Models of the coupled nonlinear Schr ödinger equations submit various critical physical phenomena with a typical equation for optical fibres with linear refraction. In this article, we will presuppose the Compact Finite Difference method with Runge-Kutta of order 4 (explicit) method, which is sixth-order and fourth-order in space and time respectively, to solve coupled nonlinear Schr ödinger equations. Many methods used to solve coupled nonlinear Schr ödinger equations are second order in time and need to use extra-technique to rise up to fourth-order as Richardson Extrapolation technique. The scheme obtained is immediately fourth-order in one step. This approach is a conditionally stable method. The conserved quantities and the exact single soliton solution indicate the competence and accuracy of the article’s suggestion schemes. Furthermore, the article discusses the two solitons interaction dynamics.
An enormous assortment of physical situations can be represented by the coupled nonlinear Schrödinger equations (CNLSEs). These equations have been exhibited in a fibre communication system to capture vibration diffusion over perpendicular polarization axes in nonlinear optical fibres and wavelength division of multiplexed systems. CNLSEs also model radiation inside photorefractive matter or crystals by modelling the radiation as water wave collision. Singular waves in these equations are overwhelmingly called vector solitons in the writing as singular waves, in general, consist of two components. In the previous physical situations, clashing vector solitons is a significant case. In the last decade, the system has been examined seriously. Studies have found that, in addition to crossing through the clash, vector solitons can also rebound each other or hinder one another. This article will present (CNLSEs) as the follows [
i Φ 1 t + 1 2 Φ 1 x x + ( | Φ 1 | 2 + c | Φ 2 | 2 ) Φ 1 = 0 , − ∞ < x < ∞ (1)
i Φ 2 t + 1 2 Φ 2 x x + ( c | Φ 1 | 2 + | Φ 2 | 2 ) Φ 2 = 0 , − ∞ < x < ∞ (2)
where Φ 1 and Φ 2 are the wave amplitudes in pair polarizations, and c is the cross-phase modulation coefficient. The initial conditions are:
Φ 1 ( x , 0 ) = ζ 1 ( x ) , Φ 2 ( x , 0 ) = ζ 2 ( x ) (3)
and the boundary conditions are
Φ 1 ( x , t ) = Φ 2 ( x , t ) = 0, as | x | → ∞ (4)
For linearly birefringent fibres c = 2 3 , and for elliptically birefringent fibres, c
is a positive number. When c = 0 , this system enhances two (decoupled) nonlinear Schrödinger equations (NLS), and when c = 1 , the system is a Manakov equations. In both situations, we get an integrable system. In particular, the solitons of one polarization should pass through the pulses of the opposite interaction’s polarization in the absence of forming shadows, creating an elastic collision. We have a nonintegrable system for other values of c. The clash may be nontrivial, and several complex phenomena like reflection, transmission, trapping, and creation of other solitary waves can happen. Solitons in optical fibres can be described as nonlinear beats that propagate nearly distortion-free, extending into the distance and undergoing (elastic) collision. The sixth-order compact finite difference method is perfect to derive the analytical solution of the CNLS system. We determined the exact solution of the CNLSEs as follows:
Φ 1 ( x , t ) = 2 α 1 + c sec h ( x − v 1 t ) exp i { v 1 x − [ v 1 2 2 − α ] t } ,
Φ 2 ( x , t ) = ± 2 α 1 + c sec h ( x − v 1 t ) exp i { v 1 x − [ v 1 2 2 − α ] t } ,
Several improved numerical methods have been presented for the nonlinear Schrödinger equations [
The conserved quantities of Equations (1) and (2) are follows [
1) Mass conservations:
I 1 = ∫ − ∞ ∞ | Φ 1 | 2 d x , (5)
I 2 = ∫ − ∞ ∞ | Φ 2 | 2 d x (6)
2) Energy conservations:
I 3 = ∫ − ∞ ∞ { ∑ j = 1 2 1 2 | ∂ Φ j ∂ x | 2 − 1 2 ∑ j = 1 2 | Φ j | 4 − c | Φ 1 | 2 | Φ 2 | 2 } d x . (7)
We suppose that, outside the interval x 0 ≤ x ≤ x M , the solution of the system (1) and (2) is negligible. Therefore, to study this system numerically, we prefer to consider the system
i ∂ Φ 1 ∂ t + 1 2 ∂ 2 Φ 1 ∂ x 2 + ( | Φ 1 | 2 + c | Φ 2 | 2 ) Φ 1 = 0 , x 0 < x < x M (8)
i ∂ Φ 2 ∂ t + 1 2 ∂ 2 Φ 2 ∂ x 2 + ( c | Φ 1 | 2 + | Φ 2 | 2 ) Φ 2 = 0 , x 0 < x < x M (9)
where Φ 1 and Φ 2 are the wave gage in two polarizations and the cross-phase modulation coefficient is c, with
Φ 1 ( x , 0 ) = ζ 1 ( x ) , Φ 2 ( x , 0 ) = ζ 2 ( x )
as initial conditions and
Φ 1 ( x , t ) = Φ 2 ( x , t ) = 0 , at x = x 0 and x = x M
as boundary conditions. To conclude the numerical method to solve 8 and 9, the rectangular mesh point with coordinates
x m = x 0 + m ( h ) , m = 0 , 1 , ⋯ , M ,
t n = n k , n = 0 , 1 , 2 , ⋯
which cover the region R = [ x 0 < x < x M ] × [ t > 0 ] . Numerically, we prefer to disjoint the complex functions Φ 1 and Φ 2 into their real and imaginary portions by
Φ 1 ( x , t ) = u 1 ( x , t ) + i u 2 ( x , t ) , Φ 2 ( x , t ) = u 3 ( x , t ) + i u 4 ( x , t ) (10)
where u i ( x , t ) , i = 1 , 2 , 3 , 4 are real functions, and we write,
u 1 ( x , 0 ) = ζ 1 R ( x ) , u 2 ( x , 0 ) = ζ 1 I ( x ) u 3 ( x , 0 ) = ζ 2 R ( x ) , u 4 ( x , 0 ) = ζ 2 I ( x ) (11)
where we have assumed
ζ 1 ( x ) = ζ 1 R + i ζ 1 I and ζ 2 ( x ) = ζ 2 R + i ζ 2 I
and ζ 1 R , ζ 1 I , ζ 1 R and ζ 1 I are all real functions.
By substituting (10) into (8) and (9), the next system is obtained:
1 2 ∂ 2 u 2 ∂ x 2 = − ∂ u 1 ∂ t − G 1 u 2 (12)
1 2 ∂ 2 u 1 ∂ x 2 = ∂ u 2 ∂ t − G 1 u 1 (13)
1 2 ∂ 2 u 4 ∂ x 2 = − ∂ u 3 ∂ t − G 2 u 4 (14)
1 2 ∂ 2 u 3 ∂ x 2 = ∂ u 4 ∂ t − G 2 u 3 (15)
The previous system in a matrix-vector is
∂ u ∂ t + 1 2 A ∂ 2 u ∂ x 2 + F ( u ) u = 0 (16)
where
u = [ u 1 u 2 u 3 u 4 ] , A = [ 0 1 0 0 − 1 0 0 0 0 0 0 1 0 0 − 1 0 ] , F ( u ) = [ 0 G 0 0 − G 0 0 0 0 0 0 G 0 0 − G 0 ] .
At the grid point ( x m , t n ) , the exact solution is denoted by u i , m n while the numerical one is denoted with U i , m n . The Compact Finite Difference (CFD) formula is derived by [
α ( ∂ 2 u i ∂ x 2 ) m − 1 + ( ∂ 2 u i ∂ x 2 ) m + α ( ∂ 2 u i ∂ x 2 ) m + 1 = b 4 h 2 δ x ^ 2 U i , m + a h 2 δ x 2 U i , m (17)
where
δ x 2 U i , m = U i , m + 1 − 2 U i , m + U i , m − 1 ,
δ x ^ 2 U i , m = U i , m + 2 − 2 U i , m + U i , m − 2 , i = 1 , 2 , 3 , 4.
Now, by Taylor Expansion, we can have the truncation error as the following [
R ≡ ( 2 α + 1 − b − a ) ( ∂ 2 u i ∂ x 2 ) m + ( α − 1 3 b − 1 12 a ) h 2 ( ∂ 4 u i ∂ x 4 ) m + ( 1 12 α − 2 45 b − 1 360 a ) h 4 ( ∂ 6 u i ∂ x 6 ) m
if we solve ( 2 α + 1 − b − a ) = 0 and ( α − 1 3 b − 1 12 a ) = 0 , we get
a = 4 3 ( 1 − α ) and b = 1 3 ( 10 α − 1 )
so the truncation error becomes
R ≡ − 4 6 ! ( 11 α − 2 ) h 4 ( ∂ 6 u i ∂ x 6 ) m + O ( h 6 )
If α = 0 then a = 4 3 and b = − 1 3 , which gives the explicit scheme in order four for the second derivative. Furthermore, when α = 2 11 , the scheme becomes sixth-order accurate, in this case a = 12 11 and b = 3 11 .
By using (12)-(15), Equations (17) can be written as
− α ( ∂ u 1 ∂ t + G u ) m − 1 − ( ∂ u 1 ∂ t + G u ) m − α ( ∂ u 1 ∂ t + G u ) m + 1 = 1 2 [ b 4 h 2 δ x ^ 2 U 2 , m + a h 2 δ x 2 U 2 , m ] (18)
α ( ∂ u 2 ∂ t − G u 1 ) m − 1 + ( ∂ u 2 ∂ t − G u 1 ) m + α ( ∂ u 2 ∂ t − G u 1 ) m + 1 = 1 2 [ b 4 h 2 δ x ^ 2 U 1 , m + a h 2 δ x 2 U 1 , m ] (19)
− α ( ∂ u 3 ∂ t + G u 4 ) m − 1 − ( ∂ u 3 ∂ t + G u 4 ) m − α ( ∂ u 3 ∂ t + G u 4 ) m + 1 = 1 2 [ b 4 h 2 δ x ^ 2 U 4 , m + a h 2 δ x 2 U 4 , m ] (20)
α ( ∂ u 4 ∂ t − G u 3 ) m − 1 + ( ∂ u 4 ∂ t − G u 3 ) m + α ( ∂ u 4 ∂ t − G u 3 ) m + 1 = 1 2 [ b 4 h 2 δ x ^ 2 U 3 , m + a h 2 δ x 2 U 3 , m ] (21)
The above we can rewrite as
− α U ˙ 1 , m − 1 − U ˙ 1 , m − α U ˙ 1 , m + 1 − α ( G U 2 ) m − 1 − ( G U 2 ) m − α ( G U 2 ) m + 1 = p 1 ( U 2 , m − 2 − 2 U 2 , m + U 2 , m + 2 ) + p 2 ( U 2 , m − 1 − 2 U 2 , m + U 2 , m + 1 ) (22)
α U ˙ 2, m − 1 + U ˙ 2, m − α U ˙ 2, m + 1 − α ( G U 1 ) m − 1 − ( G U 1 ) m − α ( G U 1 ) m + 1 = p 1 ( U 1, m − 2 − 2 U 1, m + U 1, m + 2 ) + p 2 ( U 1, m − 1 − 2 U 1, m + U 1, m + 1 ) (23)
− α U ˙ 3, m − 1 − U ˙ 3, m − α U ˙ 3, m + 1 − α ( G U 4 ) m − 1 − ( G U 4 ) m − α ( G U 4 ) m + 1 = p 1 ( U 4, m − 2 − 2 U 4, m + U 4, m + 2 ) + p 2 ( U 4, m − 1 − 2 U 4, m + U 4, m + 1 ) (24)
α U ˙ 4, m − 1 + U ˙ 4, m + α U ˙ 4, m + 1 − α ( G U 3 ) m − 1 − ( G U 3 ) m − α ( G U 3 ) m + 1 = p 1 ( U 4, m − 2 − 2 U 4, m + U 4, m + 2 ) + p 2 ( U 4, m − 1 − 2 U 4, m + U 4, m + 1 ) (25)
where U ˙ i , m = ∂ u i ∂ t , i = 1 , 2 , 3 , 4 , p 1 = b 8 h 2 and p 2 = a 2 h 2 .
This system in a compact form will be written as
M U ˙ i = F i ( U 1 n , U 2 n , U 3 n , U 4 n ) , (26)
where i = 1,2,3,4 ,
M = 1 11 ( 11 2 0 0 ⋯ ⋯ ⋯ 0 2 11 2 0 0 ⋯ ⋯ 0 0 2 11 2 0 0 ⋯ 0 0 ⋱ ⋱ ⋱ ⋱ ⋱ ⋱ ⋮ ⋮ ⋱ ⋱ ⋱ ⋱ ⋱ ⋱ 0 ⋮ ⋱ ⋱ ⋱ ⋱ ⋱ ⋱ 0 ⋮ ⋱ ⋱ ⋱ 0 2 11 2 0 ⋯ ⋯ ⋯ 0 0 2 11 ) ,
U ˙ i = [ U i ,1 U i ,2 ⋮ ⋮ U i , M − 2 U i , M − 1 ] and F i = [ F i ,1 F i ,2 ⋮ ⋮ F i , M − 2 F i , M − 1 ]
and
F 1 , m = − p 1 ( U 2 , m − 2 n − 2 U 2 , m n + U 2 , m + 2 n ) − p 2 ( U 2 , m − 1 n − 2 U 2 , m n + U 2 , m + 1 n ) + α G m − 1 U 2 , m − 1 n + G m U 2 , m n + α G m + 1 U 2 , m + 1 n (27)
F 2, m = p 1 ( U 1, m − 2 n − 2 U 1, m n + U 1, m + 2 n ) + p 2 ( U 1, m − 1 n − 2 U 1, m n + U 1, m + 1 n ) + α G m − 1 U 1, m − 1 n + G m U 1, m n + α G m + 1 U 1, m + 1 n (28)
F 3, m = − p 1 ( U 4, m − 2 n − 2 U 4, m n + U 4, m + 2 n ) − p 2 ( U 4, m − 1 n − 2 U 4, m n + U 4, m + 1 n ) + α G m − 1 U 4, m − 1 n + G m U 4, m n + α G m + 1 U 4, m + 1 n (29)
F 4 , m = p 1 ( U 3 , m − 2 n − 2 U 3 , m n + U 3 , m + 2 n ) + p 2 ( U 3 , m − 1 n − 2 U 3 , m n + U 3 , m + 1 n ) + α G m − 1 U 3 , m − 1 n + G m U 3 , m n + α G m + 1 U 3 , m + 1 n (30)
The solution of (26), using the explicit RK4, can be displayed as follows:
U j , m n + 1 = U j , m n + 1 6 [ K j ,1 + 2 K j ,2 + 2 K j ,3 + K j ,4 ] , (31)
K j ,1 = k M − 1 F j , m ( U 1, m n , U 2, m n , U 3, m n , U 4, m n )
K j ,2 = k M − 1 F j , m ( U 1, m n + 1 2 K 1,1 , U 2, m n + 1 2 K 2,1 , U 3, m n + 1 2 K 3,1 , U 4, m n + 1 2 K 4,1 )
K j ,3 = k M − 1 F j , m ( U 1, m n + 1 2 K 1,2 , U 2, m n + 1 2 K 2,2 , U 3, m n + 1 2 K 3,2 , U 4, m n + 1 2 K 4,2 )
K j ,4 = k M − 1 F j , m ( U 1, m n + K 1,3 , U 2, m n + K 2,3 , U 3, m n + K 3,3 , U 4, m n + K 4,3 )
for j = 1 , 2 , 3 , 4
The proposed scheme is of sixth order in space and fourth order in time. The previous scheme, which applies the Runge-Kutta of order 4 method, is conditionally stable.
This section presents the numerical results for the aimed scheme. This method’s accuracy is tested with by studying its conservation properties and the truncation error using L 2 and L ∞ norms. Trapezoidal rule is used to calculate the conserved quantities. To reliably estimate the smooth solution of CNLSEs, discrete conservation laws are critical. The accuracy is scaled by using the L 2 error norm and L ∞ error norm.
‖ E R ‖ ∞ = max 1 < m < N { | ( ‖ Φ 1 ( x m , t n ) ‖ − ‖ U 1 , m n + i U 2 , m n ‖ ) | }
‖ E R ‖ 2 = [ ∑ m = 1 N ( ‖ Φ 1 ( x m , t n ) ‖ − ‖ U 1 , m n + i U 2 , m n ‖ ) 2 ] 1 2
In the following sections, we will analyze the subsequent problems that arose in studying the properties of the obtained scheme.
In this experiment, the initial condition is determined by
Φ 1 ( x ,0 ) = 2 α 1 + c sec h ( 2 α x ) exp i { v 1 x } ,
Φ 2 ( x ,0 ) = 2 α 1 + c sec h ( 2 α x ) exp i { v 1 x }
where α , c and v 1 are constants.
To estimate the numerical solution, we use the following parameters:
x 0 = − 50 , x M = 50 , h = 0.1 , k = 0.001 , v 1 = 0.5 , α = 1.0 , c = 1
In
To examine the interaction of two solitons, we exercise the following initial conditions.
| Time | I1 | I2 | I3 |
|---|---|---|---|
| 0 | 1.0000000000 | 1.0000000000 | 0.0867481599 |
| 2 | 1.0000000001 | 1.0000000001 | 0.0867481598 |
| 4 | 1.0000000003 | 1.0000000003 | 0.0867481574 |
| 6 | 1.0000000003 | 1.0000000003 | 0.0867481612 |
| 8 | 1.0000000003 | 1.0000000003 | 0.0867481594 |
| 10 | 1.0000000004 | 1.0000000004 | 0.0867481590 |
| Time | L∞(u1) | L∞(u2) | L2(u1) | L2(u2) |
|---|---|---|---|---|
| 2 | 0.0000000369 | 0.0000000482 | 0.0000000398 | 0.0000000456 |
| 4 | 0.0000000774 | 0.0000000649 | 0.0000000849 | 0.0000000679 |
| 6 | 0.0000000906 | 0.0000001139 | 0.0000000962 | 0.0000001366 |
| 8 | 0.0000001521 | 0.0000001014 | 0.0000001814 | 0.0000001244 |
| 10 | 0.0000000951 | 0.0000001854 | 0.0000001483 | 0.0000002170 |
Φ 1 ( x , 0 ) = ∑ j = 1 2 2 α j 1 + c sec h ( 2 α j x j ) exp i { v 1 j x j } ,
Φ 2 ( x , 0 ) = ∑ j = 1 2 2 α j 1 + c sec h ( 2 α j x j ) exp i { v 1 j x j }
These initial conditions draw two waves. The complete sum of the masses asymptotically can be shown as I = 2 1 + c ∑ j = 1 2 2 α j .
In this test we choose the parameters
x 0 = − 50 , x M = 50 , h = 0.1 , k = 0.001 , x 1 = − 25 , x 2 = 25 , v 11 = 0.5 , v 12 = − 0.5 , α 1 = 0.5 , α 2 = 0.5 , c = 1
This method is very nearly conserves all conserved quantities (see
| Time | I1 | I2 | I3 |
|---|---|---|---|
| 0 | 2.4142135390 | 2.4142135390 | 0.6896907735 |
| 20 | 2.4142135381 | 2.4142135381 | 0.6896908019 |
| 40 | 2.4142135368 | 2.4142135368 | 0.6896957423 |
| 60 | 2.4142135385 | 2.4142135385 | 0.6896907927 |
| 80 | 2.4142135380 | 2.4142135380 | 0.6896907866 |
We have used a sixth-order finite difference method and Runge-Kutta of order 4 method to solve CNLSEs. The RK4 scheme is fourth order in time and sixth order in space, and it remains conditionally stable. Obviously, from the results, the scheme obtains fourth-order instantly without the need for an extra procedure to improve the accuracy in the temporal direction.
The authors declare no conflicts of interest regarding the publication of this paper.
Alamoudi, K. and Hammoudeh, M.S. (2021) Explicit High-Order Method to Solve Coupled Nonlinear Schrödinger Equations. Advances in Pure Mathematics, 11, 472-482. https://doi.org/10.4236/apm.2021.115033