On applicability of truncation method for damped axially moving string
Sanaullah Dehraj^{1} , Sajad H. Sandilo^{2} , Rajab A. Malookani^{3}
^{1, 2, 3}Department of Mathematics and Statistics, QuaideAwam University of Engineering, Science and Technology, 67480, Nawabshah, Sindh, Pakistan
^{1}Corresponding author
Journal of Vibroengineering, Vol. 22, Issue 2, 2020, p. 337352.
https://doi.org/10.21595/jve.2020.21192
Received 25 November 2019; received in revised form 11 February 2020; accepted 22 February 2020; published 31 March 2020
In this paper, the detailed study of the transversal vibrations of a damped axially moving string is considered. Two end pulleys of the string are taken to be fixed and the initial conditions are assumed to be of general displacement field and the general velocity field. The axial speed of the string is considered to be sinusoidal, timedependent and small compared to wavevelocity. A two timescales perturbation method with a combination of Fouriersine series which fits the boundary conditions is employed in order to formulate the valid and uniform asymptotic approximations of the exact solutions for the equation. It is found that there are infinitely many values of frequency parameter $\mathrm{\Omega}$ which cause the internal resonances in system. The fundamental resonant frequency, the nonresonant frequency and the detuning cases have been discussed and analyzed in detail. It has been found explicitly that the total mechanical energy of the infinite dimensional system decreases for two cases of the damping parameter, that is, for $\delta =\text{2}$ and for $\delta >\text{2}$. By truncation method it has been shown that the modeamplitude response for first few modes is stable. So, Galerkin’s truncation method may be possible for these two cases of the parameter $\delta $. But for case $\delta <\text{2}$ the total mechanical energy of belt system is increasing exponentially. Therefore, it is evident that the Galerkin’s truncation method cannot be applied in order to obtain valid approximations on long timescales, that is, on timescales of $O\left(1/\epsilon \right)$.
Keywords: conveyor belt, viscous damping, internal resonances, perturbation method.
1. Introduction
There are numerous applications in engineering such as elevators [15], aerial cables, crane and mining hoists, conveyor belts [69], oil pipelines [10, 11], magnetic and paper tapes and bandsaw blades [12], are often known as axially moving systems. Since last few decades, there has been vast research activity on examining the stability of such systems, for instance, see [1319]. Irregular speed of driven motor, nonuniform material properties and environmental disturbances can lead to severe vibrations, which are not desirable phenomena. Such severe vibrations can discomfort human beings and sometimes may create great damage to these mechanical structures. The main goal of applied mathematicians, engineers and physicists is to understand, analyze and mitigate these vibrations from the mechanical systems. In order to reduce unnecessary noise and vibrations in these mechanical systems, researchers have used different kinds of dampers at different positions of these systems, such as internal dampers [20], external dampers [21], wire rope [22, 23], elastomeric bearing [24] and KelvinVoigt damping [25] are extensively used in practical and industrial applications. Darmawijoyo and van Horssen [26] considered wave equation and studied the behaviour of springmassdashpot system attached at one boundary by using perturbation method. In this paper it was shown that the boundary damping is an effective phenomenon to suppress amplitudes of oscillations. Sandilo and van Horssen [27] studied beamlike equation with nonclassical boundary condition at one end and simply support on other end. In this paper though authors did not find any conclusion whether beam energy was increasing or decreasing, but authors found very interesting results. Gaiko and van Horssen [28] employed two timescales perturbation method and obtained the asymptotic approximations for (lateral) oscillations in axially moving string under the effect of boundary damping. Darmawijoyo and van Horssen [29] used two timescales perturbation method for finding the solution of weakly nonlinear wave equation with nonclassical boundary conditions. Darmawijoyo et al. [30] studied weakly nonlinear string equation, where one end of string was kept fixed and to the other end a dashpot was attached. A two timescales perturbation method with combination of method of characteristics was employed and it was shown that for large damping parameter solutions tend to zero. Chen and Ferguson [31] studied the axially moving viscoelastic string under viscous damping and, constant and timevarying length. The linear and nonlinear models were discussed from numerical solutions point of view. Malookani et al. [32] studied an axially moving string where they considered springdashpot system at one end and other end was kept fixed. Asymptotic approximations of the exact solutions were obtained by using a two timescales perturbation method with method of characteristic coordinates. Malookani and van Horssen [33] examined the lateral vibrations of axially moving system and computed the amplituderesponse of the system for all modes. The authors used method of two timescales together the Laplace transform method.
This paper aims to examine the applicability of Galerkin’s truncation method for the model describing the transversal vibrations of axially moving string under the influence of viscous damping, with timevarying velocity.
This paper is organized as follows. In Section 2, the governing equations of motion are established. In Section 3, the asymptotic approximations of the exact solution of the initialboundary value problem are constructed by using a two timescales perturbation method. These solutions will be analyzed and a Galerkin’s truncation method will be applied in order to truncate few modes from the infinite dimensional system of ODE’s. The detuning and the nonresonant cases will also be discussed in detail. In Section 4, the results and the discussion are presented. Finally, in Section 5, some conclusions will be drawn and the remarks will be made.
2. Governing equations of motion
In this Section, we consider viscous damped axially translating string, moving with timevarying velocity $V\left(t\right)$ as shown in Fig. 1. It is assumed that the displacement field is zero at end points of string, i.e., at $x=0$ and$x=L$, where$L$ is the constant distance between the pair of pulleys. The mathematical formulation of a string with viscous damping is carried out by extended Hamilton’s principle [34]. The mathematical formulation of the model describing the vertical vibrations of string with viscous damping is given as under:
with the Dirichlet boundary conditions:
and the initial conditions:
where $t$ is the time, $x$ is the spatial coordinate, $u(x,t)$ is the vertical displacement field, $V\left(t\right)$ is the belt velocity, $\rho $ is the linear constant massdensity, $T$ is the constant tension, and ${\delta}_{0}$ is viscous damping coefficient. At $t=$ 0, the displacement and velocity of the string are represented by the functions $f\left(x\right)$ and$g\left(x\right)$, respectively. In order to convert the equation of motion with associated initialboundary conditions in nondimensional form, we use the following nondimensional parameters:
${\Omega}^{*}=\frac{\Omega L}{c},{f}^{*}\left({x}^{*}\right)=\frac{f\left(x\right)}{L},{g}^{*}\left({x}^{*}\right)=\frac{g\left(x\right)}{c},{\delta}_{0}^{*}=\frac{{\delta}_{0}L}{\rho c},$
where $c=\sqrt{T/\rho}$, is a wave speed. Substitution of Eq. (4) and all required derivatives of unknown function $u(x,t)$ into initialboundary value problem Eqs. (1)(3) give the following dimensionless form of equations of motion (where asterisks have been neglected):
It is assumed that the quantity ${\delta}_{0}L$ is small in comparison to $\rho c$, where$c=\sqrt{T/\rho}$. Thus, we can write${\delta}_{0}^{*}={\delta}_{0}L/\rho c=\epsilon \delta $, where $\epsilon $ is small dimensionless parameter with $0<\epsilon \ll 1$. In addition to this, it is also assumed that the axial speed $V\left(t\right)$ is timevarying and small in comparison to wavespeed $c.$ Thus, we can write ${V}^{*}=V/c=\epsilon ({V}_{0}+\alpha \mathrm{sin}\left(\Omega t\right))$, where${V}_{0}$ and $\alpha $ are constants with ${V}_{0}0$ and ${V}_{0}\left\alpha \right$; this condition guarantees that the belt will always move in one direction. The velocity fluctuation frequency of belt is denoted by $\Omega $. The sinusoidal form of the belt velocity is of practical usage. In reality, however, due to belt imperfections, roll eccentricities, speed variations in driven motors, and nonuniform material properties can cause small variations in the belt velocity. This variation in the belt velocity exhibits interesting mathematical complexities and dynamical features.
Fig. 1. The schematic model of a damped axially moving belt with two fixedends
3. Construction of asymptotic approximations
In this section, we shall construct the asymptotic approximations of the solutions of the initialboundary value problem Eqs. (5)(7). We assume that the string velocity is timevarying and is of the $O\left(\epsilon \right)$, as given below:
We also assume that the damping parameter is of the $O\left(\epsilon \right)$, as given by:
By plugging Eq. (8) and Eq. (9) into Eq. (5), we collect the terms up to $O\left(\epsilon \right)$, we get:
with the boundary conditions:
and the initial conditions:
In order to construct the asymptotic approximations of the solution of the initialboundary value problem Eqs. (10)(12), we expand $u(x,t)$ in Fouriersine series, given as under:
The orthogonality properties of the eigenfunctions are given by:
By making use of Eq. (13) with required time and space derivatives into Eq. (10), it follows:
By multiplying Eq. (16) with $\mathrm{sin}\left(k\pi x\right)$ on both sides and then by integrating the soobtained equation from $x=$ 0 to $x=$ 1, and by using Eq. (14) and Eq. (15), it yields:
Eq. (17) represents an infinite dimensional system of ODE’s, which is not easy to be solved exactly. In the subsequent Section, the application of a two timescales perturbation method will be carried out to obtain approximations of the solutions of Eq. (17) for different values of the parameter $\mathrm{\Omega}$.
3.1. A two timescales perturbation method
In this section, we discuss the application of a two timescales perturbation method for constructing the approximations of the solutions of the infinite dimensional system of ODE’s given in Eq. (17). A straightforward expansion in $\epsilon $ will lead to unbounded terms which cause the nonuniformity in the solutions and this method is only applicable for $t<1/\epsilon $. Therefore, to approximate the exact solutions valid on long timescales, that is a timescales of $O\left({\epsilon}^{1}\right)$, it is reasonable to use a two timescales perturbation method. We introduce two timescales, ${t}_{0}=t$ (fast timescale) and ${t}_{1}=\epsilon t$ (slow timescale). We assume that the solution of Eq. (17) in the form ${u}_{k}\left(t;\epsilon \right)={w}_{k}({t}_{0},{t}_{1};\epsilon )$. The following transformations are required to express the time derivatives:
We plug Eq. (18) and Eq. (19) into Eq. (17), it follows:
An approximation of ${w}_{k}\left({t}_{\begin{array}{c}0\\ \end{array}},{t}_{1};\epsilon \right)$ is sought in the following form (up to $O\left(\epsilon \right)$ and neglecting higher order terms):
where ${w}_{k0}\left({t}_{0},{t}_{1}\right)$, ${w}_{k1}\left({t}_{0},{t}_{1}\right)$,… are of $O\left(1\right)$. By substituting Eq. (21) into Eq. (20), and equating the coefficients of ${\epsilon}^{0}$ and ${\epsilon}^{1}$, the $O\left(1\right)$ and the $O\left(\epsilon \right)$problem for ${w}_{k0}$ and ${w}_{k1}$ are given.
The $O\left(1\right)$ problem:
The $O\left(\epsilon \right)$ problem:
$+\sum _{\begin{array}{c}n=1\\ n\pm kisodd\end{array}}^{\infty}\left(\frac{nk}{{n}^{2}{k}^{2}}\right)\left[4\alpha \mathrm{\Omega}\mathrm{cos}\left(\mathrm{\Omega}{t}_{0}\right){w}_{n0}+8\left({V}_{0}+\alpha \mathrm{sin}\left(\mathrm{\Omega}{t}_{0}\right)\right)\frac{\partial {w}_{n0}}{\partial {t}_{0}}\right].$
The solution of Eq. (22) can easily be obtained, and is given by:
where ${A}_{k0}\left({t}_{1}\right)$ and ${B}_{k0}\left({t}_{1}\right)$ are still arbitrary functions of slow timescales and they can be determined from the $O\left(\epsilon \right)$problem free from the secular terms. Since we have assumed that the functions ${w}_{k0}\left({t}_{0},{t}_{1}\right)$ and ${w}_{k1}\left({t}_{0},{t}_{1}\right)$ are bounded on timescales of $O\left(1/\epsilon \right)$ so these unbounded/secular terms must be prevented to have valid and uniform approximations on long timescales. From Eq. (23), it turns out that the resonances only occur if$\mathrm{\Omega}=\left(k+n\right)\pi $, $\mathrm{\Omega}=\left(kn\right)\pi $, or $\mathrm{\Omega}=\left(nk\right)\pi $ when $n\pm k$ is odd.
3.2. The fundamental resonance case $\mathit{\Omega}=\mathit{\pi}$
This section discusses the fundamental resonant frequency case, that is, the frequency $\Omega $ of the moving string is equal to fundamental natural frequency of the string, that is $\Omega =\pi $. After putting $\mathit{\Omega}=\pi $ into the $O\left(\epsilon \right)$problem given in Eq. (23) and by avoiding the secular terms in ${w}_{k1}\left({t}_{0},{t}_{1}\right)$; the functions ${A}_{k0}\left({t}_{1}\right)$ and ${B}_{k0}\left({t}_{1}\right)$ have to satisfy the following solvability conditions:
$\frac{d{B}_{k0}}{d{\stackrel{}{t}}_{1}}=\frac{\stackrel{}{\delta}}{2}{B}_{k0}\left({t}_{1}\right)\left[\left(k+1\right){A}_{\left(k+1\right)0}+\left(k1\right){A}_{\left(k1\right)0}\right],$
where ${\stackrel{}{t}}_{1}=\alpha {t}_{1}$, $\stackrel{}{\delta}=\delta /\alpha $ and $k=\mathrm{1,2},3\dots $. The functions ${A}_{k0}$ and ${B}_{k0}$ are defined to be zero for nonpositive indices$k$. For sake of suitability, the bar from ${\stackrel{}{t}}_{1}$ and $\stackrel{}{\delta}$ is omitted. The coupled system Eq. (25) is an infinite dimensional system of ODE’s. It is evident from system Eq. (25) that there are infinitely many interfaces between the vibration modes. For $\delta =0$ in Eq. (25) is referred to [6].
3.2.1. Mathematical analysis of infinite dimensional system (25)
This subsection computes the energy of the axially moving system from coupled system given in Eq. (25) by using following transformations.
Let ${X}_{k0}\left({t}_{1}\right)=k{A}_{k0}\left({t}_{1}\right)$ and ${Y}_{k0}\left({t}_{1}\right)=k{B}_{k0}\left({t}_{1}\right)$, then Eq. (25) becomes:
where $k=\mathrm{1,2},3\cdots $ and the functions ${X}_{k0}$ and ${Y}_{k0}$ are zero for nonpositive indices $k.$ By multiplying ${X}_{k0}$ and ${Y}_{k0}$ with first and second equations in Eq. (26) respectively, we get:
By addition both equations in system Eq. (27), and by taking the sum from $k=1$ to $\infty $, it yields:
By differentiating Eq. (28) with respect ${t}_{1}$,it yields:
and then by putting $\sum _{K=1}^{\infty}\left({X}_{k0}^{2}+{Y}_{k0}^{2}\right)=w\left({t}_{1}\right)$ into Eq. (29) yields:
The solution of Eq. (30) is:
where ${p}_{1}$ and ${p}_{2}$ are constants and can be computed by applying the given initial conditions. Now by multiplying Eq. (5) with $\left({u}_{t}+V{u}_{x}\right)$ and after long but elementary calculations we get:
Integrate Eq. (32) first with respect to $x$ over the interval $[0$,$1]$ and then with respect to $t$ over $[0,t$] it yields:
Thus, the total mechanical energy of the string under viscous damping is given by:
The energy $E\left(t\right)$ of the axially moving string can also be computed by using the energy function $w\left({t}_{1}\right)$. Using Eq. (24) into Eq. (13) the approximated solution up to $O\left(\epsilon \right)$ is given by:
Thus, approximate energy of belt system can be obtained by plugging Eq. (35) into Eq. (34) it becomes:
On further simplification, it yields:
This implies that:
As $\sum _{K=1}^{\infty}\left({X}_{k0}^{2}+{Y}_{k0}^{2}\right)=w\left({t}_{1}\right)$, and using Eq. (31), so Eq. (37) becomes:
The following cases arise for damping parameter $\delta :$
– Case I: For $\delta =2,$ the energy of system decreases in the smaller domain of time and then remains constant.
– Case II: For $\delta >2,$ the energy decays as time increases.
– Case III: For $\delta <2,$ the energy increases without bound as time grows.
– Case IV: For $\delta =$ 0, then the system exhibits the similar behaviour as shown in [6].
3.2.2. Galerkin’s truncation method
This subsection investigates the application of truncation method for the system Eq. (25). The truncation up to three modes is given below:
where:
This linear system has the eigenvalues $\delta /2$, $\delta /2\pm 2\sqrt{2}i$, all with multiplicity of$2$ and their associated eigenvectors are given as follows: $\left(3,\mathrm{3,0},\mathrm{0,1},1\right)\text{,}$$\left(\mathrm{3,0},\mathrm{0,0},\mathrm{1,0}\right)\text{,}$$\left(\mathrm{1,1},\sqrt{2}i,\sqrt{2}i,\mathrm{1,1}\right)\text{,}$$\left(\mathrm{0,1},\sqrt{2}i,\mathrm{0,0},1\right)\text{,}$$\left(\mathrm{1,1},\sqrt{2}i,\sqrt{2}i,\mathrm{1,1}\right)\text{,}$$\left(\mathrm{0,1},\sqrt{2}i,\mathrm{0,0},1\right)\text{,}$ respectively. Thus, the general solutions of a linear system Eq. (40) is given by:
${B}_{10}\left({t}_{1}\right)={e}^{\frac{\delta}{2}{t}_{1}}\left[{C}_{3}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)+{C}_{4}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)3{C}_{5}\right],$
${A}_{20}\left({t}_{1}\right)={e}^{\frac{\delta}{2}{t}_{1}}\left[\sqrt{2}{C}_{4}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)+\sqrt{2}{C}_{3}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)\right],$
${B}_{20}\left({t}_{1}\right)={e}^{\frac{\delta}{2}{t}_{1}}\left[\sqrt{2}{C}_{2}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)\sqrt{2}{C}_{1}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)\right],$
${A}_{30}\left({t}_{1}\right)={e}^{\frac{\delta}{2}{t}_{1}}\left[{C}_{1}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)+{C}_{2}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)+{C}_{6}\right],$
${B}_{30}\left({t}_{1}\right)={e}^{\frac{\delta}{2}{t}_{1}}\left[{C}_{3}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)+{C}_{4}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)+{C}_{5}\right],$
where ${C}_{1}$, ${C}_{2}$,…, ${C}_{6}$ are all constants and are to be determined via initial conditions: $u\left(x,0\right)=f\left(x\right)$, ${u}_{t}\left(x,0\right)=g\left(x\right)$, $0<x<1$, it follows that:
Moreover, since ${u}_{k}\left(0;\epsilon \right)={w}_{k}\left(\mathrm{0,0};\epsilon \right)={w}_{k0}\left(\mathrm{0,0}\right)+\epsilon {w}_{k1}\left(\mathrm{0,0}\right)+\cdots $ and${\dot{u}}_{k}\left(0;\epsilon \right)={\dot{w}}_{k}\left(\mathrm{0,0};\epsilon \right)={\dot{w}}_{k1}\left(\mathrm{0,0}\right)+\epsilon {\dot{w}}_{k2}\left(\mathrm{0,0}\right)+\cdots $ it follows that:
Thus, by using Eq. (24) and Eq. (45) finally we get:
Now the constants in Eq. (42) can easily be determined by utilizing Eq. (46). Thus for $f\left(x\right)=0.01\mathrm{sin}\left(\pi x\right)$, and $g\left(x\right)=0$ we find first three approximate modes as under:
${u}_{2}\left(x,t\right)\approx {e}^{\frac{\delta}{2}{t}_{1}}\left[\begin{array}{c}0.01\mathrm{cos}\left(\pi {t}_{0}\right)\mathrm{cos}\left(\sqrt{2}{t}_{1}\right)\mathrm{sin}\left(\mathit{\pi x}\right)\\ \frac{0.01}{\sqrt{2}}\mathrm{sin}\left(\sqrt{2}{t}_{1}\right)\mathrm{sin}\left(2\pi {t}_{0}\right)\mathrm{sin}\left(2\pi x\right)\end{array}\right],$
$\frac{\left(0.01\right)\sqrt{2}}{4}\mathrm{sin}\left(2\sqrt{2}{t}_{1}\right)\mathrm{sin}\left(2\pi {t}_{0}\right)\mathrm{sin}\left(2\pi x\right)$
$\left.+\left(\frac{0.01}{4}\mathrm{cos}\left(2\sqrt{2}{t}_{1}\right)\frac{0.01}{4}\right)\mathrm{cos}\left(3\pi {t}_{0}\right)\mathrm{sin}\left(3\pi x\right)\right].$
Eq. (47) shows that first three modes are clearly damped out and amplitude of oscillations gets reduced. It is, however, difficult to calculate four and more than four eigenvalues and corresponding eigenvectors manually so we use computer software package Mapple16, to obtain the eigenvalues of coupled system up to $7$ modes and are given listed in Table 1. All of these eigenvalues are multiplicity of 2 and the real parts of eigenvalues have negative sign which shows that system is stable in nature. Further for $\delta =\text{0}$ system has same eigenvalues as given in [6].
Table 1. The eigenvalues of truncated system Eq. (25)
No. of modes  The Eigenvalues of matrix $A$ (All multiplicity of 2)  Dimension of $A$ 
1  $\frac{\delta}{2}$  2 
2  $\frac{\delta}{2}\pm \sqrt{2}i$  4 
3  $\frac{\delta}{2}\pm 2\sqrt{2}i,\frac{\delta}{2}$  6 
4  $\frac{\delta}{2}\pm 1.13i,\frac{\delta}{2}\pm 4.33i$  8 
5  $\frac{\delta}{2}\pm 2.302i,\frac{\delta}{2}\pm 5.89i,\frac{\delta}{2}$  10 
6  $\frac{\delta}{2}\pm 1.00i+,\frac{\delta}{2}\pm 7.50i,\frac{\delta}{2}\pm 3.56i,$  12 
7  $\frac{\delta}{2}\pm 4.89i,\frac{\delta}{2}\pm 2.05i,\frac{\delta}{2}\pm 9.15i,\frac{\delta}{2}$  14 
3.3. The detuning case: $\mathit{\Omega}=\mathit{m}\mathit{\pi}+\mathit{\epsilon}\mathit{\sigma}$
This section presents the (in) stability of the damped axially moving string close to the resonances, i.e.,$\Omega ~m\pi $, where the constant $m$ is taken to be positive odd integer. Thus, we demonstrate the closeness of velocity fluctuation $\Omega $ by using the relation:
where the parameter $\sigma $ is a detuning parameter and $\epsilon $ is a small dimensionless parameter, that is, $0<\epsilon \ll 1$. Putting Eq. (48) into Eq. (23) gives for the $O\left(\epsilon \right)$ for${w}_{k1}$:
To avoid the unbounded terms in Eq. (49), the functions ${A}_{k0}$and ${B}_{k0}$ have to satisfy the following solvability conditions:
$\left.\left(mk\right)\left({A}_{\left(mk\right)0}\mathrm{sin}\sigma {t}_{1}+{B}_{\left(mk\right)0}\mathrm{cos}\sigma {t}_{1}\right)\left(km\right)\left({A}_{\left(km\right)0}\mathrm{sin}\sigma {t}_{1}{B}_{\left(km\right)0}\mathrm{cos}\sigma {t}_{1}\right)\right],$
$\frac{d{B}_{k0}}{d{t}_{1}}=\frac{\delta}{2}{B}_{k0}\left({t}_{1}\right)\frac{\alpha}{m}\left[\left(m+k\right)\left({A}_{\left(m+k\right)0}\mathrm{cos}\sigma {t}_{1}{B}_{\left(m+k\right)0}\mathrm{sin}\sigma {t}_{1}\right)\right.$
$\left.+\left(mk\right)\left({A}_{\left(mk\right)0}\mathrm{cos}\sigma {t}_{1}{B}_{\left(mk\right)0}\mathrm{sin}\sigma {t}_{1}\right)+\left(km\right)\left({A}_{\left(km\right)0}\mathrm{cos}\sigma {t}_{1}+{B}_{\left(km\right)0}\mathrm{sin}\sigma {t}_{1}\right)\right],$
where $k=\mathrm{1,2},3,\cdots $ and the functions ${A}_{k0}$ and ${B}_{k0}$ are defined to be zero for $k\le 0$. It can be observed that for $\sigma =\text{0}$and $m=\text{1}$ we get same system given in Eq. (25) and for $\delta =0$ in above coupled system we get same system as given in [33].
3.3.1. Mathematical analysis of infinite dimensional system Eq. (50)
In this subsection we analyze the coupled system of ODE’s for $m=$ 1, and obtain the energy of the system to examine its behaviour for detuning case. For $m=$ 1, Eq. (50) reduces as:
$\left.\left(k1\right)\left({A}_{\left(k1\right)0}\mathrm{sin}\sigma {t}_{1}{B}_{\left(k1\right)0}\mathrm{cos}\sigma {t}_{1}\right)\right],$
$\frac{d{B}_{k0}}{d\stackrel{}{{t}_{1}}}=\frac{\stackrel{}{\delta}}{2}{B}_{k0}\left({t}_{1}\right)\left[\left(k+1\right)\left({A}_{\left(k+1\right)0}\mathrm{cos}\sigma {t}_{1}{B}_{\left(k+1\right)0}\mathrm{sin}\sigma {t}_{1}\right)\right.$
$\left.+\left(k1\right)\left({A}_{\left(k1\right)0}\mathrm{cos}\sigma {t}_{1}+{B}_{\left(k1\right)0}\mathrm{sin}\sigma {t}_{1}\right)\right],$
where $\stackrel{}{{t}_{1}}=\alpha {t}_{1}$ and $\stackrel{}{\delta}=\delta /\alpha $ and $k=$ 1, 2, 3…. For convenience, we drop the bar from $\stackrel{}{{t}_{1}}$ and $\stackrel{}{\delta}$. By introducing ${X}_{k0}=k{A}_{k0}$ and ${Y}_{k0}=k{B}_{k0}$, where $k=$ 1, 2, 3…, the system Eq. (51) becomes:
The functions ${X}_{k0}\left({t}_{1}\right)$ and ${Y}_{k0}\left({t}_{1}\right)$ are zero for $k\le 0$. By multiplying the functions ${X}_{k0}\left({t}_{1}\right)$ and ${Y}_{k0}\left({t}_{1}\right)$, respectively, the first and the second equations of Eq. (52), it yields:
By adding both sides of Eq. (53), and then by taking the sum from $k=1$ to $\infty $, it becomes:
After differentiating Eq. (54) twice with respect to ${t}_{1}$, we obtain:
where $\sum _{K=1}^{\infty}\left({X}_{k0}^{2}+{Y}_{k0}^{2}\right)=w\left({t}_{1}\right)$, thus the roots of auxiliary Eq. (55) are $\delta $, $\delta \pm \sqrt{4{\sigma}^{2}}$.
Three cases arise:
Case I: When $4{\sigma}^{2}=0$, that is, $\sigma =\pm 2$ then $w\left({t}_{1}\right)=\left({c}_{1}+{c}_{2}{t}_{1}+{{c}_{3}t}_{1}^{2}\right){e}^{\delta {t}_{1}}$ where ${c}_{1},{c}_{2}$and ${c}_{3}$ are arbitrary constants. In this case, if $\delta >\text{0}$ the energy of system decays as time increases without bound and in this case the system is stable, whereas if $\delta =\text{0}$ then energy grows polynomially; so the energy of infinite dimensional system remains unbounded.
Case II: When $4{\sigma}^{2}>0$ that is, $\left\sigma \right<\text{2}$ then:
and if $\delta >\sqrt{4{\sigma}^{2}}$ the energy of system decays as time increases and system is stable. For $\delta <\sqrt{4{\sigma}^{2}}$ the energy of infinite system of coupled ODE’s grow exponentially, that is sign for unstable system.
Case III: When $4{\sigma}^{2}<\text{0}$ that is,$\left\sigma \right\text{2}$, then:
In this case, the energy remains to be bounded.
3.4. The nonresonant case
In this case we assume that the fluctuation frequency $\mathrm{\Omega}$ in not within an $O\left(\epsilon \right)$ neighbourhood of the frequencies that cause the internal resonance, that is not within an $O\left(\epsilon \right)$ neighbourhood of $\pi $, then we may have following equation after eliminating the secular terms:
The solution of Eq. (56) is ${A}_{k0}\left({t}_{1}\right)={D}_{1}{e}^{\frac{\delta}{2}{t}_{1}}$ and ${B}_{k0}\left({t}_{1}\right)={D}_{2}{e}^{\frac{\delta}{2}{t}_{1}}$where ${D}_{1}$ and ${D}_{2}$ are arbitrary constants. By inserting the solution of Eq. (56) into Eq. (35), we obtain:
Eq. (57) clearly shows that the system damps out due to the presence of damping in the system. The energy of damped string system for nonresonant case can also be approximated by putting Eq. (57) to Eq. (34) it yields:
It can easily be observed from Eq. (58) that energy of damped axially moving string seems stable for nonresonant case.
4. Results and discussion
This section presents the results for the transverse vibrations of the damped axially moving string for the resonant, nonresonant cases. It is assumed that the string moves in one direction with timedependent velocity $V\left(t\right)=\epsilon \left({V}_{0}+\alpha \mathrm{sin}\left(\Omega t\right)\right)$, where $0<\epsilon \ll 1$ and ${V}_{0}$, $\alpha $, $\mathrm{\Omega}$ are positive constants. A two timescales perturbation method with conjunction of Fouriersine series has been employed in search of infinite mode approximate solutions. It has been found that there are infinitely many values of $\mathrm{\Omega}$ which give rises to the resonances in system. This study, however, is restricted to the fundamental resonance case, that is, $\mathrm{\Omega}=\pi $. The energy of system is obtained from infinite dimensional system of coupled ordinary differential equations. For $\delta =$ 2, it has been observed that the energy of system decreases in the smaller domain of time and then remains constant. For $\delta >$ 2 the energy of system has been damped out as the time progresses, while the energy grows without bound when $\delta <$ 2. However, for $\delta =\text{0}$ the system exhibits the similar behavior as obtained in [6]. Fig. 2 depicts the energy and modeamplitude response for the damping parameter$\delta =$ 2. Fig. 2(a) represents the energy of the damped system, while Fig. 2(b), Fig. 2(c) and Fig. 2(d) represent, respectively, the first, the second and the third modeamplitude responses. It can clearly be seen in these figures that both the modeamplitude response and energy are damped out as time increases. This implies that the moderesponse and energy response exhibits the similar behavior, so there does not seem a problem in modetruncation. The energy and mode responses are obtained for $\delta >$ 2 and is shown in Fig. 3. The energy response is shown in Fig. 3(a), while Fig. 3(b), Fig. 3(c) and Fig. 3(d) represent the first, the second and the third modeamplitude responses, respectively. It can easily be observed in these figures that the energy and modeamplitude responses have similar behavior, so modetruncation for $\delta >$ 2 may also be possible. Finally, Fig. 4(a) represents the energy for $\delta <$ 2, and it grows exponentially. Fig. 4(b), Fig. 4(c) and Fig. 4(d) depict, respectively, the first, the second and the third modeamplitude responses for $\delta <$ 2. In these figures, it can easily be observed that both the energy and modeamplitude responses have different behavior, so the modetruncation for this case does not seem possible.
– Case I. $\delta =$ 2.
Fig. 2. For $\epsilon =$ 0.01, $\delta =$ 2 and $x=$ 0.5: a) energy $E$vs time$t$, b) first mode, c) second mode, d) third mode
a)
b)
c)
d)
– Case II. $\delta >$ 2.
Fig. 3. For $\epsilon =$ 0.01, $\delta =$ 5 and $x=$ 0.5: a) energy $E$ vs time $t$, b) first mode, c) second mode, d) third mode
a)
b)
c)
d)
– Case III. $\delta <$ 2.
Fig. 4. For $\epsilon =$ 0.01, $\delta =$ 0.05 and $x=$ 0.5: a) energy $E$ vs time $t$, b) first mode, c) second mode, d) third mode
a)
b)
c)
d)
5. Conclusions
In this paper, we have examined the applicability of truncation method for stringlike model under the effect of viscous damping. Axial velocity of the string is assumed to be sinusoidal, timevarying and small compared to wave velocity. In order to obtain the formal approximations of the solutions of the initialboundary value problem, a two timescales perturbation method along with Fouriersine series is employed. It turns out that there are infinitely many values of parameter $\mathrm{\Omega}$ which give rise to the resonances in system. The fundamental resonant, detuning and nonresonant cases have been discussed. In resonantcase, the modeamplitude response and energy of the damped system are computed. For$\delta =$ 2 and $\delta >$ 2, it has been shown that the modetruncation may not be problematic for damped stringlike model as was claimed in [6, 33]. However, for $\delta <$ 2, the modetruncation is not possible due to exponential growth of the energy of damped system and oscillatory behaviour of modeamplitude responses.
In addition to this, the energy of system in the neighbourhood of fundamental resonance is discussed. It has been observed that the system remains stable for detuning parameter $\sigma =$ ±2 and damping parameter $\delta >$ 0. In case of detuning parameter $\left\sigma \right<$ 2, the energy of system is shown to be bounded for damping parameter $\delta >\sqrt{4{\sigma}^{2}}$, while the system remains unstable for $\delta <\sqrt{4{\sigma}^{2}}$. However, the system remains stable due to trigonometric functions for detuning parameter $\left\sigma \right>\text{2}$. Furthermore, for nonresonant case, the system is shown to be stable.
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