Ultrawide dynamic modulation of perfect absorption with a Friedrich–Wintgen BIC

Enduo Gao; Rong Jin; Zhenchu Fu; Guangtao Cao; Yan Deng; Jian Chen; Guanhai Li; Xiaoshuang Chen; Hongjian Li

doi:10.1364/PRJ.481020

1. INTRODUCTION

Surface plasmon polaritons (SPPs), which are generated by the coupling between photons in the incident light source and electrons on a metal or insulator, can break the diffraction limit of conventional optics and localize light in the subwavelength range. Thus, SPP-based metamaterials hold potential applications in sensing, imaging, and communications [1 –3]. In particular, SPP-based perfect absorbers have been widely studied, such as the dual-band absorber based on the dielectric grating and Fabry–Perot cavity [4], the narrowband absorber based on multiridge gratings [5], and the broadband absorber based on tungsten ring-disc array [6]. However, the majority of absorbers can only be statically regulated, seriously hindering their practical application. Graphene, due to its ultracompact configuration, low loss, and flexible tunability, has become the research focus. In general, perfect absorption can be achieved when the radiation loss and absorption loss of the graphene system are equal [7]. The variation of the Fermi level of graphene inevitably leads to the difference between radiation loss and absorption loss. In addition, as the Fermi level of graphene decreases, the coupling between the in-plane electric field and the interband absorption of graphene becomes weaker, resulting in a lower absorption rate of the system [8 –16]. Thus, it is a challenge to ensure the perfect absorption of the system while dynamically regulating the frequency. Despite the fact that a small number of devices can obtain perfect absorption of dynamic regulation, the frequency modulation range is less than 2 THz [17 –22].

Originally derived from the quantum theory, the bound states in the continuum (BICs) refer to the isolated eigenvalues of the single-particle Schrödinger equation of positive energy states in the continuum [23]. Subsequently, it was extended to many fields, such as electromagnetism [24], acoustics [25], fluid dynamics [26], and optics [27]. The optical BICs behave as a resonant state with zero linewidth and infinite quality factor ( $Q$ -factor). Kivshara et al. discussed the potential mechanism of the optical BIC [28] and proposed a polarization-insensitive quasi-BIC [29]. This feature was verified experimentally in the transmission of the metasurfaces. Remarkably, the optical BIC is employed into the field to generate higher harmonics up to the 11th order [30]. An accidental BIC is the unexpected disappearance of the coupling between the bound state and the continuum by tuning the parameters of the system [31,32]. It can be subdivided into the Fabry–Perot (F–P) BIC [33] and Friedrich–Wintgen (F–W) BIC [34]. The F–P BIC arises from the destructive interference between two identical resonant modes when the phase difference between them is an integer multiple of $π$ . The F–W BIC occurs from a destructive interference between two different excitation modes, and their radiation channels avoid crossing. However, it is worth noting that in the modulation of the F–W quasi-BIC, one mode gradually disappears to form the BIC, and the other mode changes to a limited extent due to the complicated underlying physics [35 –37]. Until now, introducing the F–W BIC tuned by the Fermi level to achieve the dynamic modulation of perfect absorption remains unresolved and is very desirable.

In this work, we propose a new strategy to realize a tunable perfect absorption based on F–W BICs. First, a pentaband ultrahigh absorber arising from the interaction of Fabry–Perot resonance (FPR) and guided mode resonance (GMR) is demonstrated. The absorption rates of three modes in the pentaband absorber are higher than 98%, which are far better than other single-band [38,39], dual-band [40 –44], and multiband [45 –48] absorbers. Further studies show that statically modulating the width of graphene gratings can lead to a strong coupling between FPR and GMR modes, resulting in an F–W BIC. Theoretical analysis based on the coupled-mode theory (CMT) [49,50] reveals the strong coupling between the two modes and fits well with the absorption spectrum of the numerical simulation. To demonstrate the BIC, the band structure of the proposed system is shown, with the real part of the complex frequency of the BIC coinciding with the BIC position of the absorption spectrum. The free-space radiation in the field distribution of the BIC is zero, which further proves that the F–W BIC is an eigenstate of the system. Furthermore, the F–W BIC realized by the dynamic modulation of the Fermi level of graphene gratings can break the traditional modulation with the incidence angle. Most interestingly, thanks to the formation of the F–W BIC, the like-FPR mode can be dynamically modulated while ensuring its perfect absorption. The modulation range is up to 3.5 THz, which is much higher than that of other perfect absorbers [17 –22].

2. STRUCTURAL DESIGN AND ANALYSIS

Figure 1 represents the proposed model. The monolayer graphene is sandwiched in the dielectric, the graphene grating is placed on top, and the substrate is gold. The graphene surface conductivity can be expressed as [51] $σ_{g} = \frac{i e^{2} E_{F}}{π κ^{2} (ω + i τ^{- 1})},$ (1)where $ω$ is the angular frequency of the light source, $E_{F}$ is the graphene Fermi level, $e$ is the electron charge, $κ$ is the reduced Planck constant, and $τ$ is the carrier relaxation time, which can be represented by $τ = μ E_{f} / (e v_{F}^{2})$ . The Fermi velocity and carrier mobility of the system are $v_{F} = 10^{6} m / s$ and $μ = 1 m^{2} / (V \cdot s)$ , respectively [52]. A side view of the system is plotted in Fig. 1(b) to show the structure more clearly. The period of the structural unit is $P = 490 nm$ , the width of the graphene grating is $w = 400 nm$ , the refractive index of the ${SiO}_{2}$ is $n = 1.6$ , and the distance between the graphene grating and graphene sheet is $h_{1} = 12 nm$ . Since the carrier concentration of single-layer graphene can be as high as $4 \times 10^{18} m^{- 2}$ , the Fermi level of graphene can reach 1.17 eV [53]. Thus, the Fermi level $E_{f}^{'}$ of graphene gratings and the Fermi level $E_{f}$ of graphene sheets are set to a maximum of 1.0 eV.

Figure 1.(a) 3D schematic diagram composed of graphene gratings and graphene sheets; (b) 2D side view of the proposed system; the specific parameters are as follows: $P = 490 nm$ , $w = 400 nm$ , $h_{1} = 12 nm$ , $h_{2} = 1350 nm$ , $h_{3} = 100 nm$ , $E_{f}^{'} = E_{f} = 1.0 eV$ .

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In this paper, the finite-difference time-domain (FDTD) method is adopted to explore the absorption spectrum of the proposed system. A transverse magnetic (TM) wave is used as an excitation source to irradiate the system vertically. The Bloch period condition and the perfectly matched boundary are set in the $x$ direction and $y$ direction, respectively. The simulation temperature and time are 300 K and 8000 fs, respectively. Mesh accuracy is 5 nm in both the $x$ and $y$ directions. The gold mirror is used to block the transmission of TM waves, so the absorption of the system is $A = 1 - R$ .

3. SIMULATION RESULTS AND DISCUSSION

Since an F–W BIC is a strong coupling between two modes, we first analyze the specific mode. The TM-polarized wave as an excitation source can produce an excellent pentaband absorber with absorption rates above 90%, of which three bands are as high as 98% or more, as shown in Fig. 2(a). Since the impedance mismatch between the regions with and without an upper graphene grating, the graphene surface plasmon polaritons (GSPPs) propagating along the $x$ direction reflect back and forth between the two boundaries, forming a standing wave. For visual observation, the positive and negative charges of the electric field distribution are represented by “+” and “−.” This standing wave can also be called lateral FPRs [54], which can be expressed as $ω_{FPR} = \frac{Kc}{2 w n_{M}} .$ (2)Here, $n_{M}$ is the effective refractive index of the standing wave, and $c$ is the light velocity. $K$ , corresponding to the mode order of the FPR mode, is the number of the electric field nodes [Figs. 2(b)–2(e)], which is equal to integer multiples of the half-wavelength. The vertically incident TM-polarized light can only excite the odd mode of the FPR because the effective charge dipole provides the restoring force for the collective oscillating wave [55]. In addition, graphene gratings enable momentum matching between incident light and GSPPs to excite GMR [Fig. 2(f)], which can be expressed as [56] $ω_{GMR} = \sqrt{\frac{e^{2} E_{F}}{κ^{2} ε_{0} ε_{r} P}} .$ (3)Here, $ε_{0}$ is the permittivity in vacuum, and $ε_{r}$ is the relative permittivity of the ${SiO}_{2}$ .

Figure 2.(a) Absorption spectra of the proposed system; (b)–(f) electric field distribution of different modes in the $y$ direction.

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To explore modes corresponding to different excitation mechanisms, the electric field diagrams of different modes in the $y$ direction are shown in Figs. 2(b)–2(f). As we predicted, FPR modes are generated in the F–P cavities constructed from graphene gratings and graphene sheets, and the corresponding $K$ are 1, 3, 5, 7, respectively. A first-order GMR mode appears on the outside of graphene gratings and graphene sheets. It is worth noting that the coupling between the FPR ( $K = 7$ ) and the GMR ( $K = 1$ ) modes occurs due to their close proximity, so those two modes are named like-FPR and like-GMR modes. The ultrahigh absorption of the system is mainly manifested by three aspects. On the one hand, the FPR resonance mode ( $K = 1$ , 3, 5, 7) interacts with graphene gratings and the graphene sheets to enhance the light absorption. On the other hand, the GMR mode excited by the graphene grating similarly enhances the absorption. In addition, the strong coupling between the FPR ( $K = 7$ ) and GMR modes further enhances the light localization.

To observe the formation process of the F–W BIC, the absorption spectrum as a function of the width of the graphene grating is shown in Fig. 3(a). An avoided resonance crossing with a Rabi splitting is observed around 33 THz. Due to the destructive interference between FPR ( $K = 3$ ) and GMR modes at the phase-matching conditions [57], an F–W BIC is generated at an off-Γ point. The hybridization of FPR and GMR modes forms a new polaritonic-optical quasi-particle [58,59]. In short, the nature of the F–W BIC is a destructive interference between two different resonance modes, and their radiation channels avoid crossing. The BIC at $w = 168 nm$ and quasi-BIC (white circle) at $w = 144 nm$ are denoted in Fig. 3(b). The yellow circle in Fig. 3(a) is also the strong coupling between the different modes, one of which does not completely disappear even though their radiation channels avoid crossing, which occurs because the two modes do not reach the suitable phase-matching condition. Therefore, the position of yellow circle also can achieve an F–W BIC by modulating the parameters to achieve the correct phase-matching conditions. The absorption spectra at different $w$ [Fig. 3(c)] indicate an avoided crossing behavior with Rabi splitting. The Rabi energy can reach 18.9 meV when $w = 176 nm$ [60].

Figure 3.BIC formation in the hybrid FPR–GMR system. (a) Absorption spectrum as a function of the width of the graphene grating; (b) cross sections of the absorption spectra at $w = 168 nm$ and 144 nm show the appearance of the collapsed F–W BIC to quasi-BIC. (c) Avoided crossing and linewidth vanishing due to the coupling of FPR and GMR modes at different w.

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The strong coupling between FPR and GMR modes can be resolved by CMT [Fig. 4(a)]. The $A_{n}$ stands for the FPR or GMR mode, and its amplitude is $a_{n}$ . $γ_{on} = ω_{n} / 2 Q_{on}$ and $γ_{in} = ω_{n} / 2 Q_{in}$ are the inter-external and inter-internal loss coefficients of the two modes. $Q_{on}$ and $Q_{in}$ are the inter-external and inter-internal loss quality factor, and they can be satisfied by $1 / Q = 1 / Q_{on} + 1 / Q_{in} (Q$ is the total quality factor of quasi-BIC or like-FPR mode). The coupling coefficient between modes can be represented by $μ_{12}$ and $μ_{21}$ . $A_{n}^{in / out}$ ( $n = 1$ , 2) indicates the incident or outgoing wave along the positive or negative direction of the mode. The interaction between the two modes can be represented as $(\begin{matrix} γ_{1} & - i μ_{12} \\ - i μ_{21} & γ_{2} \end{matrix}) \cdot (\begin{matrix} a \\ b \end{matrix}) = (\begin{matrix} - γ_{o 1}^{1 / 2} & 0 \\ 0 & - γ_{o 2}^{1 / 2} \end{matrix}) \cdot (\begin{matrix} A_{1 +}^{in} + A_{1 -}^{in} \\ A_{2 +}^{in} + A_{2 -}^{in} \end{matrix}),$ (4)where $γ_{1 (2)} = i ω - i ω_{1 (2)} - γ_{i 1 (2)} - γ_{o 1 (2)}$ . The coupling between FPR and GMR satisfies the energy conservation, $A_{2 +}^{in} = A_{1 +}^{out} e^{i φ}, A_{1 -}^{in} = A_{2 -}^{out} e^{i φ} .$ (5)Here, $φ$ is the phase difference between the FPR and GMR modes. For one of two modes, energy conservation still holds, which can be expressed as $A_{n \pm}^{out} = A_{n \pm}^{in} - a_{n} γ_{on}^{1 / 2}, n = 1, 2.$ (6)Due to the presence of the substrate gold, the electromagnetic waves emitted from the GMR mode return to continue interacting with the one, which can be expressed as $A_{2 -}^{in} = A_{2 +}^{out} e^{2 i ϕ} .$ (7)Thus, the reflection coefficient $r$ of the coupling system can be obtained by $r = \frac{A_{-}^{out}}{A_{+}^{in}} = e^{2 i (φ + ϕ)} - \frac{γ_{o 1}^{1 / 2} a_{1} [1 + e^{2 i (φ + ϕ)}] + γ_{o 2}^{1 / 2} a_{2} e^{i φ} (1 + e^{2 i ϕ})}{A_{+}^{in}} .$ (8)The specific coefficients are as follows: $\frac{a}{A_{+}^{in}} = \frac{γ_{o 1}^{1 / 2} [1 + e^{2 i (φ + ϕ)}] k_{2} - γ_{o 1}^{1 / 2} e^{i φ} (1 + e^{2 i ϕ})}{k_{1} k_{2} + χ_{2}},$ (9) $\frac{b}{A_{+}^{in}} = \frac{γ_{o 2}^{1 / 2} e^{i φ} (1 + e^{2 i ϕ}) - γ_{o 1}^{1 / 2} e^{i φ} [1 + e^{2 i (φ + ϕ)}] χ_{2}}{k_{1} k_{2} + χ_{1} χ_{2}},$ (10)where $χ_{1} = i μ_{12} + γ_{o 1}^{1 / 2} γ_{o 2}^{1 / 2} e^{i φ} (1 + e^{2 i ϕ}), χ_{2} = i μ_{21} + γ_{o 1}^{1 / 2} γ_{o 2}^{1 / 2} e^{i φ} (1 + e^{2 i ϕ}),$ (11) $k_{1} = γ_{o 1} e^{2 i (φ + ϕ)} - γ_{1}, k_{2} = γ_{o 2} e^{2 i ϕ} - γ_{2} .$ (12)Therefore, the absorption rate of the system is $A = 1 - r^{2}$ . The coupled absorption spectrum between FPR and GMR modes at $w = 144 nm$ is shown in Fig. 4(b), and the results of CMT are consistent with the data of the FDTD.

Figure 4.(a) Schematic diagram of CMT; (b) coupled absorption spectra of FDTD numerical simulation and CMT fitting at $w = 400 nm$ .

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To demonstrate the F–W BIC, the band structures and the corresponding $Q$ -factor evolution of the FPR–GMR hybrid system are plotted in Fig. 5. The band structures of the FPR and GMR modes avoid crossing, marking the formation of an F–W BIC [61]. The position of the band structure corresponding to the maximum value in the $Q$ -factor evolution is BIC. The $Q$ value is finite due to absorption loss. The real part of the corresponding complex frequency of the BIC at $k_{x} = 0.068$ is 33 THz, which is consistent with the position of the BIC in the boundary value problem [Fig. 3(b)]. Also, the electric field distribution of the BIC at $k_{x} = 0.068$ is represented in the inset of Fig. 5(a). The rapid decay of the far field of the eigenmode to 0 further demonstrates the BIC. Therefore, the F–W BIC of the proposed system is an eigenstate with 0 radiative loss, but it still has absorption loss.

Figure 5.(a) Band structures of the proposed FPR–GMR hybrid system. Here, the illustration shows electric field distribution at F-W BIC. (b) Simulated $Q$ -factor evolution for the GMR band.

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Figure 6.(a) F–W BIC dynamically modulated by the Fermi energy level of a graphene grating ( $w = 144 nm$ ); (b)–(e) field distribution of the two modes in the $y$ direction when $E_{f}^{'} = 1.0 eV$ and 0.3 eV; (f) perfect absorption frequency modulator and optical switch based on F–W BIC.

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4. CONCLUSION

In summary, we have achieved dynamic modulation of the perfect absorption spectrum in a pentaband ultrahigh absorption system composed of graphene gratings and graphene sheets by introducing an F–W BIC. The radiation loss of the system is suppressed due to the destructive interference between FPR and GMR modes at coherent phase-matching conditions, producing an F–W BIC. Its nature originates from the avoidance of crossing when two different modes are coupled to the same radiation channel. Remarkably, the largest modulation range, 3.5 THz, is achieved by controlling the Fermi level of the graphene grating with our structure. It holds great promise in applications like optical switches and frequency modulators with perfect absorption. We believe this work will provide a new strategy to develop frequency modulators with perfect absorption and stimulate the development of multiband ultracompact devices.

Category: Optical Devices

Received: Nov. 23, 2022

Accepted: Jan. 4, 2023

Published Online: Feb. 28, 2023

The Author Email: Guanhai Li (ghli0120@mail.sitp.ac.cn)

DOI:10.1364/PRJ.481020