Introduction

The representative nonlinear Schrödinger (NLS) equation can be used to describe distinguishing wave phenomena arising in many nonlinear physical fields such as nonlinear optics, Bose-Einstein condensates (alias Gross-Pitaevskii equation), the deep ocean, DNA, plasmas physics and even financial market, etc.1,2,3,4,5,6,7,8,9. The dynamics of fundamental bright and dark solitons (also vortices and light bullets in higher-dimensional cases) of the NLS model and self-similar modes in its generalized forms have been addressed (see refs 10, 11, 12, 13, 14, 15, 16, 17 and references therein). Recently, inspired by the non-Hermitian -symmetric potentials first suggested by Bender and Boettcher18,19 in the classical Hamiltonian operators, Musslimani et al.20 first introduced the complex -symmetric potentials in the NLS model such that some novel phenomena with stable modes were found. After that, a variety of distinguishing -symmetric or non--symmetric potentials were introduced to the continuous or discrete NLS equations to explore dynamical behaviors of -symmetric nonlinear modes (see, e.g., refs 21, 22, 23, 24, 25, 26, 27, 28, 29, 30, 31, 32, 33, 34, 35, 36, 37, 38, 39, 40, 41, 42 and references therein). Meanwhile, more and more physical experiments have also been designed to observe new wave phenomena in the sense of non-Hermitian -symmetric potentials43,44,45,46,47,48. Here the parity and temporal operators are defined as19: , and , , . The one-dimensional complex potential U(x) is -symmetric provided that the sufficient (not necessary) conditions UR(x) = UR(−x) and UI(−x) = −UI(x) hold19, where U(x) is also called the refractive-index in optical fibre.

In the study of ultra-short (e.g., 100 fs1) optical pulse propagation, the higher-order dispersive and nonlinear effects become significant such as third-order dispersion (TOD), self-steepening (SS) and the self-frequency shift (SFS) arising from the stimulated Raman scattering. The third-order NLS equation was introduced from the Maxwell equation49,50. The generalized inhomogeneous third-order NLS equation with modulating coefficients in the complex gain-or-loss term has been verified to admit optical rogue waves51. Recently, the NLS equation with only third-order dispersion was used to numerically confirm the experimental observation of the spectral signature of the collision between a soliton and the dispersive wave52. To our best knowledge, the -symmetric linear and nonlinear modes in the third-order NLS equation were not studied before. Our aim in this paper is to investigate the linear and nonlinear modes of the third-order NLS equation in the presence of physically interesting -symmetric potentials, e.g., Scarff-II-like potential and harmonic-Gaussian potential. We find that some parameters can modulate the stable nonlinear modes even if the linear -symmetric phases are broken. Moreover, we also understand that the adiabatic changes of control parameters can be used to excite the initial modes subject to exact bright solitons to generate stable nonlinear modes.

The rest of this report is arranged as follows. In Section of Results, we introduce the NLS equation with third-order dispersion in the presence of complex -symmetric potentials. We consider the nonlinear modes and their stability in the -symmetric Scarff-II-like and harmonic-Gaussian potentials. The problems of nonlinear modes excitations is also investigated, which can excite initial nonlinear modes to reach stable modes. Moreover, we also give some methods used in this paper. Finally, some conclusions and discussions are presented.

Results

Nonlinear wave model with -symmetric potentials

We focus on the generalized form of the third-order NLS equation52,53,54 in non-Hermitian potentials, that is, the NLS equation with third-order dispersion (TOD) and complex -symmetry potentials

where Raman effect, nonlinear dispersion terms (e.g., self-steepening term and self-frequency shift effect) and higher-order dispersion terms are neglected49,50,55,56, ψ ≡ ψ(x, z) is a complex wave function of x, z, z denotes the propagation distance, the real parameter β stands for the coefficient of TOD, the -symmetric potential requires that V(x) = V(−x) and W(x) = −W(−x) describing the real-valued external potential and gain-and-loss distribution, respectively and g > 0 (or <0) is real-valued inhomogeneous self-focusing (or defocusing) nonlinearity. The power of Eq. (1) is given by and one can readily know that . Equation (1) becomes the usual higher-order NLS equation in the absence of the gain-and-loss distribution53. Equation (1) with β = 0 becomes the -symmetric nonlinear model, which has been studied21,22,23,24,25,26,27,28,29,30,31,32,33,34,35,36,37,38,39,40. In the following we consider the case in the presence of TOD term (β ≠ 0) and gain-and-loss distribution. Here our following results are also suitable for the case x → t in Eq. (1).

Linear spectrum problem with -symmetric potential

We start to study the physically interesting potential in Eq. (1) as the -symmetric Scarff-II-like potential

where the real constant V0 and TOD parameter β can be used to modulate the amplitudes of the reflectionless potential V(x)57 and gain-and-loss distribution W(x), respectively. Moreover, V(x) and W(x) are both bounded (i.e., 0 < |V(x)| ≤ |V0|, ) with and V(x), W(x) → 0 as |x| → ∞ (see Fig. 1a). It is easy to see that the gain-and-loss distribution is always balanced since and has only the limit effect on linear and nonlinear modes since W(x) ~ 0 as |x| > M > 0. The sole difference between the potential (2) and the usual Scraff-II potential58 is that the gain-and-loss distribution in Eq. (2) will more quickly approaches to zero than one (i.e., β sec h x tan h x) in Scarff-II potential for the same amplitudes.

Figure 1
figure 1

Linear spectrum problem.

(a) -symmetric potential (2) with V0 = −0.8, β = 1, (b) The phase transitions for the linear operator L (3) with -symmetric Scarff-II-like potentials (2). The domain of unbroken (broken) -symmetric phase is inside (outside) the domain in (V0, β)-space. (c) Real and (d) imaginary parts of the eigenvalues λ [see Eq. (3)] as functions of V0 for the -symmetric potential (2) at β = 0.1, in which the imaginary parts are almost zero. (e) Real and (f) imaginary parts of the eigenvalues λ [see Eq. (3)] as functions of β for the -symmetric potential (2) at V0 = −2.

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We firstly consider the linear spectrum problem (i.e., Eq. (1) with g = 0) in the -symmetric Scarff-II-like potential (2) and use the stationary solution transformation ψ(x, z) = Φ(x)e−iλz to yield

where λ and Φ(x) are the corresponding eigenvalue and eigenfunction, respectively and lim|x|→∞Φ(x) = 0. Since the discrete spectrum of a complex -symmetric potential is either real or appears in complex conjugated pairs, thus we may find some proper parameters V0, β for which the complex -symmetric potential keep unbroken.

Here we consider V0 < 0 such that the shape of potential V(x) seems to be V-shaped with zero boundary conditions (see Fig. 1a). We numerically study the discrete spectra of the operator L (see Methods). Figure 1b exhibits the regions of broken and unbroken -symmetric phases on the (V0, β) space. Two almost parallel straight lines (β ≈ ±0.12) separate the limited space {(V0, β)|−0.02 ≤ V0 ≤ −3, |β| ≤ 0.5}. The regions of broken and unbroken -symmetric phases are outside and inside between two lines, respectively. For the given TOD parameter β = 0.1 and varying V0, the spontaneous symmetry breaking does not occur from the two lowest states since the maximum absolute value of imaginary parts of λ is less than 6 × 10−14 and they can be regarded as zero (see Fig. 1(c,d)). However, for the given V0 = −2 and varying β, the spontaneous symmetry breaking occurs from two lowest states starting from some β = 0.12 (see Fig. 1(e,f)).

Nonlinear localized modes and stability

For the given -symmetric Scarff-II-like potential (2), based on some transformations, we can find the unified analytical bright solitons of Eq. (1) for both the self-focusing and defocusing cases (see Methods)

where the phase wavenumber is defined by TOD coefficient with v = ±1, the potential is μ = (3κ2 + 3βκ − βκ3 − 3)/6 and the existent condition g(V0 − κβ + 1) > 0 is required. For the signs of parameter v and nonlinearity g, we find the following four cases for the existent conditions of bright solitons (4) (let ): (i) v = −g = −1 and V0 > −α (i.e., the right-side domain of the hyperbola of one sheet V0 = −α on (V0, β)-space); (ii) v = g = −1 and V0 < −α (i.e., the left-side domain of the hyperbola of one sheet V0 = −α on (V0, β)-space); (iii) v = g = 1 and V0 > α (i.e., the right-side domain of the hyperbola of one sheet V0 = α on (V0, β)-space); (iv) v = −g = 1 and V0 < α (i.e., the left-side domain of the hyperbola of one sheet V0 = α on (V0, β)-space).

In the following we numerically59 study the robustness (linear stability) of nonlinear localized modes (4) for both self-focusing and defocusing cases (g = ±1) via the direct propagation of the initially stationary state (4) with a noise perturbation of order about 2% in Fig. 2 (see Methods). Figure 2(a1) exhibits the stable and unstable (approximate) regions for Case (i) v = −g = −1 and different parameters V0 and β. For V0 = −0.8, β = 0.1 belonging to the domain of the unbroken linear -symmetric phase [cf. Eq. (3) and Fig. 1b], the stable nonlinear mode is generated (see Fig. 2(a2)). For the fixed V0 = −0.8, if we change β = 1.1 corresponding to the domain of the broken linear -symmetric phase, then a stable nonlinear mode is found too, that is, the focusing nonlinear term can modulate the unstable linear modes (broken -symmetric phase) to stable nonlinear modes (see Fig. 2(a3)). But if β increases a little bit (e.g., β = 1.5), then the nonlinear mode becomes unstable (see Fig. 2(a4)). In particular, for V0 = −1.1, β = 0.7, which does not satisfy the required existent condition of solution V0 > −α, that is, the expression (4) for this case, , is not an analytical solution of Eq. (1), but we still use it as the initial solution with a noise perturbation of order 2% to make numerical simulations such that we find the initial mode ϕ0(x, 0) can be excited to a stable and weakly oscillatory (breather-like behavior) situation (see Fig. 2(a5)). For Case (ii) v = g = −1, we also have the similar results (see Fig. 2(b3–b5)). For the last two Cases (iii) and (iv), we fix V0 > 0, in which the potential is similar to a Gaussian-like profile and the linear problem (3) has no discrete spectra, but we still find the stable nonlinear modes (see Fig. 2(c3–c5)) and unstable (see Fig. 2(c2) nonlinear modes.

Figure 2
figure 2

Stability of nonlinear modes (4).

(a1–a5) v = −g = −1, (a1) stable and unstable regions [the maximal absolute value of imaginary parts of the linearized eigenvalue δ on (V0, β) space (common logarithmic scale), similarly hereinafter], (a2) V0 = −0.8, β = 0.1 (stable), (a3) V0 = −0.8, β = 1.1 (stable), (a4) V0 = −0.8, β = 1.5 (unstable), (a5) V0 = −1.1, β = 0.7 (periodically varying); (b1–b5) v = g = −1, (b2) V0 = −1.5, β = 0.1 (stable), (b3) V0 = −1.5, β = 1.9 (stable), (b4) V0 = −1.5, β = 2 (unstable), (b5) V0 = −0.9, β = 0.2 (stable); (c1–c5) v = g = 1, (c2) V0 = 1.2, β = 0.1 (unstable), (c3) V0 = 1.2, β = 1 (stable), (c4) V0 = 1.2, β = 1.2 (periodically varying), (c5) V0 = 0.9, β = 0.2 (stable); (d1–d5) v = −g = 1, (d2) V0 = 0.8, β = 0.1 (unstable), (d3) V0 = 0.8, β = 1 (stable), (d4) V0 = 0.8, β = 1.1 (unstable), (d5) V0 = 1.1, β = 0.7 (stable).

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For the above-obtained nonlinear modes (4), we have the corresponding transverse power-flow or Poynting vector given by with (V0 − κβ + 1)/g > 0 and . We here consider the only case β > 0 (the case β < 0 can also be considered). For v = 1 (or −1), we have S > 0 (or <0), which implies that the pamaeter v change the directions of power flows from gain to loss regions. The power of the solutions (4) is , which is conserved.

Interactions of bright solitons

We here study the interactions of two bright solitons in the -symmetric potential. For the defocusing case g = −1, if we choose V0 = 1.1, β = v = 1 and consider the initial condition with ϕ(x, 0) given by Eq. (4) such that the elastic interaction is generated (see Fig. 3a). If we choose V0 = −1.5, β = 0.1, v = −1 and consider the initial condition with ϕ(x, 0) given by Eq. (4) such that the elastic interaction is generated (see Fig. 3c). For the self-focusing case g = 1, if we choose V0 = 1.2, β = v = 1 and consider the initial condition with ϕ(x, 0) given by Eq. (4) such that the elastic interaction is generated (see Fig. 3b). If we choose V0 = −0.8, β = 0.1, v = −1 and consider the initial condition with ϕ(x, 0) given by Eq. (4) such that the elastic interaction is generated (see Fig. 3d).

Figure 3
figure 3

The interactions of bright solitons (4) of

Eq. (1) . (a) V0 = 1.1, β = v = −g = 1, (b) V0 = 1.2, g = β = v = 1, (c) g = v = −1, V0 = −1.5, β = 0.1, (d) g = −v = 1, V0 = −0.8, β = 0.1.

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Exciting stable nonlinear localized modes in equation (1)

Nowadays we turn to the excitation of nonlinear modes by means of a slow change of the control TOD parameter β → β(z) in Eq. (1) which is regarded as a function of propagation distance z, that is, we focus on simultaneous adiabatic switching on the TOD and gain-and-loss distribution, modeled by

where V(x), W(x) are given by Eq. (2) with β → β(z) and β(z) is chosen as

with β1,2 being real constants. It is easy to see that the solutions (4) with β → β(z) do not satisfy Eq. (5), but for z = 0 and z ≥ 1000 solutions (4) indeed satisfy Eq. (5).

Figure 4 displays the wave propagation of the solutions ψ(x, z) of Eq. (5) subject to the initial condition given by Eq. (4) with β → β(z) given by Eq. (6). For v = 1 and different parameters g, V0, β1,2, Fig. 4(a–c) exhibit the stable modes in which the initial states |ψ(x, 0)|2 given by Eq. (4) with z = 0, β = β1 are all of the higher amplitudes and then the amplitudes decrease slowly as z increases such that they reach the alternative stable sates beginning from about z = 1000. For v = −1 and different parameters g, V0, β1,2, Fig. 4(e,f) also exhibit the stable modes in which the initial states are all of the lower amplitudes and then the amplitudes grow step and step as z increases such that they reach the stable and weakly oscillatory (breather-like behavior) situations beginning from about z = 1000, but Fig. 4d shows that the stable mode keeps from z = 0 to z = 1100 and then the wave slowly increases a little bit to reach another stable and weakly oscillatory (breather-like behavior) feature. In particular, in Fig. 4(b,f), we can excite the initial states subject to inexact solitons (4) of Eq. (1) for v = −g = 1, V0 = 0.8, β = 0.7 (or v = −g = −1, V0 = −1.1, β = 0.7) to the stable states subject to exact solitons (4) of Eq. (1) for v = −g = 1, V0 = 0.8, β = 1 (or v = −g = −1, V0 = −1.1, β = 0.8 of Eq. (1)).

Figure 4
figure 4

Exciting stable nonlinear localized modes [cf.

Eq. (5) ]. (a) v = −g = 1, V0 = 0.8, β1 = 0.4, β2 = 0.1, (b) v = −g = 1, V0 = 0.8, β1 = 0.7, β2 = 0.3, (c) v = g = 1, V0 = 1.2, β1 = 0.5, β2 = 0.1, (d) v = g = −1, V0 = −1.5, β1 = 0.6, β2 = 0.1, (e) v = −g = −1, V0 = −0.8, β1 = 1, β2 = 0.1, (f) v = −g = −1, V0 = −1.1, β1 = 0.7, β2 = 0.1.

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Nonlinear model with the spatially varying TOD

We here consider nonlinear modes of the generalized form of Eq. (1) with x-spatially varying TOD coefficient β → β(x), that is,

We here are interested in the TOD coefficient β(x) of a Gaussian function

with β0 ≠ 0 being a real amplitude of the Gaussian profile and another complex -symmetric harmonic-Gaussian potential

in which β = β(x) is given by Eq. (8) and we have introduced the function with σ ≠ 0 being a real constant. In fact, we can also consider the general case β(x). We know that the potential V(x) approaches to the harmonic potential x2/2 (which is related to the usual physical experiments) and W(x) → 0 as |x| → ∞ (see Fig. 6(b,d)).

Figure 6
figure 6

Stability and dynamical behaviors with g = 1.

(a) stable and unstable regions, (b) -symmetric potential with sing-well σ = β0 = 0.1, (c) stable nonlinear mode for σ = β0 = 0.1 (linear unbroken -symmetric phase), (d) -symmetric potential with double-well σ = 0.1, β0 = 1, (e) stable nonlinear mode for σ = 0.1, β0 = 1 (linear broken -symmetric phase).

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For the given -symmetric harmonic-Gaussian potential (9), we studied the discrete spectra of linear problem (3) such that we give the separated regions for the broken and unbroken -symmetric phase (see Fig. 5(a)). When |σ| is greater than about 0.16, we only find the discrete spectra for β0 very approaching to zero (here we consider |β0| ≤ 0.3). For the given amplitude β0 = 0.1 of TOD coefficient, we give the first six lowest eigenvalues (see Fig. 5(b,c)), where the spontaneous symmetry breaking occurs from the two lowest states.

Figure 5
figure 5

Linear spectrum problem.

(a) The phase transitions for the linear operator L (3) with -symmetric harmonic-Gaussian potential (9). The unbroken (broken) -symmetric phase is in the domain inside (outside) the almost rectangle domain on (σ, β0)-space. (b) Real and (c) imaginary parts of the eigenvalues λ [see Eq. (3)] as functions of σ for the -symmetric potential (9) at β0 = 0.1.

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We find the exactly analytical solutions of Eq. (7) with the Gaussian TOD coefficient in the -symmetric harmonic-Gaussian potential (9) in the form

where g > 0 and erf(·) is an error function. In the following we take g = 1 without loss of generality.

In what follows we numerically investigate the robustness (linear stability) of nonlinear localized modes (10) for self-focusing case (g = 1) via the direct propagation of the initially stationary state (10) with a noise perturbation of order about 2% in Fig. 6 (see Methods). The linear stability of the solutions (10) is displayed in Fig. 6a) such that we find the solutions (10) are possibly stable nearby σ = 0. For σ = β0 = 0.1, in which the potential becomes almost a harmonic potential x2/2 (see Fig. 6b), we find the stable nonlinear mode (see Fig. 6c). But for σ = 0.2, β0 = 0.35, in which the potential is a double-well potential (see Fig. 6d), we also obtain the stable nonlinear mode (see Fig. 6e).

For the above-obtained nonlinear modes (10), we have the corresponding transverse power-flow or Poynting vector given by , which implies that sgn(S) = sgn(σ). Since the gain-and-loss distribution W(x) given by Eq. (9) depends on TOD parameter β0 and σ, which generate that there are more one intervals for gain (or loss) distribution, thus though the power flows along the positive (negative) direction for the x axis as σ > 0 (<0), it is of the complicated structures from the gain-and-loss view.

Moreover, we also study the interactions of two bright solitons in the -symmetric potential. For the focusing case g = 1, if we choose σ = −0.1, β0 = 0.1 and consider the initial condition with ϕ(x, 0) given by Eq. (10) such that the elastic interaction is generated (see Fig. 7(a)). If we choose σ = 0.2, β0 = 0.1 and consider the initial condition with ϕ(x, 0) given by Eq. (10) such that the elastic interaction is generated too (see Fig. 7(b)).

Figure 7
figure 7

The interactions of bright solitons (10) of

Eq. (5) . (a) σ = −0.1, (b) σ = 0.2. Other parameters are g = 1, β0 = 0.1.

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Nowadays we turn to the excitation of nonlinear modes by means of a slow change of the control TOD parameter β(x) → β(x, z) in Eq. (5) whose amplitude β0 is regarded as a function of propagation distance z, that is, we focus on simultaneous adiabatic switching on the TOD, potential and gain-and-loss distribution.

For the given σ = 0.1, we consider the varying amplitude β0 → β0(z) in Eq. (8) in the form

which makes the TOD coefficient given by Eq. (8), potential V(x) and gain-or-loss distribution W(x) given by Eq. (9) change, but it does not change the expression of solutions (10). Now we study the wave evolution of the solution ψ(x, z) satisfied by Eq. (5) with Eqs (8), (9) and (11) subject to the initial condition given by Eq. (10). As a consequence, we find the stable nonlinear modes by using the excitation (11), that is, we can steadily excite one stable mode (Fig. 6(c)) to reach another stable one (Fig. 6(e)), which is exhibited in Fig. 8(a).

Figure 8
figure 8

Exciting stable nonlinear localized modes.

(a) σ = 0.1 and β0(z) given by Eq. (11), (b) β0 = 0.1 and σ(z) given by Eq. (12), (c) β0(z) and σ(z) given by Eqs (11) and (12).

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Now we fix the amplitude of TOD, β0 = 0.1 and consider the effect of varying amplitude σ → σ(z) on nonlinear modes:

which makes the potential V(x) and gain-or-loss distribution W(x) given by Eq. (9) and solutions (10) change, but it does not change the TOD coefficient given by Eq. (8). We consider the wave evolution of the solution ψ(x, z) satisfied by Eq. (5) with Eqs (8), (9) and (12) subject to the initial condition given by Eq. (10) such that we find the stable nonlinear modes by using the excitation, that is, we can smoothly excite one stable mode (see Fig. 6(c)) to another stable mode (see Fig. 8(b)). Moreover, if we simultaneously consider the effect of varying β0(z) and σ(z) given by Eqs (11) and (12) then we also find the similar result (see Fig. 8(c)).

Discussion

In conclusions, we have introduced some non-Hermitian (e.g., complex -symmetric) potentials in the nonlinear Schrödinger equation with third-order dispersion. For the chosen physically interesting -symmetric Scarff-II-like and harmonic-Gaussian potentials, we found exact analytical bright solitons of this equation. In the presence of these -symmetric potentials, we study the broken and unbroken of -symmetric phases of the corresponding linear problem (third-order linear operator with complex potentials) for TOD and potential parameters such that we find the TOD parameter has a strong effect on the spectra (it only admit a few discrete spectra). We have studied the linear stability of exact bright solitons. In particular, we find the stable nonlinear modes for some control parameters for which even if the corresponding linear -symmetric phase is broken. Moreover, we also investigate the problems of nonlinear modes excitations, which can excite initial nonlinear modes to reach stable modes. The method in this paper can also be extended to explore other higher-order or/and higher-dimensional NLS equations in the presence of non-Hermitian potentials and may open a new window to investigate similar problems. Our results may be useful to provide theoretical researchers and experimental scientists with more new data about the -symmetric nonlinear modes in higher-order nonlinear wave models.

Methods

Linear spectrum problem

For Eq. (1) in the absence of nonlinear term (g = 0), we assume that ψ(x, z) = Φ(x)e−iλz, then we have Eq. (3), which with the -symmetric potential (2), as |x| → ∞, reduces to , whose characteristic equation is , whose roots, in general, are complex numbers and complicated. For example, if λ = 1/(3β2) and β > 0 (without loss of generality), we have its three roots Λ1 = i/β, , which probably lead to the result that the corresponding eigenfunctions should satisfy periodic boundary conditions. Additionally, if β depends on the space x, e.g., β(x) = β0 exp(−x2) and V(x), W(x) are given by Eq. (9), then we have β(x), W(x) → 0 and V(x) → x2/2 as |x| → ∞. Thus for this case Eq. (3) reduces to as |x| → ∞, where the condition is used and we have the asymptotic solutions . Based on the standard conditions of wave function, we only take , which generally corresponds to zero boundary conditions and discrete spectra. Therefore, in order to verify these results, we use the Fourier collocation method59,60,61 to numerically study the above-mentioned linear spectrum problems and obtain the agreeable conclusions as ones by the theoretical analysis.

Nonlinear stationary modes

We consider the stationary solutions of Eq. (1) in the form ψ(x, z) = ϕ(x)e−iμz, where ϕ(x) is a complex field function and μ the corresponding propagation constant. We have . To study nonlinear modes of this equation we assume that with ρ(x) and φ(x) being real functions and separate the real and imaginary parts to yield

For the given -symmetric potential (2) we can find the exact bright solitons (4) of Eq. (1). Similarly, we can also find the solutions of Eq. (5) in the -symmetric potential (9).

Linear stability of nonlinear stationary modes

To further study the linear stability of the above-obtained nonlinear stationary solutions ψ(x, z) = ϕ(x)e−iμz of Eq. (1), we considered a perturbed solution59,62 , where , δ and F(x) and G(x) are the eigenvalue and eigenfunctions of the linearized eigenvalue problem. We substitute the expression into Eq. (1) and linearize it with respect to ϵ to yield the following linear eigenvalue problem

where . It is easy to see that the -symmetric nonlinear modes are linearly stable if δ has no imaginary component, otherwise they are linearly unstable.

Additional Information

How to cite this article: Chen, Y. and Yan, Z. Solitonic dynamics and excitations of the nonlinear SchrÖedinger equation with third-order dispersion in non-Hermitian -symmetric potentials. Sci. Rep. 6, 23478; doi: 10.1038/srep23478 (2016).