Nonreciprocal Phonon Laser in an Asymmetric Cavity with an Atomic Ensemble

Kai-Wei Huang; Xin Wang; Qing-Yang Qiu; Long Wu; Hao Xiong

doi:10.1088/0256-307X/40/10/104201

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Nonreciprocal Phonon Laser in an Asymmetric Cavity with an Atomic Ensemble

School of Physics, Huazhong University of Science and Technology, Wuhan 430074, China

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Corresponding author:
Hao Xiong, E-mail: haoxiong1217@gmail.com

Received Date: June 24, 2023

Published Date: September 06, 2023

Abstract

Abstract

Phonon lasers, as a novel kind of lasers for generating coherent sound oscillation, has attracted extensive attention. Here, we theoretically propose a nonreciprocal phonon laser in a hybrid optomechanical system, which is composed of an asymmetric Fabry–Pérot cavity, an ensemble of N identical two-level atoms, and a mechanical oscillator. The effective driving amplitude related to driving direction leads to an obvious difference in mechanical gain and threshold power, bringing about a nonreciprocal phonon laser. In addition, the dependence of the phonon laser on the atomic parameters is also discussed, including the decay rate of the atoms and the coupling strength between the atoms and the cavity field, which provides an additional degree of freedom to control the phonon laser action. Our work provides a path to realizing a phonon laser in an atoms-cavity optomechanical system and may aid the manufacture of directional coherent phonon sources.

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Article Text

Moiré optical lattices, which are composite lattices when two identical periodic patterns (lattices) are rotated to each other by some angle (twisting angle) and then overlapped, have recently received great theoretical and experimental interests. Using optical induction technology in photorefractive crystals,^[1] reconfigurable optical Moiré lattices are created and localization of light in them is reported.^[2] Thanks to the suppression of light diffraction in Moiré lattices, nonlinear Moiré lattices are found to support optical solitons,^[3,3] second harmonic generation,^[5] and Bose–Einstein condensate (BECs)^[6] under lower power limits.

Moiré optical lattices have potential applications in ultra-cold atomic systems.^[7–10] Researchers have found that the periodic optical lattices in ultracold atoms exhibit finite atomic band gaps,^[11–13] which is the potential research direction of gap solitons (GSs).^[14–19] Among periodic optical lattices, parity-time (PT) symmetric lattices have received much attention in research of nonlinear physics in optical^[20–22] and matter-wave^[23,23] systems, providing an ideal platform for finding nonlinear waves.^[25–27]

In research of solitons in nonlinear media, many models have been proposed.^[28–32] Theoretical^[33] and experimental^[34] studies revealed that strong and long-range optical nonlinearities can be built by Rydberg–Rydberg interaction (RRI) between remote atoms.^[35] Especially, RRI can be mapped to a nonlocal optical nonlinearity through electromagnetically induced transparency (EIT), which is strong even at the single photon level.^[36] This provides an important platform for studies of optical soliton dynamics with tunable parameters.^[37] Interestingly, systems with Rydberg atoms are proven to be an effective medium to generate stable solitons with low energies for the strong and long-range optical nonlinearities between Rydberg atoms.^[38–40] However, to the best of our knowledge, combination of Rydberg–Rydberg interaction, moiré patterns, and PT symmetry has not yet been reported.

Model. We consider a cold lifetime-broadened four-level atomic system with an inverted-Y type configuration, as shown in Fig. 1(a).^[40] A standard Λ-type EIT configuration is constructed by the states |1〉, |2〉, |3〉 and the probe and control fields. The probe/control/auxiliary laser fields are coupled to the transitions |1〉 → |3〉, |2〉 → |3〉, and |3〉 → |4〉, with spontaneous emission decay rate Γ₁₃, Γ₂₃, and Γ₃₄, respectively; Δ₂, Δ₃ and Δ₄ are detunings. This EIT configuration is dressed by a high-lying Rydberg state |4〉, which is far off-resonantly coupled to |3〉 through an auxiliary laser field. The scheme of Rydberg-dressed EIT is used to exploit the advantages of both EIT and the Rydberg states.^[40]

Fig. Fig. 1. Excitation scheme of the 4-level atomic Rydberg system with an inverted-Y type configuration and the band structures for the two-dimensional (2D) PT-symmetric moiré lattices. A gain to the probe field has be provided to realize an optical PT symmetry in this weakly absorbed Rydberg-dressed EIT system. Band structures at θ = arctan (3/4) with increasing imaginary potential strength V₀ (b) and lattice strength ratio p (c). The band diagrams of moiré lattices in the reduced zone representation with V₀ = 0.02 and p = 1 at θ = arctan (3/4) (d), θ = arctan (5/12) (e), and θ = arctan (7/12) (f).

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Under the slowly varying amplitude approximation, the wave equation of the probe field following from the Maxwell equations has the following form^[25,25]

$\begin{array}{l} i (\frac{\partial}{\partial z} + \frac{1}{c} \frac{\partial}{\partial t}) Ω_{p} + \frac{c}{2 ω_{p}} (\frac{\partial^{2}}{\partial x^{2}} + \frac{\partial^{2}}{\partial y^{2}}) Ω_{p} \\ + \frac{ω_{p}}{2 c} χ_{p} Ω_{p} = 0, \end{array}$

(1)

where

$χ_{p} = N_{a} {(e_{p} \cdot P_{13})}^{2} ρ_{31} / (ε_{0} ℏ Ω_{p})$ is the susceptibility of probe field, N_a is the atom density, ρ_ij is the density-matrix element, z is the propagation direction. P_ij represents the electric-dipole matrix element, the subscripts i and j indicate the state |i〉 and |j〉. Ω_p and ω_p are, respectively, the Rabi frequency and angular frequency of probe field. The time derivative in Eq. (1) can be neglected and one is concerned with a stationary state. When the probe field is weak, the population of atomic levels does not change much with the application of the probe field, and consequently, a perturbation expansion can be employed to solve Eq. (1).^[27]

The evolution of the probe pulse is governed by the dimensionless (2+1)D nonlinear Schrödinger equation:

$\begin{array}{l} i \frac{\partial ψ}{\partial s} + (\frac{\partial^{2} ψ}{\partial ξ^{2}} + \frac{\partial^{2} ψ}{\partial η^{2}}) - Π ψ + γ | ψ |^{2} ψ \\ + α \int d^{2} r^{'} G_{2} (r^{'} - r) | ψ |^{2} ψ = 0, \end{array}$

(2)

where ψ = Ω_p/ψ₀, with ψ₀ being the typical Rabi frequency of the probe pulse, s = z/(2L_diff), r = (x,y), (ξ,η) = (x,y) / R_⊥,

$L_{diff} = 2 ω_{p} R_{⊥}^{2} / c$ and R_⊥ the typical radius of the probe pulse. Further, γ is the local Kerr nonlinear coefficient, and α is the degree of nonlocality of the system, G₂ (r – r′) = C₆/|r – r′|⁶ is the effective interaction potential contributed by RRI, with C₆ < 0 being the dispersion parameter.^[25] The stationary solution of Eq. (2) can be expressed in the form ψ = qe^ibs, where b is the propagation coefficient and s is the propagation distance.

A moiré optical potential is adopted with the form^[1,2,3]

$\begin{array}{l} Π = V_{1} {(\cos^{2} x + \cos^{2} y) + i V_{0} [\sin (2 x) + \sin (2 y)]} \\ + V_{2} {[(\cos^{2} x^{'} + \cos^{2} y^{'}) + i V_{0} [\sin (2 x^{'}) + \sin (2 y^{'})]}, \end{array}$

(3)

where V_1,2 are the lattice strengths and V₀ is the imaginary potential strength. The strength ratio between the two sub-lattices is defined as p = V₂/V₁ for discussion. It is noted that the potential Eq. (3) matches PT symmetry, Re[V_pt(r)] = Re[V_pt(–r)] and Im[V_pt(r)] = –Im[V_pt(–r)], and it reduces to the usual (non-PT) moiré lattice at V₀ = 0, and to the conventional PT lattice at V₂ = 0. The (x,y) plane is related to the rotation plane (x′,y′) with a twisting angle θ.

$(\begin{matrix} x^{'} \\ y^{'} \end{matrix}) = (\begin{matrix} \cos θ, & - \sin θ \\ \sin θ, & \cos θ \end{matrix}) (\begin{matrix} x \\ y \end{matrix}) .$

(4)

The spatial distributions of moiré lattices with PT-symmetric structure at different twist angles are shown in Fig. 2. With different twist angles, moiré optical lattices have both periodic and aperiodic characteristics. Only with special twist angles, such as θ = arctan (3/4) and θ = arctan (5/12), moiré optical lattices have periodic structures. The first and second rows show the periodic structures at θ = arctan (3/4) and θ = arctan (5/12). When choosing the other twisting angle such as θ = arctan (7/12) in Figs. 2(g), 2(h), and 2(i), the spatial distribution of moiré lattices is aperiodic. To take advantage of PT-symmetric structures, the twisting angle is fixed as θ = arctan (3/4) in this work.

Fig. Fig. 2. Contour plots and spatial distributions of moiré lattices with PT-symmetric structure at θ = arctan (3/4) (a)–(d), θ = arctan (5/12) (e)–(h), and θ = arctan (7/12) (i)–(l). The PT-symmetric moiré potentials are shown in the fourth column, where the real and imaginary (insets) parts of potentials at y = 0 display even and odd symmetries, respectively.

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Results and Discussions. The band structures for the 2D PT-symmetric moiré lattice at different twisting angles are shown in Figs. 1(b)–1(g). The curves of propagation coefficient b versus imaginary lattice strength V₀ and lattice strength ratio p are plotted in Figs. 1(b) and 1(c), respectively. One can find that the band gaps decrease rapidly with the increasing V₀ at θ = arctan (3/4). The band gaps decrease continuously with the increase of V₀, and there is almost no gap at V₀ = 0.5. The bands show flap characteristics with the changing lattice strength ratio p. The band structures of the moiré lattice at different twisting angles in the 2D reciprocal space are shown in Figs. 1(d), 1(e), and 1(f). It is found that the bands are localized in the reciprocal space, which is a key factor for the formation of stable solitons. For the periodic case in Figs. 1(d) and 1(e), the band structures are more complex so that there are some band crossings between the first and second gaps; while for the aperiodic structure in Fig. 1(f), the bands are located such that there is no band crossing.

A family of solitons, including fundamental GSs, two-pole ones composed of two in-phase or out-of-phase GSs, and vortex GSs, are found in this system. The dynamic properties of these solitons are studied by means of numerical simulations. Their stabilities are evaluated through linear stability analysis and direct perturbed simulation by the fourth-order Runge–Kutta method.

Fundamental and Two-Pole GSs. The profiles of fundamental and two-pole GSs are shown in Fig. 3. These solitons all present zero-vortex properties. For the fundamental case, the real part of wavefunction, Re(ψ), shows a single peak [Figs. 3(a) and 3(b)], while the imaginary part, Im(ψ), has a dipole form [Fig. 3(c)]. By changing the system parameters, two modes of two-pole GSs, the in-phase and out-of-phase ones, are found. Both the real and imaginary parts of wavefunctions have two poles. The main difference between the two modes of two-pole GSs is the directions of the dipoles of Re(ψ). For the out-of-phase mode, Re(ψ) has one positive and one negative pole [Fig. 3(d)]; while the in-phase case in Fig. 3(g) has two positive poles. The formation of these two kinds of solitons can be modulated and switched by changing the system parameters, such as propagation coefficient b, local nonlinearity coefficient γ, and nonlocal nonlinearity coefficient α.

Fig. Fig. 3. Profiles of zero-vortex solitons. (a)–(c) Fundamental GSs. (d)–(f) Two-pole GSs grouped as two out-of-phase fundamental GSs. (g)–(i) Two-pole GSs grouped as two in-phase fundamental GSs. The first and second columns show the distribution of the real part of wavefunctions ψ and their contour plots. The third column shows the distribution of the imaginary part of ψ. Parameters are b = 6, γ = 1, α = 2.5 for the fundamental GSs, b = 3.1, γ = 2.5, α = 5 for the out-of-phase mode, b = 4, γ = 2.5, α = 5 for the in-phase case. Parameters of moiré lattices are θ = arctan (3/4), V₀ = 0.02, V₁ = V₂ = 1.

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The modulation of fundamental and two-pole GSs are shown in Fig. 4. The light intensity, U = ∫ |ψ|²dr, as a function of propagation coefficient b is shown in Fig. 4(a). The U(b) relation does not meet an ‘anti-Vakhitov–Kolokolov’ (anti-VK) criterion, dU/db > 0, a necessary but not a sufficient condition for the stability of solitons in periodic structures with repulsive local nonlinearity.^[41] The stable zone of fundamental GSs is much larger than that of two-pole ones. For the two-pole GSs, the stable zone is divided into three parts: 2.5 < b < 2.99, 3.0 < b < 3.21, and 3.21 < b < 5.0. In the first and third parts (red solid lines), the solitons have the in-phase mode, while in the second part (green dotted line), the solitons take the out-of-phase mode. It is noted that the stable zone of two-pole GSs with out-of-phase mode is very small and nearly depressed to a point. In Fig. 4(b), it is found that U decreases monotonously with α for the fundamental and two-pole GSs with in-phase mode, while only four points, α = 3.4, 3.47, 3.5, 5, have stable out-of-phase mode. It is relatively hard to obtain the out-of-phase mode as this kind of solitons would collapse even with a subtle derivation of the specific values. This phenomenon is also found when changing other parameters, such as V₀ and p, which are shown in Figs. 4(c) and 4(d). For the out-of-phase mode, due to the interference of the two opposite components, the wavefunction cannot maintain stably easily. Only at finite states, the out-of-phase GS can be obtained. The potential applications of this effect is the encryption and decryption of signals by the parameters of these finite states.

Fig. Fig. 4. Modulation of fundamental and two-pole GSs. [(a), (b), (c), (d)] The light intensity U with respect to the propagation coefficient b, the nonlocal nonlinearity coefficient α, imaginary potential strength V₀, and lattice strength ratio p, respectively. The blue, red, and green lines represent the fundamental GSs, and two-pole GSs with in-phase and out-of-phase modes, respectively. The solid and dashed lines represent the stable and unstable states. Other parameters are the same as those in Fig. 3.

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The imaginary strength V₀ and the lattice strength ratio p are tuned in order to study the roles of the PT-symmetric moiré lattices in the system. It is found that the light intensity of solitons increases slowly with the increasing V₀, as shown in Fig. 4(c). When changing the lattice strength ratio p, the fundamental GSs have a large stable zone, while the two-pole GSs, including in-phase and out-of-phase modes, are stable only when p = 1, as shown in Fig. 4(d).

According to the above discussions, one finds that the stable zones for the three kinds of zero-vortex solitons are dramatically different. The stable zone of the fundamental GSs is much larger and can be obtained much easier. On the other hand, the stable zones of two-pole GSs are smaller. Especially the stable zone of the out-of-phase mode is so narrow that we can only get it with specific dots. The points a (b = 6, γ = 1, α = 2.5), b (b = 3.1, γ = 2.5, α = 5), and c (b = 4, γ = 2.5, α = 5) give each of the stable states of fundamental GSs, out-of-phase and in-phase modes, respectively. The moiré lattices parameters of the three points are θ = arctan (3/4), V₀ = 0.02, and p = 1.

Vortex Solitons. Besides the zero-vortex soliton, vortex ones are also found in this work. The profiles of the real part and imaginary parts and the corresponding phase structures are shown in Figs. 5(a), 5(b), 5(c), and 5(d). One finds that both the real and imaginary parts of the vortex solitons have dipole features, one has a positive value and the other has a negative value, which is similar to the two-pole GSs with out-of-phase mode. The main difference between the two cases is the phase structure. Evidently, the phase in Fig. 5(d) has vortex features. The dipole feature of real and imaginary parts of ψ may be explained by the unique structure of PT-symmetric potential, together with the localized and non-localized band structures that arise from the periodic moiré lattices.

Fig. Fig. 5. Vortex solitons. [(a), (b)] The real and imaginary parts of the wavefunction ψ, respectively. (c) The contour plot of Re(ψ). (d) The phase structure of wavefunction. (e)–(h) The modulation of the light intensity U by tuning the propagation coefficient b, the nonlocal nonlinearity coefficient α, imaginary potential strength V₀, and lattice strength ratio p. The fixed parameters are b = 4, γ = 2.5, α = 7, V₀ = 0.02, and p = 1.

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The stability of vortex solitons is evaluated by the linear stability analysis. The light intensity U with respect to the propagation coefficient b shows a positive slope [Fig. 5(e)]. It is found that the light intensity has simple relations with parameters: decreasing monotonously with the local nonlinear coefficient α [Fig. 5(f)], and increasing monotonously with imaginary lattice strength V₀ [Fig. 5(g)]. However, when changing the lattice strength ratio p, the vortex solitons have two narrow stable zones, 0 < p < 0.06 and 0.82 < p < 1.0 [Fig. 5(h)].

Dynamics of GSs. The stability of all the 2D localized solitons, including the fundamental GSs, two-pole GSs, and vortex solitons, have been performed by the perturbed evolution and linear-stability analysis.^[27] The perturbed evolutions of fundamental GSs and two-pole GSs with in-phase mode are shown in Figs. 6(a), 6(e), 6(i) and Figs. 6(c), 6(g), 6(k), respectively. One can see that they are stable, in good agreement with their linear eigenvalue spectra produced by linear-stability analysis (Re(λ) = 0). However, the two-pole GSs with out-of-phase mode [Figs. 6(c), 6(g), 6(k)] and vortex GSs [Figs. 6(d), 6(h), 6(j)] are unstable during the propagation, agreeing with the linear-stability analysis (Re(λ) ≠ 0).

Fig. Fig. 6. Profiles of fundamental GSs (a), two-pole GSs with out-of-phase (b) and in-phase (c), vortex solitons (d). The corresponding perturbed evolutions [(e), (f), (g), (h)] and linear eigenvalue spectra for each case are shown in the second and third rows, respectively.

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In summary, we have addressed a scheme to generate stable 2D solitons in a cold Rydberg atomic system with PT-symmetric moiré optical lattices. The formation, properties, and dynamics of fundamental, two-pole with in-phase and out-of-phase modes, and vortical GSs are studied numerically. It is realized that the PT symmetry, the degree of local and nonlocal nonlinearity can be used to control solitons. The stability regions of the localized modes are inspected by linear-stability analysis and perturbed evolution with direct simulations. It is found that the stable domains vary considerably with the changing of system parameters. The GSs in the Rydberg-dressed PT-symmetric moiré lattices system could keep being stable owing to the localized band structures and the existence of band gaps. Our results provide an insightful understanding of solitons physics in combined versatile platforms of PT-symmetric systems and Rydberg–Rydberg interaction in cold gases.

Acknowledgments: This work was supported by the National Key Research and Development Program of China (Grant No. 2021YFA1400700), the National Natural Science Foundation of China (Grant Nos. 11774113 and 12022507), and the Fundamental Research Funds for the Central Universities (Grant No. 2019kfyRCPY111).

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