World Journal of Mechanics
Vol.2 No.1(2012), Article ID:17679,8 pages DOI:10.4236/wjm.2012.21001

Modulation Equations for Roll Waves on Vertically Falling Films of a Power-Law Fluid

Abdelaziz Boudlal1, Valery Liapidevskii2

1Laboratoire de Mecanique de Lille, Villeneuve d’Ascq, France

2Lavrentyev Institute of Hydrodynamics, Novosibirsk State University, Novosibirsk, Russia


Received November 20, 2011; revised December 20, 2011; accepted December 30, 2011

Keywords: Power-Law Fluid; Thin Film Flow; Vertical Wall; Modulation Equations; Nonlinear Stability; Roll Wave


Waves of finite amplitude on a thin layer of non-Newtonian fluid modelled as a power-law fluid are considered. In the long wave approximation, the system of equations taking into account the viscous and nonlinear effects has the hyperbolic type. For the two-parameter family of periodic waves in the film flow on a vertical wall the modulation equations for nonlinear wave trains are derived and investigated. The stability criterium for roll waves based on the hyperbolicity of the modulation equations is suggested. It is shown that the evolution of stable roll waves can be described by self-similar solutions of the modulation equations.

1. Introduction

Mud flows are frequently encountered in mountainous regions, especially after torrential rains, and often exhibit a series of breaking waves (roll waves). These type of waves can also be observed as an event following volcano eruptions. A report on roll waves can be found in extensive references quoted by Ng & Mei [1]. The roll waves which occur in inclined open channels are important in drainage problems and have received an extensive treatement in turbulent regime by Jefffreys [2], Dressler [3], Boudlal & Liapidevskii [4], among others, and for a laminar sheet flow by considering the flow with quadratic distribution of velocity profile (Alekseenko & Nakoryakov [5]; Buchin & Shaposhnikova [6]; Julien & Hartley [7]; Boudlal & Liapidevski [8]).

The discontinuous waves play an important role in engineering and geophysical processes. Roll waves consist of a periodic pattern of bores separated by continuous profiles of free boundary. The transition from uniform flow to intermittent flow regime is usually tackled by resorting to stability theory. When it is perturbed, a steady flow becomes unstable, if certain criteria are satisfied, and evolves towards wave breaking. Dressler has been the first, who gave the analytical solution for such waves in open channel flows. Based on long wave approximation, Dressler’s theory of roll waves was extended in [1] to a shallow layer of fluid mud, which has been modelled as a power law fluid. It has been shown, particularly, that if the fluid is highly non-Newtonian, very long waves may still exist even if the corresponding uniform flow is stable to infinitesimal perturbations.

The aim of the paper is to give a nonlinear study on stability of permanent roll waves on a shear thinning fluid in the frame of one-dimensional, unsteady, gradually varied, laminar mud flow with the shear stress being evaluated in a conventional manner. Starting from long waves equations averaged over the normal to the bed [1], the standard procedure of roll wave construction is used by matching continuous solutions of shallow water equations through stable hydraulic jumps. As the amplitude and the phase velocity of waves are slowly varying during their propagation and as these variations give rise to instability, the problem of stability is solved by deriving modulation equations for wave series. The stability criterion is formulated in terms of hyperbolicity of modulation equations that need the calculation of averaged quantities.

All results presented herein can be regarded as a generalization to a power law mud fluid in laminar flow regime of non linear stability method alredy applied to Newtonian turbulent flows in open channels (Boudlal & Liapidevskii [9]).

2. Governing Equations

Consider two-dimensional film flows of a non-Newtonian liquid on a vertical wall. The coordinate system is defined as follows: the axis is directed vertically down and axis is horizontal and directed outward of the liquid layer. The longitudinal velocity component is denoted by The boundary layer approximation is assumed to be valid, with a power-law shear stress relation for laminar flows taken in the form


Here is the viscosity coefficient of dimension

and is the flow index. The case n = 1 corresponds to the Newtonian fluid and is the ordinary dynamic viscosity [1]. By assuming the following form of the velocity profile in the film flow

, (2.2)

the governing equations, which consist of the mass and momentum conservation equations averaged in the ordinate direction, are reduced to the system [1].


Here h is the layer thickness, is the depth-averaged velocity, is the bottom stress, g is the gravity acceleration, is the momentum flux factor. For a shear-thinning fluid, which will be considered bellow, we have and, consequently,.

In dimensionless variables introduced in [1]; namely,


Equation (2.3) take the form (asterisks are omitted)


Here the reference depth and the reference velocity are expressed through the given flow rate and the viscosity as follows:


Note that Equation (2.5) are hyperbolic with the characteristics

. (2.7)

It is shown by linear analysis in [1] that any steady-state solution of (2.5)

is unstable. The instability of the uniform steady-state flow also can be easily checked by the Whitham method [9]. The flow is unstable if the velocity of the kinematic wave exceeds the velocity of long waves in (2.5), i.e.

. (2.8)

It is clear that (2.8) is satisfied for, since


3. Roll Waves

Analogously to unstable flow regimes in open channel flows, the roll waves or periodic discontinuous solutions, have been constructed for (2.5) [1]. In this section we give the short description of roll waves in the form suitable for the purposes of the paper.

Consider the travelling waves propagating with a constant velocity. Introducing the variable and assuming the flow being steady in the coordinate system moving with the velocity, Equation (2.5) are reduced to the ODE

, (3.1)

where and


Let y and be the critical depth and the critical velocity with It follows from (3.1) that the necessary condition of roll wave existence is


In view of (3.2) we have

. (3.4)

Note that


and, consequently, at the critical depth.

Let be fixed and. Equations (3.1)-(3.2) take the form

. (3.6)

To find the function in (3.6), the following identity is used:


Furthermore, the function can be represented as follows


where, and is a root of the equation at the interval. The continuous function

is positive for. It means that the function vanishes only at two points and for [1]. Therefore, for and


Now we can construct the two-parameter family of roll waves as follows: for given and we put, ,. Note that and are the conjugate depths, since the Rankine-Hugoniot conditions for discontinuous solutions of (2.5), which are reduced to the relation



are fulfilled. The stability condition for shocks satisfying (3.8) takes the form (Rozhdestvenskii and Janenko [10])



Thus the admissible values of the governing parameters, for which a roll wave exists, belong to the domain

For, a roll wave consists of the smooth part defined by the monotonous solution of (3.6) at the interval and of the jump with the conjugate depths and

4. Modulation Equations

It is shown in the previous section that analogously to the roll waves in open channel flows governed by the classic shallow water theory (Whitham [10]), the periodic travelling waves (roll waves) in film flow of a non-Newtonian fluid can be represented by the two-parameter family of discontinuous solutions of (2.5). We chose and as such parameters. The problem on nonlinear stability of periodic wave trains with slowly varying values and can be solved by analysis of hyperbolicity of the modulation equations for roll waves (Boudlal and Liapidevskii, [11]). After averaging (2.5) over the fixed length scale, which is large enough compared with the length of roll waves, we have the following modulation equations:


All averaged quantities can be expressed as functions of and as follows :


Here we have used (3.1)-(3.2), (3.8) for periodic roll waves defined by parameters and.

In view of (4.2) and (3.4) the modulation equations take the form




The nonstationary evolution of the governing parameters for a periodic wave train is described by Equation (4.3). We say the roll waves are stable if the modulation Equation (4.3) for corresponding values are hyperbolic. Considering and as new dependent variables instead of and, we can find the characteristics of (4.3) from the quadratic equation




Here “·” denotes the differentiation on and.

Equation (4.3) are hyperbolic for. It means that the hyperbolicity domain depends only on the variable or Note that for. It can be shown by numerical calculations that the hyperbolicity interval is rather narrow and it lies in vicinity of. For n = 1 the values of corresponding to the hyperbolicity domain belong to the interval with Therefore, the boundary of the hyperbolicity domain can be found effectively by the following approximation of the function for long waves


Approximate values of characteristics are given by (4.5)-(4.6) with instead of and instead of. In this case the modulation equations simplify considerably since the functions and are linear on:


The dependence for Equations (4.3), (4.8) with n = 1 is shown in Figure 1 for real roots of (4.5) (). Note that the corresponding graphs for (4.3), (4.4) and the approximate system (4.3), (4.8) practically concide, so we can use the latter system for the analysis of nonlinear stability of roll waves in the flows governed by (2.5). It follows from Figure 1 that the hyperbolicity interval for (4.3), (4.8) lies inside of the admissible interval of roll wave existence. It means that short roll waves and very long roll waves are unstable.

The simple centered waves, i.e. the self-similar solutions of (4.3) depending on the variable, can be found analytically. Equations (4.3), (4.8) for simple

Figure 1. Dependence for (4.3), (4.8).

waves take the form


A solution of (4.9) can be represented in the form


Here is a solution of (4.3) for the corresponding family of characteristics. The solution (4.10) can be applied to explain some specific features of roll wave dynamics considered below.

5. Roll Wave Dynamics

In this section we compare the numerical calculations performed for the model derived by Meza and Balakotaiah (2008) for vertically falling films of Newtonian fluid with numerical solutions of (2.3) for n = 1. Both models are derived for moderate Reynolds numbers of flow, but in contrast to the former model, the surface tension in Equation (2.3) is ignored. Let us rescale (2.3) slightly according to (Meza and Balakotaiah, 2008). For that we introduce the Reynolds number and the Weber number as follows

Here is the surface tension. Consider two models of film flows on a vertical wall depending on and explicitly. The first one is the Shkadov model [12], which with the dependent variables and takes the form


It is clear that for and. Equations (2.5) are equivalent to (5.1) and the systems can be transformed to each other by dilatation of independent variables. The momentum equation derived by Meza and Balakotaiah [13] gives the more accurate dispersion relations comparing with the Shkadov model as it has reported in their paper:


We will compare below numerical solutions of the model (5.2) presented in [13] with the corresponding numerical solutions of the hyperbolic model (5.1) with. It will be shown that despite of the difference in the shape of individual roll waves for the models with and without surface tension, the evolution of nonlinear periodic wave trains generated by monochromatic initial perturbations is very alike for both models. Note that Equations (5.1) and (5.2) are written in dimensionless variables. The characteristics of (5.1) with coincide with (2.7) and are positive. Therefore, to find a solution of (5.1) in the domain , we must put the values of at the boundaries and. The corresponding data are taken from (Meza and Balakotaiah, 2008) for the cases considered in their paper, namely:


We restrict our attention to the case 1 in [13] with. The Weber number for (5.2) is finite () and it vanishes for (5.1). The values of the dimensionless frequency are varied to demonstrate its influence on roll wave dynamics.

Numerical calculations using a variant of the Godunov standard scheme illustrate the development of roll waves on the free surface of a thin film flowing on a vertical wall in the frame of the hyperbolic model (5.1). In Figures 2-4 the perturbations of free surface of the liquid layer calculated by (5.1) are comparing with correspond-


Figure 2. Wave profile in the forced film flow of the Newtonian fluid (): (a) Equation (5.1), We = 0; (b) Equation (5.2), We = 10.


Figure 3. Wave profile in the forced film flow of the Newtonian fluid (): (a) Equation (5.1), We = 0; (b) Equation (5.2), We = 10.

ing calculations from [13], at given time. In both cases small perturbations, which amplitudes do not exceed a small fraction of the depth of the initial steady-state flow, are developing into roll waves of finite amplitude. Note that the waves stop to grow after they reach some critical value of amplitude. The interesting feature of roll wave evolution is the transition from “saturated” waves to very long waves (“tsunami” waves according [11]). Such transition is most pronounced in Figure 4. It is seen from Figures 4(a)-(c) that the length of the transition zone is increasing with time linearly. The analysis of the nonstationary evolution of roll wave packets is the subject of future investigations. Here we just give an idea how the self-similar solutions (4.10) can be applied to describe the transition “0” - “1” shown in Figures 4(a)-(c). First of all, for given frequency of the monochromatic wave packet “0”, the governing parameters are uniquelly determined by (3.4), (4.2), (4.7). Furthermore, in virtue of (4.10) the left boundary of the centered simple wave is known. The right boundary of the simple wave is calculated using (4.10) and the additional condition for “tsunami” waves:.

This algorithm gives the reasonable values for the boundaries of the states “0” and “1” in numerical calculations of the nonstationary problem of roll wave evolution. Therefore, the transition “0” - “1” in Figures 4(a)- (c) can be described by the centered simple wave of (4.9) moving on the left and the roll waves shown in Figure 4 are stable, since the governed parameters in a simple wave always belong to the hyperbolicity domain of the modulation equations

6. Conclusion

We have investigated the roll wave generation on vertically falling films by the nonlinear hyperbolic model (2.3), in which the viscous effects are taken into account by assuming that the velocity profile of an exact steady-state solution of the two-dimensional problem can be used also in the one-dimensional wavy flows. The model is based on the first order long-wave approximation of non-Newtonian fluid flows, which shear rate is modeled by a power law [1]. The capillarity effects are ignored to reveal the interplay between nonlinear and viscous terms in the governing equations. It is shown that


Figure 4. Wave profile in the forced film flow of the Newtonian fluid (): (a)-(d) Equation (5.1), We = 0; (e)-(f) Equation (5.2), We = 10; (a); (b); (c)-(f).

the periodic discontinuous solutions of (2.3) (roll waves) can be described by two parameters analogously to the roll waves in open channel flows. Moreover, the nonlinear stability of finite amplitude roll waves can be expressed in the terms of the hyperbolicity of modulation Equations (4.3) for the governing parameters of roll waves. Comparison of numerical calculations of roll wave evolution for the models with and without surface tension effects reveal that in spite of the difference in the individual wave shapes the behavior of roll wave packets is very alike for the models. In particular, the transition from “saturated” to “tsunami” waves described in [13] can be described by a simple wave of the modulation Equations (4.3).

7. Acknowledgements

The work was supported by the Russian Foundation for Basic Research (Grant No. 10-01-00338) and by the Program for support of leading scientific schools of the Russian Federation (Grant No. NSh-6706.2012.1).


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