison with that of a pure WS2 monolayer. Therefore, the SHG intensity in the area of nanoholes of the Au-WS2 interface is estimated to be enhanced by two orders of magnitude ( times). Previous work indicates that the WS2 monolayer has a large second-order susceptibility of ~5 nm/V , and the effective second-order susceptibility of the Au-WS2 interface is estimated to be ~25 nm/V which is three orders of magnitude larger than the one of typical plasmonic metasurfaces (~pm/V).
The underlying physics of the SHG phase control in the integrated Au-WS2 interface is illustrated in Figure 3(a). It refers to a pixel for generating an SH signal with phase information. For a single Au nanohole, the rotation angle, , is defined as the angle between the long axis of the rectangular nanohole and the -axis. The nanohole can be considered as an ideal polaroid with an extinction ratio , and letting , the Jones’ matrix can be calculated by where is the rotation angle of a nanohole and is the rotation matrix. When a linearly polarized (LP) fundamental beam, , a -axis polarized is normally incident on the rectangular Au nanohole, the transmitted beam will be then it can be decomposed into
It indicates that the transmitted beam can be decomposed into three components: left-handed circularly polarized (LCP, ) and right-handed circularly polarized (RCP, ) beams, with geometric phase discontinuity ±2θ, and a LP beam without geometric phase, which are written as , , and , accordingly. For the WS2 monolayer with the point group symmetry, and assuming that the symmetry axis of the WS2 monolayer is parallel to the -axis, the second-harmonic susceptibility is , and we have
And then it can be decomposed into
As these fundamental beams further pump the WS2 monolayer, the emitted SH from the WS2 monolayer/Au nanohole has five components with different phase jump and polarization. The 0th-order SHG beam is a LP beam without deflection (along the -axis). The ±1st-order and ±2nd-order deflected beams are CP beams (LCP and RCP) with a phase delay of and , respectively. Due to the conservation of angular momentum, these deflected SHG beams have a polarization state orthogonal to the excitation fundamental beams. Therefore, the ±1st-order and ±2nd-order deflected beams can be written as and , respectively. The SHG phase can therefore be precisely controlled by orientating the Au nanoholes, which are also entangled with a spin angular momentum (SAM). Note that the intensity of the ±1st-order deflected beams is much stronger than the one of the ±2nd-order beams, so we mainly focus on the manipulation of ±1st-order SHG beams in the following. We stress that the results as well as its underlying mechanisms are fundamentally different from conventional nonlinear metasurfaces made of symmetric nanostructures (see Sections 1 and 2 in SI for further discussions), suggesting that this approach of hybridizing linear plasmonic metasurfaces with monolayer semiconductors with giant nonlinearity offers a new frontier in plasmonic metasurfaces. Therefore, we can realize multifunctional SH wavefront controls by designing an Au metasurface with a specific phase information.
Next, we elaborate on how this strategy can be implemented to realize multifunctional nonlinear optical devices. To demonstrate SHG manipulation, we designed a linear plasmonic nanosieve with a gradient phase as shown in the SEM image in Figure 3(b). The array is formed by a patterned rectangular Au nanohole with varying orientations, realizing a photonic spin-Hall metasurface with a geometric phase gradient (∇φ) along the -axis [13, 50]. A hexagonal arrangement with a period of 400 nm is employed to increase the density of unit cells. Specifically, Figure 3(c) shows the polarization distribution of the fundamental beam as it passes through the Au nanohole array (indicated by the rectangle area in Figure 3(b)), which is predominantly polarized along the short axis of each nanohole (indicated by the arrows). The deeper color indicates a stronger local field in the Au nanohole, which is further confirmed by FDTD simulation results in the same area shown in Figure 3(d).
In the inset of Figure 4(a), we show the phase distribution of the SH signals of the sample shown in Figure 3(b). Figure 4(a) presents the measured propagation of emitted SHG along the -axis. It can be seen clearly that the emitted SH signals are split into three beams. The inset images captured at different positions along the -axis present a clear illustration of the SHG spots, indicating a low divergence angle of the SHG beams. Specifically, the 0th-order SHG beam propagates along the -axis without any deflection due to the fundamental laser not carrying a geometric phase, while the rest travel along two sides of the -axis with the same deflection angle (±1st order). The deflection angle α is measured to be 10°, in good agreement with the theoretical design (10°). Furthermore, the polarization states of the SH beams are analyzed. The Stokes parameters of -1-, 0-, and 1-order SH beams are determined to be -0.90, -0.32, and 0.95, respectively. This indicates that the ±1st-order deflected beams have opposite CP with almost pure polarization, while the 0th-order SH beam is approximately LP. In Figures 4(b)–4(d), we show the extracted RCP component from the experimental results of different samples with designed deflection angles of 5°, 10°, and 15°, respectively. Correspondingly, the deflected RCP beams are observed at , 10°, and 15°, while the RCP component of the 0th-order beam propagates without deflection and the LCP component is blocked by a quarter-wave plate coupled with a Glan-laser polarizer. Interestingly, a weak 2nd-order SH beam can also be observed with a deflection angle of ~10° (Figure 4b), which is approximately twice the design angle of 5°. However, this cannot be observed in Figures 4(c) and 4(d), which may be ascribed to a low diffraction efficiency at a large deflection angle and limited detection efficiency in our experiment. Figures 4(e)–4(g) present that the numerical simulated results corresponded with the experimental results in Figures 4(b)–4(d), respectively, which is in good agreement with the experimental results (see Figure S2 in SI for further discussions).
Following the beam steering results, two deflected SHG beams propagate along different sides of the -axis with opposite spin angular momentums (SAMs). By reversing the order of the supercells arranged on the Au nanosieve, the SAM of the deflected SHG beams can be reversed, while keeping the same deflection angle. As a result, this integrated interface can generate a LP beam by a superposition of two SHG beams with opposite SAMs, whose polarization can be arbitrarily controlled by adjusting the phase difference of the two SHG beams. Figure 4(h) illustrates the schematic of versatile polarization control of the deflected SHG beam under excitation with a LP fundamental laser (-axis polarized). Specifically, by reversing the direction of the phase gradient of the supercells arranged on the odd lines of the Au metasurface, half are converted to deflect an opposite SAM while keeping the same deflection angle (), thus generating a LP beam. Note that both deflected LP beams have the same polarization. The phase difference of and can be controlled by adjusting the optical path difference, , where is the offset of the odd and even lines of the metasurfaces with an inversed order of the supercells. Figures 4(i)–4(k) present the polarimetric plots of the measured SHG intensity as a function of the polarization angle, , at phase differences, , 0.25λ, and 0.5λ, respectively. implies that the SHG beam is linearly polarized along the -axis. All measured SHG beams are approximately purely linearly polarized. The polarization directions for each beam are indicated by the long axis of the patterns at 10°, 55°, and 100°, respectively. This is in good agreement with the design rule , where is the SHG wavelength. We find the same deviation angle of 10° for each SHG beam, which is attributed to the orientation of the WS2 monolayer . This is quite different from the polarization control in the linear case . Such versatile nonlinear polarization generation can find applications in commercial polarization modulators .
The inset of Figure 5(a) presents the phase distribution of the 1st-order RCP component of the SH emission from each pixel under a LP pumping (-axis polarized), which can be described as where is the coordinates of the nanoholes, is the wavelength of SHG, is the deflection angle, is the topological charge, and is the azimuth angle in a circular coordinate system. Here, the deflection angle is and the geometric topological charge is . In Figure 5(a), we show the measured spatial intensity profiles of the emitted SH signals under a LP fundamental beam (-axis polarized), and five SHG beams are clearly seen as predicted by our theory. Specifically, the 0th-order beam with a circular spot is the LP beam without deflection. The ±1st-order SH beams are propagated along both sides of the -axis with the same deflection angle, indicating a doughnut-shaped spot due to the properties of OAM beam propagation. Both beams have opposite CP with the same value of deflection angle, , which is consistent with our design. Importantly, the topological charge is determined to be ±1 by the interference pattern between the 0th-order and ±1st-order beams (the details for the interference patterns are described in Figures S3 and S4 in SI). Note that both ±2nd-order SHG beams present a thinner doughnut-shaped pattern with a much weaker intensity than the ±1th-order SHG beams, whose topological charge is ±2 in theory. The deflection angle is measured to be around 20°, which is twice that of the ±1st-order beams under the small deflection angle approximation.
Interestingly, the phase plate of SH emission of the same sample appears to be quite different under the excitation of a CP fundamental beam, as shown in the inset of Figure 5(b), since the phase delay is doubled under CP excitation as compared to LP excitation. Figure 5(b) shows only two SHG beams: the SHG beam along the -axis is LP without deflection, similar to the 0th order in Figure 5(a). The -1st-order deflected SHG with a deflection angle of 20°, whose intensity distribution is doughnut-shaped with a topological charge of -2, is consistent with theoretical expectations. The spot shape, polarization, deflection angle, and topological charge of the -1st-order deflected SHG beam are the same as the -2nd-order SHG beam under LP excitation shown in Figure 5(a). Such difference can be attributed to the dependence of SHG on the amplitude of the fundamental beam. Our demonstration of dynamic nonlinear OAM generation under excitation with different polarizations can serve as the nonlinear version of the recently demonstrated metasurface-enabled quantum entanglement of SAM and OAM . The change of the spatial deflection angle of the -1st order in different pumping polarizations, i.e., resulting in different spots in the image plane, can also be further explored to realize a nonlinear quantum metasurface for photon state reconstruction . Thus, our demonstration of spin-entangled and spatially tunable nonlinear OAM here becomes very powerful for free-space quantum imaging, generation of entangled photon states, and other applications. Overall, these results provide clear evidence of the hundred-nanometer-precision phase control of SHG from the Au-WS2 interface.
Such a nonlinear integrated interface also allows holographic imaging, as schematically illustrated in Figure 6(a), where the circle with a diameter of 30 μm indicates the Au nanohole array. Under a LCP fundamental beam, the LCP component of the emitted SHG beam from the WS2 monolayer can be imaged in the Fresnel region. The image plane is designed to be 200 μm away from the sample, and each letter in the pattern is 25 μm wide. The designed objective images are the abbreviations for “Huazhong University of Science and Technology” and “National University of Singapore” (Figure 6(b)). The phase plane can be generated by an iterative method (further details are available in Figure S5 in SI). The theoretical images calculated by Fresnel-Kirchhoff’s diffraction formula and the measured experimental images are shown in Figures 6(c) and 6(d), respectively. The intensity distributions of the measured images match the theory very well.
In conclusion, we have proposed and experimentally demonstrated a new platform for full control of the nonlinear wavefront of SHG based on the Au-TMDC nonlinear optical interface. The hybrid nonlinear interface hybridizes an Au nanosieve with a WS2 monolayer, and the former acts as an unprecedentedly strong and precise “spatial light modulator” down to the pixel size of a hundred nanometers for the latter. Our results prove that multifunctional SHG control, such as SH beam steering; versatile polarization control; dynamic OAM generation; and holography are enabled, together with large effective second-order nonlinear susceptibility of ~25 nm/V. It provides a strategy for the efficient generation and manipulation of SHG signals. From an application viewpoint, this control enables miniaturized, high-performance nonlinear optical devices that have thickness in the nanometer scale range. This therefore opens up a wide range of opportunities to realize ultrathin, ultracompact nonlinear optical devices, such as beam splitting, versatile polarization control, and free-space quantum communications.
2.1. Sample Fabrication
(1)TheWS2 monolayers were fabricated on a sapphire substrate (SixCarbon Technology, Shenzhen). The solution of polymethyl methacrylate (PMMA, 2 wt%, Sigma-Aldrich) was drop-coated on the WS2-sapphire substrate. It was placed at room temperature for 1.5 h and then baked at 120°C for 0.5 h. The WS2-sapphire substrate was immersed in NaOH aqueous solution (3 mol/L) at room temperature for more than 4 h to etch the sapphire surface, and PMMA-WS2 films can be naturally lifted off from the sapphire substrate. The PMMA-WS2 films were fished out with a glass slide and immersed in deionized water for 3 times in order to remove the residual NaOH solution(2)A 60 nm thick gold film with a 5 nm thick Cr adhesion layer was deposited on a quartz substrate by using an e-beam evaporator. Then, the Au nanohole array with different arrangements was milled by the focused ion beam milling method (FIB, FEI Versa 3D)(3)With the help of a motorized stage-controlled needle, the PMMA-WS2 films were fished out by the fabricated metasurfaces, and then they were aligned quickly with the Au metasurface under the microscope before the water was dry. Finally, they were baked at 120°C for 1 h to improve the combination of the WS2 monolayers and the Au nanosieve and immersed in acetone for 3 times to remove the PMMA film
2.2. SHG Characterization
A mode-locked Ti-sapphire femtosecond laser centered at 810 nm (Vitara Coherent, 8 fs and 80 MHz) was used for the fundamental beam source. The polarization was adjusted by a quarter-wave plate (WPQ05M-808, Thorlabs). A home-built optical system was used to measure an emitted SH signal under an excitation of a plane-wave laser. The fundamental beam was focused by an 8 cm lens or an objective (Olympus, 10x and 0.25 NA) to generate different sizes of focal spots. The emitted signal was collected by an objective lens (Olympus, 40x and 0.65 NA), filtered spectrally, and imported to a CMOS camera (Prime 95B, Photometrics) or to a spectrometer (Acton 2500i with Pixis CCD camera, Princeton Instruments) through a fiber. The emitted SH signal was extracted by a Glan-laser polarizer with a quarter-wave plate at the SH wavelength (GL10-A and WPQ05M-405, Thorlabs). To measure the spatial intensity of the SH signals, we captured the SHG images at the different planes from 0 μm to 200 μm along the -axis with a step-size of 0.5 μm.
Additional Information. Supporting information is available.
Conflicts of Interest
The authors declare no competing financial interests.
K.W., P.X.L., and C.W.Q. conceived the project. K.W., P.X.L., A.A., and C.W.Q. supervised the project. K.W., G.W.H., A.A., and C.W.Q. designed the experiments. X.M.H., W.C.Z., K.W., and W.W.L. performed the experiments. G.W.H., K.W., B.W., P.X.L., A.A., and C.W.Q. analyzed the data. All authors discussed the results. G.W.H. and K.W. drafted the paper with the inputs from all authors. Xuanmiao Hong, Guangwei Hu, and Wenchao Zhao contributed equally to this work.
This work was supported by the National Natural Science Foundation of China (nos. 91850113 and 11774115), the 973 Programs under grant 2014CB921301, the Fundamental Research Funds for the Central Universities (2019kfyRCPY105), the Air Force Office of Scientific Research, and the Defense Advanced Research Projects Agency. C.-W.Q. acknowledges financial support from A*STAR Pharos Program (grant number 15270 00014, with project number R-263-000-B91-305) and the National Research Foundation, Prime Minister’s Office, Singapore, under its Competitive Research Program (CRP award number NRFCRP 15-2015-03). We give special thanks to the Center of Nano-Science and Technology of Wuhan University for their support of sample fabrication.
Figure S1: the schematic sketch of the experiment setup for SHG characterization. Figure S2: the emitted SHG beams along the -axis from the same sample at under the excitation of the LP and the RCP fundamental beam. Figure S3: numerically stimulated phase plates for the OAM generations shown in Figure 5 in the manuscript. Figure S4: determination of the topological charge of OAM. Figure S5: generative process of phase plates of holography. (Supplementary Materials)
- Y. Nakayama, P. J. Pauzauskie, A. Radenovic et al., “Tunable nanowire nonlinear optical probe,” Nature, vol. 447, no. 7148, pp. 1098–1101, 2007.
- B. E. Cohen, “Biological imaging beyond fluorescence,” Nature, vol. 467, no. 7314, pp. 407-408, 2010.
- P. Pantazis, J. Maloney, D. Wu, and S. E. Fraser, “Second harmonic generating (SHG) nanoprobes for in vivo imaging,” Proceedings of the National Academy of Sciences, vol. 107, no. 33, pp. 14535–14540, 2010.
- M. Cazzanelli, F. Bianco, E. Borga et al., “Second-harmonic generation in silicon waveguides strained by silicon nitride,” Nature Materials, vol. 11, no. 2, pp. 148–154, 2012.
- M. L. Ren, J. S. Berger, W. J. Liu, G. R. Liu, and R. Agarwal, “Strong modulation of second-harmonic generation with very large contrast in semiconducting CdS via high-field domain,” Nature Communications, vol. 9, no. 1, p. 186, 2018.
- H. B. Hu, K. Wang, H. Long, W. W. Liu, B. Wang, and P. X. Lu, “Precise determination of the crystallographic orientations in single ZnS nanowires by second-harmonic generation microscopy,” Nano Letters, vol. 15, no. 5, pp. 3351–3357, 2015.
- R. C. Devlin, A. Ambrosio, N. A. Rubin, J. P. B. Mueller, and F. Capasso, “Arbitrary spin-to-orbital angular momentum conversion of light,” Science, vol. 358, no. 6365, pp. 896–901, 2017.
- M. Khorasaninejad, W. T. Chen, R. C. Devlin, J. Oh, A. Y. Zhu, and F. Capasso, “Metalenses at visible wavelengths: diffraction-limited focusing and subwavelength resolution imaging,” Science, vol. 352, no. 6290, pp. 1190–1194, 2016.
- M. Pu, X. Li, X. Ma et al., “Catenary optics for achromatic generation of perfect optical angular momentum,” Science Advances, vol. 1, no. 9, article e1500396, 2015.
- A. Arbabi, Y. Horie, M. Bagheri, and A. Faraon, “Dielectric metasurfaces for complete control of phase and polarization with subwavelength spatial resolution and high transmission,” Nature Nanotechnology, vol. 10, no. 11, pp. 937–943, 2015.
- S. Sun, Q. He, S. Xiao, Q. Xu, X. Li, and L. Zhou, “Gradient-index meta-surfaces as a bridge linking propagating waves and surface waves,” Nature Materials, vol. 11, no. 5, pp. 426–431, 2012.
- I. Staude and J. Schilling, “Metamaterial-inspired silicon nanophotonics,” Nature Photonics, vol. 11, no. 5, pp. 274–284, 2017.
- J. X. Zhou, H. L. Qian, G. W. Hu, H. L. Luo, S. C. Wen, and Z. W. Liu, “Broadband photonic spin Hall meta-lens,” ACS Nano, vol. 12, no. 1, pp. 82–88, 2018.
- J. Xu, K. Bi, R. Zhang et al., “A small-divergence-angle orbital angular momentum metasurface antenna,” Research, vol. 2019, article 9686213, 8 pages, 2019.
- G. X. Li, S. M. Chen, N. Pholchai et al., “Continuous control of the nonlinearity phase for harmonic generations,” Nature Materials, vol. 14, no. 6, pp. 607–612, 2015.
- N. Nookala, J. Lee, M. Tymchenko et al., “Ultrathin gradient nonlinear metasurface with a giant nonlinear response,” Optica, vol. 3, no. 3, p. 283, 2016.
- N. Segal, S. Keren-Zur, N. Hendler, and T. Ellenbogen, “Controlling light with metamaterial-based nonlinear photonic crystals,” Nature Photonics, vol. 9, no. 3, pp. 180–184, 2015.
- E. Almeida, G. Shalem, and Y. Prior, “Subwavelength nonlinear phase control and anomalous phase matching in plasmonic metasurfaces,” Nature Communications, vol. 7, no. 1, 2016.
- E. Almeida, O. Bitton, and Y. Prior, “Nonlinear metamaterials for holography,” Nature Communications, vol. 7, no. 1, 2016.
- W. Ye, F. Zeuner, X. Li et al., “Spin and wavelength multiplexed nonlinear metasurface holography,” Nature Communications, vol. 7, no. 1, 2016.
- F. Walter, G. Li, C. Meier, S. Zhang, and T. Zentgraf, “Ultrathin nonlinear metasurface for optical image encoding,” Nano Letters, vol. 17, no. 5, pp. 3171–3175, 2017.
- S. Keren-Zur, O. Avayu, L. Michaeli, and T. Ellenbogen, “Nonlinear beam shaping with plasmonic metasurfaces,” ACS Photonics, vol. 3, no. 1, pp. 117–123, 2015.
- G. Li, L. Wu, K. F. Li et al., “Nonlinear metasurface for simultaneous control of spin and orbital angular momentum in second harmonic generation,” Nano Letters, vol. 17, no. 12, pp. 7974–7979, 2017.
- Y. Chen, X. Yang, and J. Gao, “Spin-selective second-harmonic vortex beam generation with Babinet-inverted plasmonic metasurfaces,” Advanced Optical Materials, vol. 6, no. 19, article 1800646, 2018.
- A. Krasnok, M. Tymchenko, and A. Alu, “Nonlinear metasurfaces: a paradigm shift in nonlinear optics,” Materials Today, vol. 21, no. 1, pp. 8–21, 2018.
- M. Kauranen and A. V. Zayats, “Nonlinear plasmonics,” Nature Photonics, vol. 6, no. 11, pp. 737–748, 2012.
- G. Li, T. Zentgraf, and S. Zhang, “Rotational Doppler effect in nonlinear optics,” Nature Physics, vol. 12, no. 8, pp. 736–740, 2016.
- J. Butet, P. F. Brevet, and O. J. F. Martin, “Optical second harmonic generation in plasmonic nanostructures: from fundamental principles to advanced applications,” ACS Nano, vol. 9, no. 11, pp. 10545–10562, 2015.
- J. Lee, M. Tymchenko, C. Argyropoulos et al., “Giant nonlinear response from plasmonic metasurfaces coupled to intersubband transitions,” Nature, vol. 511, no. 7507, pp. 65–69, 2014.
- M. Tymchenko, J. S. Gomez-Diaz, J. Lee, N. Nookala, M. A. Belkin, and A. Alu, “Gradient nonlinear Pancharatnam-Berry metasurfaces,” Physical Review Letters, vol. 115, no. 20, p. 207403, 2015.
- O. Wolf, S. Campione, A. Benz et al., “Phased-array sources based on nonlinear metamaterial nanocavities,” Nature Communications, vol. 6, no. 1, 2015.
- Y. Pu, R. Grange, C. L. Hsieh, and D. Psaltis, “Nonlinear optical properties of core-shell nanocavities for enhanced second-harmonic generation,” Physical Review Letters, vol. 104, no. 20, article 207402, 2010.
- M. L. Ren, W. J. Liu, C. O. Aspetti, L. X. Sun, and R. Agarwal, “Enhanced second-harmonic generation from metal-integrated semiconductor nanowires via highly confined whispering gallery modes,” Nature Communications, vol. 5, no. 1, 2014.
- H. Linnenbank, Y. Grynko, J. Forstner, and S. Linden, “Second harmonic generation spectroscopy on hybrid plasmonic/dielectric nanoantennas,” Light: Science & Applications, vol. 5, no. 1, p. e16013, 2016.
- Z. Wang, Z. G. Dong, H. Zhu et al., “Selectively plasmon-enhanced second-harmonic generation from monolayer tungsten diselenide on flexible substrates,” ACS Nano, vol. 12, no. 2, pp. 1859–1867, 2018.
- W. G. Xu, W. W. Liu, J. F. Schmidt et al., “Correlated fluorescence blinking in two-dimensional semiconductor heterostructures,” Nature, vol. 541, no. 7635, pp. 62–67, 2017.
- F. N. Xia, H. Wang, D. Xiao, M. Dubey, and A. Ramasubramaniam, “Two-dimensional material nanophotonics,” Nature Photonics, vol. 8, no. 12, pp. 899–907, 2014.
- D. N. Basov, M. M. Fogler, and F. J. Garcia de Abajo, “Polaritons in van der Waals materials,” Science, vol. 354, no. 6309, 2016.
- A. M. Jones, H. Y. Yu, N. J. Ghimire et al., “Optical generation of excitonic valley coherence in monolayer WSe2,” Nature Nanotechnology, vol. 8, no. 9, pp. 634–638, 2013.
- S. H. Gong, F. Alpeggiani, B. Sciacca, E. C. Garnett, and L. Kuipers, “Nanoscale chiral valley-photon interface through optical spin-orbit coupling,” Science, vol. 359, no. 6374, pp. 443–447, 2018.
- L. Y. Sun, C. Y. Wang, A. Krasnok et al., “Separation of valley excitons in a MoS2 monolayer using a subwavelength asymmetric groove array,” Nature Photonics, vol. 13, no. 3, pp. 180–184, 2019.
- P. K. Jha, N. Shitrit, X. X. Ren, Y. Wang, and X. Zhang, “Spontaneous exciton valley coherence in transition metal dichalcogenide monolayers interfaced with an anisotropic metasurface,” Physical Review Letters, vol. 121, no. 11, 2018.
- Z. L. Ye, T. Cao, K. O'Brien et al., “Probing excitonic dark states in single-layer tungsten disulphide,” Nature, vol. 513, no. 7517, pp. 214–218, 2014.
- X. Q. Lin, Y. Liu, K. Wang et al., “Hybrid three-dimensional spiral WSe2Plasmonic structures for highly efficient second-order nonlinear parametric processes,” Research, vol. 2018, article 4164029, 8 pages, 2018.
- N. Kumar, S. Najmaei, Q. N. Cui et al., “Second harmonic microscopy of monolayer MoS2,” Physical Review B, vol. 87, no. 16, article 161403, 2013.
- M. Merano, “Nonlinear optical response of a two-dimensional atomic crystal,” Optics Letters, vol. 41, no. 1, pp. 187–190, 2016.
- C. Janisch, Y. Wang, D. Ma et al., “Extraordinary second harmonic generation in tungsten disulfide monolayers,” Scientific Reports, vol. 4, no. 1, 2015.
- D. Neshev and Y. Kivshar, “Nonlinear optics pushed to the edge,” Science, vol. 344, no. 6183, pp. 483-484, 2014.
- G. Hu, X. Hong, K. Wang et al., “Coherent steering of nonlinear chiral valley photons with a synthetic Au‐WS2 metasurface,” Nature Photonics, vol. 13, no. 7, pp. 467–472, 2019.
- X. H. Ling, X. X. Zhou, K. Huang et al., “Recent advances in the spin Hall effect of light,” Reports on Progress in Physics, vol. 80, no. 6, article 066401, 2017.
- P. C. Wu, W. Y. Tsai, W. T. Chen et al., “Versatile polarization generation with an aluminum plasmonic metasurface,” Nano Letters, vol. 17, no. 1, pp. 445–452, 2016.
- T. Stav, A. Faerman, E. Maguid et al., “Quantum entanglement of the spin and orbital angular momentum of photons using metamaterials,” Science, vol. 361, no. 6407, pp. 1101–1104, 2018.
- K. Wang, J. G. Titchener, S. S. Kruk et al., “Quantum metasurface for multiphoton interference and state reconstruction,” Science, vol. 361, no. 6407, pp. 1104–1108, 2018.
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