# Exact Solutions to the Nonlinear Schrödinger Equation with Time-Dependent Coefficients

Authors: Xin-Lei Mai; Wei Li; Shi-Hai Dong
Journal: Advances in High Energy Physics
 (2021)

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## Abstract

In this paper, a trial function method is employed to find exact solutions to the nonlinear Schrödinger equations with high-order time-dependent coefficients. This system might be used to describe the propagation of ultrashort optical pulses in nonlinear optical fibers, with self-steepening and self-frequency shift effects. The new general solutions are found for the general casea0≠0 including the Jacobi elliptic function solutions, solitary wave solutions, and rational function solutions which are presented in comparison with the previous ones obtained by Triki and Wazwaz, who only studied the special case a0=0.


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## Body

## 1. Introduction

It is well known that many physical phenomena can be described by a nonlinear Schrödinger equation (NLSE), which is found in many diverse fields such as plasma physics [1], fluid dynamics [2], nonlinear optics [3], quantum mechanics [4], hydrodynamics [5], and biology. Thus, finding the exact solutions to the NLSE has an important theoretical and practical significance in understanding the physical phenomena described by the NLSE.Recently, some useful and powerful methods have been proposed to explore its exact solutions. For example, these methods include the homogeneous balance method [6], the tanh function expansion method and its extension [7], the sine-cosine methods [7], the exp-function method [7], the multiple exp-function method [8], the first integral method [9], the Jacobi elliptic function expansion method [10], the sub-ODE method [11], the G′/G-expansion method [12], the modified simple equation method [13], the extended auxiliary equation method [14], the exp−ϕξ-expansion method [15], and the trial function method and its generalization [16].It should be recognized that most of the methods mentioned above are related to constant coefficient models. Undoubtedly, it becomes more difficult than those constant coefficient counterparts when we study the NLSE with time-dependent coefficients. Up to now, considerable attention has been paid to the varying coefficient NLSE, and many authors put forward different approaches [16–22]. Among them, Liu [21] proposed a trial function method to deal with both real and complex equations with varying coefficients. In this paper, we are going to apply Liu’s method to find the exact solutions of the following cubic-quintic NLSE with time-dependent coefficients:
(1)iqt+ftqxx+gtq2+σq4q=ihtq2qx+iptq2xq.qx,t will represent a different physical quantity when using it to describe different systems. For example, when the present equation with high-order dispersion and nonlinear terms describes the pulse transmission in the femtosecond state and considers the loss in the transmission process [17, 22], qx,t denotes the complex envelope of the electric field, x and t are the distance along the direction of propagation and time, respectively, ft is the dispersion coefficient, ht is the self-steepening coefficient, pt is the self-frequency shift coefficient, and σ is a constant. Green and Biswas [22] studied Equation (1) by using the ansatz method [23] and obtained the exact soliton solutions under some constraints on the parameters. Recently, one of the present authors has obtained analytical traveling-wave solutions to a generalized Gross-Pitaevskii (GP) equation [22] with some new time- and space-varying coefficients and external fields [24] because of their possible applications to the BECs [25–29]. Obviously, the current cubic-quintic NLSE is more complicated than the GP equation. It should be pointed out that all kinds of NLSEs with varying coefficients mentioned above [16–22] are different from Equation (1) except for reference [17], in which the authors only studied the particular case a0=0 using the direct but complicated integral approach.This paper is organized as follows. In “Exact Solutions,” we first apply the trial function method to obtain its exact solutions by using a suitable transformation, and then, we illustrate the shapes of the wave amplitude of different solutions by taking appropriate parameters for those varying coefficients. Finally, in “Concluding Remarks,” we summarize the results found in this work.


## 2. Exact Solutions

Assume that the solution to Equation (1) is given by
(2)qx,t=uξeiη,ξ=ktx+wt,η=stx+rt,where kt, wt, st, and rt are undetermined parameters related to time. Substituting them into (1) and separating the real and the imaginary parts, one finds
(3)k′tx+w′t+2ftstktu′−3ht+2ptktu2u′=0,(4)ftk2tu″−s′tx+r′t+fts2tu+gt+htstu3+σgtu5=0.If the solution satisfies(5)u′2=Fξ=∑i=0maiui,where aii=0,⋯,m are constants and m is an integer to be determined (the value of m in Eq. (5) is determined as m=6 when using the homogeneous balance theory), then substituting (5) into (4) and setting each coefficient of u′, u2u′ in (3), and uii=1,3,5 in (4) to zero allow us to obtain a set of algebraic equations as follows:
(6)k′tx+w′t+2ftstkt=0,3ht+2ptkt=0,a1=a3=a5=0,a2=s′tx+r′t+fts2tftk2t,a4=−gt+htst2ftk2t,a6=−σgt3ftk2t.Set(7)kt=k≠0,st=s≠0,rt=c1∫ftdt,gt=c2k2ft,ht=c3k2ft,a0=c4,where k, s, c1, c2, c3, and c4 are arbitrary constants, ft is an arbitrary function. In this work, we only consider three different cases, ft=1, ft=t, and ft=1/1+t, for simplicity. The other coefficients can be determined by the following forms:
(8)pt=−32c3k2ft,wt=−2sk∫ftdt,(9)a1=a3=a5=0,a2=c1+s2k2,a4=−c2+sc32,a6=−σc23.In terms of these coefficients (8), Equation (5) with m=6 is thus simplified as
(10)u′2=a0+a2u2+a4u4+a6u6.Before studying the general casea0≠0, let us first show the soliton solutions q=uξeiη for the special case a0=0 [17]:
(11)q=2a2εa42−4a2a6cosh2a2ξ−a41/2⋅eiη,a42−4a2a6>0,a2>0,brightsolitonsolution,2a2ε4a2a6−a42sinh2a2ξ−a41/2⋅eiη,a42−4a2a6<0,a2>0,singularsolitonsolution,−a2a41+εtanha22ξ1/2⋅eiη,a42−4a2a6=0,a2>0,darksolitonsolution,−a2a4sech2a2ξa42−a2a61+εtanha2ξ21/2⋅eiη,a2>0,ε=±1,brightsoliton‐likesolution.How to find the exact solution to the general casea0≠0 becomes the main purpose of this work. Applying a transformation φ=u−2 to Equation (10) enables us to obtain
(12)φ′=±2a0Gφ,Gφ=φ3+a2a0φ2+a4a0φ+a6a0.It is found that Equation (12) can be divided into three different cases depending on the factor Δ=B2−4AC by the Shengjin discrimination method, where the parameters A, B, and C are given by
(13)A=a22−3a0a4a02,B=a2a4−9a0a6a02,C=a42−3a2a6a02.Case 1.
Δ<0
In this case,Gφ=0 has three unequal roots, φ1<φ2<φ3: φ1=−a2/3a0−2Acosθ/3/3 and φ2,3=−a2/3a0+Acosθ/3±3sinθ/3/3, where θ=arccos2Aa2−3a0B/2a0A3. In terms of them, Equation (12) can be expressed as φ′=±2a0φ−φ1φ−φ2φ−φ3. According to the relation φ=u−2, a periodic wave solution qx,t=uξeiη of Equation (1) is found as
(14)q=1ϕ1cn2εa0ϕ3−ϕ1ξ,m1+ϕ2sn2εa0ϕ3−ϕ1ξ,m11/2⋅eiη,a0>0,snε−a0ϕ3−ϕ1ξ,m2ϕ1−ϕ3cn2ε−a0ϕ3−ϕ1ξ,m21/2⋅eiη,a0<0,where
(15)m1=ϕ2−ϕ1ϕ3−ϕ1,m2=ϕ3−ϕ2ϕ3−ϕ1.
To understand these solutions, we illustrate the shapes of the wave amplitude for three different cases,ft=1, ft=t, and ft=1/1+t, which are all periodic waves (k=s=1, a0=1, a2=−6, a4=11, a6=−6).Case 2.
Δ>0
Gφ=0 has a single root ϕ1=−a2/3a0−Y13+Y23/3, where Y1,2=Aa2/a0+3−B±B2−4AC/2. One has ϕ′=±2a0ϕ−ϕ1ϕ2+αϕ+β, where two parameters α and β are given by α=2a2/3a0−Y13+Y23/3 and β=Y13+Y23−2a2/a02/36+Y13−Y232/12, respectively. The periodic solutions including an elliptic function are explicitly expressed as
(16)q=1+cn2εa0ϕ12+αϕ1+β1/4ξ,m3ϕ1+ϕ12+αϕ1+β+ϕ1−ϕ12+αϕ1+βcn2εa0ϕ12+αϕ1+β1/4ξ,m31/2⋅eiη,a0>0,1+cn2ε−a0ϕ12+αϕ1+β1/4ξ,m4ϕ1−ϕ12+αϕ1+β+ϕ1+ϕ12+αϕ1+βcn2ε−a0ϕ12+αϕ1+β1/4ξ,m41/2⋅eiηa0<0,where
(17)m3=122−2φ1+αφ12+αφ1+β1/2,m4=122+2φ1+αφ12+αφ1+β1/2.
In similar way, the corresponding shapes of the wave amplitude are plotted in Figure1 (the parameters k=s=1, a0=1, a2=−1, a4=−1, and a6=−2 are chosen here). Notice that these sharp shapes are slightly different from those in Figure 2.Case 3.
Δ=0
A≠0
Gφ=0 has two roots, φ1=−B/2A and φ2=−a2/a0+B/A. It is known that Equation (12) can be transformed into ϕ′=±2a0ϕ−ϕ12ϕ−ϕ2, from which we are able to obtain the exact solutions to Equation (1).
(18)q=1ϕ2sec2a0ϕ2−ϕ1ξ−ϕ1tan2a0ϕ2−ϕ1ξ1/2⋅eiη,a0ϕ1<a0ϕ2,(19)q=1ϕ2sech2a0ϕ1−ϕ2ξ+ϕ1tanh2a0ϕ1−ϕ2ξ1/2⋅eiη,a0ϕ1>a0ϕ2.
For the casea0φ1<a0φ2, the shapes of the periodic wave amplitude are shown in Figure 3 (k=s=1, a0=1, a2=−4, a4=5, and a6=−2), which is very similar to those in Figure 1. For the case a0φ1>a0φ2 (a0>0), the shapes of the wave amplitude are displayed in Figure 4 (k=s=1, a0=1, a2=−5, a4=8, and a6=−4), which corresponds to a bright soliton wave. However, the case a0<0 generates a dark soliton wave as shown in Figure 5 (k=s=1, a0=−1, a2=4, a4=−5, and a6=2). These new and interesting phenomena do not appear in other cases due to the different signs of the parameter a0.
A=0 and B=0, i.e., a4=a22/3a0, a6=a23/27a02
Gφ=0 has three equal roots, φ1=−a2/3a0. The relation φ′=±2a0φ−φ13 enables us to obtain a rational function solution
(20)q=3a0ξ23−a2ξ21/2⋅eiη,which represents a singular solitary wave. The corresponding shapes of the wave amplitude are illustrated in Figure 6 (k=s=1, a0=1, a2=3, a4=3, and a6=1).Figure 1
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Figure 2
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Figure 3
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Figure 4
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Figure 5
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Figure 6
(a–c) The 3D wave shapes ofq: (a) ft=1, (b) ft=t, and (c) ft=1/1+t. (d) The wave propagates along the x-axis.
(a)(b)(c)(d)Before ending this section, we give a useful remark on these graphics. Comparing Figures2(a)–2(c), it is found that the amplitude is the same. This implies that the variable coefficient ft has no effect on the amplitude. We have the same conclusion for Figures 1 and 3–5, but the amplitude in Figure 6 is changed.


## 3. Concluding Remarks

In this paper, we investigated a kind of nonlinear Schrödinger equation with high-order time-dependent coefficients, which describes the propagation of ultrashort optical pulses in nonlinear optical fibers. The trial function method has been used to find general solutions such as the periodic solutions (14) and (16) including the Jacobi elliptic function, the periodic wave solutions (18) involving the trigonometric function, solitary wave solutions (19), and rational function solutions (20). To describe the properties of the solutions, three different functions, ft=1, ft=t, and ft=1/1+t, are chosen to show the shapes of the wave amplitudes. We summarize the main results as follows:
(1)
Forft=1, Figures 1(a), 2(a), and 3(a) show the shapes of the wave amplitude of the periodic wave solutions (14)-(18), respectively. Figures 4(a) and 5(a) display the case of the solitary wave solutions (19); Figure 4(a) shows the case of a bright soliton (a0>0), but Figure 5(a) illustrates the case of a dark soliton (a0<0). Figure 6(a) shows the wave shapes of the rational function solutions (20). By observing Figures 1(a), 2(a), 3(a), 4(a), 5(a), and 6(a), it is found that the velocity of the pulse remains constant during propagation because ft is a real constant(2)
For the caseft=t, the shapes of the wave amplitude of the periodic wave solutions (14)–(18) are shown in Figures 1(b), 2(b), and 3(b), respectively. The case of the solitary wave solutions (19) is plotted in Figures 4(b) and 5(b). For example, Figure 4(b) describes a bright soliton wave (a0>0), while Figure 5(b) corresponds to a dark soliton wave (a0<0). The shape of the wave amplitude of the rational function solutions (20) is illustrated in Figure 6(b). It can be found that the pulse propagation velocity has a parabolic feature by observing Figures 1(b), 2(b), 3(b), 4(b), 5(b), and 6(b).(3)
Forft=1/1+t, Figures 1(c), 2(c), and 3(c) describe the periodic wave solutions (14)–(18), respectively. Figures 4(c) and 5(c) show the case of the solitary wave solutions (19). For instance, Figure 4(c) represents a bright soliton wave (a0>0), but Figure 5(c) corresponds to a dark soliton wave (a0<0). Figure 6(c) shows the shapes of the wave amplitude of the rational function solutions (20). It is seen from Figures 1(c), 2(c), 3(c), 4(c), 5(c), and 6(c) that the pulse propagation has the feature of a logarithmic function.Before ending this work, we will make three useful remarks. First, it should be mentioned that the specific expressions of various exact solutions of the NLSE with varying coefficients also reflect the diversity of the solitary wave solutions. The existence of solitary wave solutions implies a perfect balance between the nonlinear effect and the dispersion effect, which usually requires peculiar conditions. Without doubt, this work will help us understand the physical phenomena described by Equation (1). Second, it is believed that the results such as optical solitons presented here will make a major impact in the area of nonlinear optics. The model which was used in this work for mathematical analysis gave the characteristics of stable solitary waves in the system. This confirms that the optical fiber described by the system can be transmitted stably for a long time. Third, the trial function method is also an effective and practical method for solving other kinds of nonlinear equations with varying coefficients.



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