# Single soliton solution to the extended KdV equation over uneven depth

###### Abstract

In this note we look at the influence of a shallow, uneven riverbed on a soliton. The idea consists in approximate transformation of the equation governing wave motion over uneven bottom to equation for flat one for which the exact solution exists. The calculation is one space dimensional, and so corresponding to long trenches or banks under wide rivers or else oceans.

###### pacs:

02.30.Jr, 05.45.-a, 47.35.Bb## I Introduction

Recently, we found exact solitonic KRI14 () and periodic IKRR17 () wave solutions for water waves moving over a smooth riverbed. Amazingly they were simple, though governed by a more exact expansion of the Euler equations with several new terms as compared to KdV MS90 (); BS13 (); KRR14 (); KRI14 (). Our next step is to consider how these results are modified by a rough river or ocean bottom. We start with a simple case. The geometry is one space dimensional and the wave a soliton. Even so, approximations rear their head! Considerations of a two dimensional bump on the bottom, as well as periodic waves propagating overhead, are planned for a later effort.

Here we consider the following equation governing the elevation of the water surface above a flat equlibrium at the surface (written in dimensionless variables)

(1) | ||||

The last three terms are due to a bottom profile. We emphasize, that (1) was derived in KRR14 (); KRI14 () under the assumption that are small (positive by definition) and of the same order. As usual, , the ratio of wave amplitude to mean water depth and where is mean wavelength. Parameter is the ratio of the amplitude of the bottom function to mean water depth. Up to this point are dimension quantities. Scaling to dimensionless variables allows us to apply perturbation approach to the set of Euler equations governing the model of ideal fluid. In the first order perturbation approach the KdV equation is obtained (assuming flat bottom). Applying second order perturbation approach Marchant and Smyth MS90 () derived equation (1) limited to the first line and named the extended KdV equation. Since it is derived in second order perturbation with respect to small parameters we call it KdV2. Taking into account small bottom fluctuations (again in second order perturbation approach) led us in KRR14 (); KRI14 () to the KdV2 equation for uneven bottom (1). In scaled variables amplitudes of wave and bottom profiles are equal one. In KRI14 (); IKRR17 () we derived exact soliton and periodic solutions to KdV2. These solutions are given by the same functions as the corresponding KdV solutions but with different coefficients.

This paper presents an attempt to describe dynamics of the exact KdV2 soliton when it approches a finite interval of uneven bottom. We will use reductive perturbation method introduced by Taniuti and Wei TW68 (). Using two space scales allows us to transform equation for uneven bottom (1) into KdV2 equation with some coefficients altered, that is, equation for the flat bottom. This transformation is approximate but analytical solution of the resulted equation is known. This approximate analytic description will be compared with exact numerical calculations.

## Ii KdV2 soliton (even bottom)

In this section we shortly remind exact soliton solution of the KdV2 equation given in KRI14 ().

Assume the form of a soliton moving to the right, . So, and the KdV2 equation, that is (1) without the last row, becomes ODE

(2) |

Integration gives

(3) |

Then the solution is assumed in the same form as KdV solution

(4) |

where , since in dimensionless variables the amplitude is already rescalled. However, for further consideretions it is convenient to keep the general notation. Insertion postulated form of the solution (4) and use of properties of hyperbolic functions gives (3) in polynomial form

(5) |

which requires simultanoeus vanishing of all coefficients . These three conditions are as follows

(6) | |||||

(7) | |||||

(8) |

Denoting one obtains (8) as quadratic equation with respect to with solutions

(9) |

Since , only provides real value. [In principle of imaginary argument can be expressed by a quotient of expressions given by hyperbolic functions of real arguments. However, these expressions are singular for some values of arguments and therefore physically irrelevant.]

## Iii Variable depth

Equation (1) can be written in the form

(11) |

where is given by

(12) |

We treat as slowly varying and introduce two space scales and which are treated as independent until the end of calculation TW68 ()

(13) |

We also introduce

(14) |

where is as yet undefined. To first order in

(15) |

(16) |

(17) |

(18) |

Now

(19) |

We have

(20) |

We restrict consideration to a single soliton, so as and so does . Integration of (22) yields to lowest order

(23) |

Introduce which is constant in our approximation. Now

(24) |

and from (23), (III), (24) we obtain

(25) |

Dividing by yields

(26) | |||||

This should be compared to (3) or (KRI14, , Eq. (22)). Remember that at this stage is to be treated as constant with respect to inegration over . The only difference is that and instead of 1 appear in the last term.

Following KRI14 () we obtain

(27) |

In equations (6)-(7) [(24), (25) and (20) of KRI14 ()] we replace (but not or since we modify only first order terms) by

(28) |

Now is as in (9). We obtain

(29) |

with

(30) |

Assume is nonzero only in interval .

For .

For and

(33) |

There is a change of phase as the pulse passes through the region where . The alteration in the phase is given by

(34) |

If this integral is zero phase is unaltered. This can happen if a deeper region is followed by a shallower region of appropriate shape or vice versa.

### iii.1 Examples

In the following figures we present time evolution of the approximate analytic solution (29) to KdV2 equation with uneven bottom (1) for several values of parameters of the system. These evolutions are compared with ’exact’ numerical solutions of (1). In both cases initial conditions were the exact solutions of KdV2 equation. Therefore in all presented examples and the amplitude of initial soliton is equal to 1.

In figure 1 we present the approximate solution (29) for the case when soliton moves over a trapezoidal elevation with and . We took . For smaller the effects of uneven bottom are very small, for larger second order effects (not present in analytic approximation) cause stronger overlaps of different profiles.

We compare this approximate solution of (1) to a numerical simulation obtained with the same initial condition. The evolution is shown in figure 2. We see that the approximate solution has the main properties of the soliton motion as governed by equation (1). However, since the numerical solution contains higher order terms depending on the shape of the exact motion as obtained from numerics shows additional small amplitude structures known from earalier papers, for example KRR14 (); KRI14 (). This is clearly seen in fig. 3 where profiles obtained in analytic and numeric calculations are compared at time instants on wider interval of . All numerical results were obtained with calculations performed on wider interval with periodic boundary conditions. Details of numerics was described in KRR14 (); KRI14 (); IKRR17 ().

In figures 4-6 we present results analogous to those presented in figures 1-3 but with a different shape of the bottom bump and larger values of . In this case the bump is chosen as an arc of parabola between the same and as in trapezoidal case.

In approximate analytic solution KdV2 soliton changes its amplitude and velocity only over bottom fluctuation. When the bottom bump is passed it comes back to initial shape (only phase may be changed). This is not the case for ’exact’ numerical evolution of the same initial KdV2 soliton when it evolves according to the second order equation (1). This is clearly visible in figures 3 and 6. What is this motion for much larger times? In order to answer this question one has to perform numerical calculations on much wider interval of . Such results are presented in figure 7. The interaction of soliton with the bottom bump creates two wave packets of small amplitudes. First moves with higher frequency faster than the soliton and is created when soliton enters the bump, second moves slower with lower frequency and appears when soliton leaves it. After some time both are separated from the main wave. Since periodic boundary conditions were used in numerical algorithm, the head of wave packet radiated forward travelled for larger distance than the interval chosen for calculation and is seen at left side of the wave profile.

## Iv Conclusions

We have derived a simple formula describing approximately a soliton encountering an uneven riverbed. The model reproduces the known increase in amplitude when passing over a shallower region, as well as the change in phase. However, the full dynamics of the soliton motion is much richer, the uneven bottom causes low amplitude soliton radiation both ahead and after the main wave. This behaviour was observed in our earlier papers KRI14 (); KRI15 (); KRIR17 () in which initial conditions were in the form of KdV soliton, whereas in the present cases the KdV2 soliton, that is, exact solution of the KdV2 equation was used.

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