# Nonlinear Dynamics of a Periodically Driven Duffing Resonator Coupled to a Van der Pol Oscillator

Authors: X. Wei; M. F. Randrianandrasana; M. Ward; D. Lowe
Journal: Mathematical Problems in Engineering
 (2011)

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## Abstract

We explore the dynamics of a periodically driven Duffing resonator coupled elastically
to a van der Pol oscillator in the case of 1 : 1 internal resonance in the cases of weak
and strong coupling. Whilst strong coupling leads to dominating synchronization, the
weak coupling case leads to a multitude of complex behaviours. A two-time scales
method is used to obtain the frequency-amplitude modulation. The internal resonance
leads to an antiresonance response of the Duffing resonator and a stagnant response (a
small shoulder in the curve) of the van der Pol oscillator. The stability of the dynamic
motions is also analyzed. The coupled system shows a hysteretic response pattern and
symmetry-breaking facets. Chaotic behaviour of the coupled system is also observed
and the dependence of the system dynamics on the parameters are also studied using
bifurcation analysis.


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## Body

## 1. Introduction

In  the macro world, one can easily find models of single, and coupled nonlinear oscillators in many different scientific disciplines, for example, biology, electronics and physics. However, in the small world, recent development in M/NEMS (Micro/Nano Electromechanical Systems) technology now can enable physicists to design and manufacture large arrays of coupled M/NEMS nonlinear oscillators to explore the mathematics and physics of emergent phenomena that appear in the self organization of the interacting individual elements. For instance, intrinsic localized modes and moving discrete breathers have been observed in coupled microcantilever resonators [1, 2]. Therefore, the fundamental study of coupled nonlinear oscillators is significant in understanding the emergent behaviour of complex dynamical systems and developing novel M/NEMS devices [3–5]. This work is also motivated by the fact that analysis of simpler cases as the building blocks can help us to gain insight into larger complicated systems [6, 7]. Among the building blocks studied in the literature, the essential elements are either self-sustained oscillators (van der Pol oscillators) or dissipative oscillators (Duffing type resonators) and the most intensively studied cases are the coupled van der Pol and the coupled Duffing oscillators [8–10]. To the best of our knowledge, less has been done in a dynamic system consisting of a Duffing type resonator coupled to a self-excited oscillator. Our aim in this paper is to consider the dynamics of such a system externally driven by a periodic force. The motion of the coupled dynamical system in dimensionless form is described by the following set of equations:
(1.1)ẍ1+c1ẋ1+x1+k3x13=kc(x2-x1)+fdcos(ωdω1τ),ẍ2+c2(x22-1)ẋ2+(ω2ω1)2x2=kc(x1-x2),
where x1, c1, ω1 and x2, c2, ω2 are the displacement, damping coefficient, and fundamental frequency of the Duffing resonator and the van der Pol oscillator, respectively. fd and ωd are the amplitude and frequency of the external driving force. k3 is the nonlinearity of the Duffing resonator and kc is the coupling stiffness between the two coupled elements. When kc diminishes to zero, (1.1) uncouple to yield a driven Duffing resonator and a van der Pol oscillator whose limit cycle is determined by c2. For the case of fd=0, (1.1) can be considered as a damped Duffing resonator driven by a van der Pol oscillator. The dynamics of the undriven system has been numerically studied using three control parameters, namely, two damping coefficients (c1 and c2) and coupling stiffness (kc) [11]. Three different synchronization phenomena were found and a chaotic state was clearly identified in the phase diagram. The dynamics of such an undriven system was also studied in the form of a van der Pol oscillator with a nonlinear restoring force coupled to a Duffing resonator through a mixed velocity and displacement coupling condition [12] and an inertial force condition [13]. Analytic solutions of stable oscillation states were derived in both cases and the chaotic behaviour was also observed. As a result, we can envisage that more complex dynamics could appear in such an externally driven nonlinear system of two elastically coupled oscillators of different types of attractor.This paper is organized as follows. In Section2, we give an analytic treatment of (1.1). The method of multiple time scales is used to find approximate solutions of the oscillatory states. We end this section by giving a stability analysis of the fixed points on the stable oscillation curve. Section 3 presents bifurcation analysis of the coupled system in the parameter space. Section 4 is concerned with asymptotic dynamics of the coupled system using a direct integration method. Concluding ideas are given in Section 5.


## 2. Analytic Treatment

Usually, MEMS resonators and oscillators are working in a highQ scenario while they are driven into their resonances with a small force. However, if the Duffing resonator and van der Pol oscillator are working at different fundamental frequencies (the nonresonant case ω1≠ω2), it can be proven that the dynamic systems are uncoupled and the time evolution of the amplitudes is the same as the classical driven Duffing resonator and van der Pol oscillator. In the following section, we consider only the case where both the internal and external resonances coincide (ω1=ω2). As the coupling stiffness varies across a large range, we deal separately with the system of weak coupling (kc≪1) and strong coupling (kc≫1).


### 2.1. The Resonant Case of Weak Coupling

When the van der Pol oscillator is weakly connected to the Duffing resonator, we rewrite (1.1) as follows:
(2.1)ẍ1+ϵμ1ẋ1+x1+ϵαx13=ϵβ(x2-x1)+ϵFcos(Ωτ),ẍ2+ϵμ2(x22-1)ẋ2+x2=ϵβ(x1-x2),
where c1=ϵμ1, c2=ϵμ2, k3=ϵα, kc=ϵβ, fd=ϵF, Ω=ωd/ω1 and ϵ is a small parameter.The stable response of the system driven near the primary resonance can be calculated from (2.1) using the standard two-time scales method [14]. Briefly, we introduce a fast scale τ0 (τ0=τ) and a slow scale τ1 (τ1=ϵτ0) characterizing the modulation in amplitudes and phases and seek solutions of (2.1) that are expressed in the form of an asymptotic expansion as follows: (2.2)x1=x10(τ0,τ1)+ϵx11(τ0,τ1),x2=x20(τ0,τ1)+ϵx21(τ0,τ1).Substituting (2.2) into (2.1) and equating coefficients of like powers of ϵ, we obtain that(2.3a)D02x10+x10=0,(2.3b)D02x20+x20=0,(2.3c)D02x11+x11=-2D0D1x10-μ1D0x10-αx103+β(x20-x10)+Fcos(Ωτ0),(2.3d)D02x21+x21=-2D0D1x20-μ2D0x20(x202-1)+β(x10-x20),where D0=∂/∂τ0 and D1=∂/∂τ1.The general solution of (2.3a) and (2.3b) can be expressed as
(2.4)x10=A1(τ1)eiτ0+c.c,x20=A2(τ1)eiτ0+c.c,
where A1 and A2 are arbitrary constants and c.c denotes the complex conjugate.Substitutingx10 and x20 into the right-hand side of (2.3c) and (2.3d), we obtain the following set of equations by imposing secular conditions: (2.5)2A1′+μ1A1-3iα|A1|2A1+iβ(A2-A1)-i2Feiστ1=0,2A2′+μ2(|A2|2-1)A2+iβ(A1-A2)=0.
We have introduced the frequency detuning σ to characterize the closeness of driving frequency to the fundamental frequency, given by Ω=1+ϵσ.ExpressingA1 and A2 in polar form:
(2.6)A1=a1eiθ1,A2=a2eiθ2,
and substituting the polar expressions into (2.5) and separating real and imaginary parts, we obtain the following coupled first-order differential equations:
(2.7)2a1′=-μ1a1+βa2sinγ2-F2sinγ1,2a2′=-μ2(a22-1)a2-βa1sinγ2,2a1γ1′=-(β-2σ)a1+3αa13-βa2cosγ2-F2cosγ1,2a2γ2′=(β-2σ)a2-βa1cosγ2-2a2γ1′,
where γ1=θ1-στ1 and γ2=θ2-θ1.To determine the steady-state motion, we use the condition thata1′=a2′=0 and γ1′=γ2′=0. From (2.7), we obtain the following set of algebraic equations, (2.8a)(a1(β-2σ)+3a13α-a22(β-2σ)a1)2+(a1μ1-a22μ2a1(1-a22))2=14F2,(2.8b)(β-2σ)2a22+μ22a22(1-a22)2=a12β2.Equation (2.8b) shows Duffing-type behaviour of the van der Pol oscillator, provided that the coupling and damping coefficients are not zero. If the coupling effect diminishes, then (2.8a) will be reduced to the frequency-amplitude modulation of a normal Duffing resonator.


### 2.2. The Resonant Case of Strong Coupling

If the coupling stiffnesskc is not the same order of magnitude as the other parameters, the analysis in Section 2.1 does not hold, so a modified analysis considering strong coupling is given as follows. When kc is larger than 4.5 for example, 1/(2kc+1) is less than 0.1. Therefore, We choose ϵ=1/(2kc+1) and assume all other coefficients are small as defined in Section 2.1. Then (1.1) can be rewritten as (2.9)ẍ1+ẍ2+ϵμ1ẋ1+ϵμ2(x22-1)ẋ2+x1+x2+ϵαx13=ϵFcos(Ωτ),ϵ(ẍ1-ẍ2)+ϵ2μ1ẋ1-ϵ2μ2(x22-1)ẋ2+x1-x2+ϵ2αx13=ϵ2Fcos(Ωτ).Repeating the same analysis in Section2.1, we obtain the solutions of (2.9) for the zero-order approximation as (2.10)D02(x10+x20)+x10+x20=0,(2.11)x10-x20=0.
Equation (2.11) means that the Duffing resonator and the van der Pol oscillator are completely synchronised. As shown in Section 2.1, we can easily write down the solutions of (2.10) and (2.11) as follows:
(2.12)x10=x20=Aeiτ+c.c.The first-order approximation gives(2.13)D02(x11+x21)+x11+x21=-2D1D0(x10+x20)-μ1D0x10-μ2(x202-1)D0x20-αx103+Fcos(Ωτ),x11-x21=0.Apparently, the Duffing resonator and the van der Pol oscillator are still completely synchronised in the first-order approximation when they are strongly coupled. Substituting the expressions ofx10 and x20 into the right-hand side of (2.13), we obtain the following equation by imposing secular conditions:(2.14)4A′+(μ1-μ2)A+μ2A|A|2-3iαA|A|2+i12Feiστ1=0.ExpressingA in polar form as defined in Section 2.1 (note that a1=a2=a, θ1=θ2 as (2.12) holds), and substituting into (2.14), we obtain the following set of first-order differential equations for the amplitude and phase:
(2.15)4a′=(μ2-μ1)a-μ2a3-12Fsinγ1,4aγ1′=-4aσ+3αa3-12Fcosγ1.
For the steady state solutions, we obtain the following algebraic equation describing the amplitude response of the system:(2.16)a2(-4σ+3αa2)2+a2(μ1-μ2+μ2a2)2=14F2.After eliminating the secular terms in the two-time scales analysis, the second-order differential equation, (2.13) can be solved. Accordingly, x11 and x21 are obtained as follows:
(2.17)x11=x21=116(α-μ1i)A3e3iτ+cc.
Therefore, the general solution of the strongly coupled Duffing resonator and van der Pol oscillator in the first-order approximation is given by(2.18)x1=x2=ℜ(x10+ϵx11)=(aei(Ωτ+γ)+116ϵ(α-μ2i)a3e3i(Ωτ+γ)+cc),
which shows that in the case of strong coupling, the van der Pol oscillator is completely synchronized to the Duffing resonator and their oscillations are also locked to the external driving force by a phase lag.


### 2.3. Stability Analysis

The frequency-amplitude relation for weak coupling and strong coupling is, respectively, governed by (2.8a)-(2.8b) and (2.16). By varying the frequency detuning σ, the amplitudes (a1 and a2) are computed numerically with other parameters provided. Figure 1 shows a frequency response for a weakly coupled system. The amplitude of the Duffing resonator bends towards the higher frequency side like a normal Duffing resonator with a hardening cubic stiffness, but there is another antiresonance peak in addition to the hysteresis domain. Interestingly, even though the van der Pol oscillator is weakly connected to the Duffing resonator, its dynamic behaviour is strongly affected by the Duffing resonator as shown in Figure 1.Figure 1
The frequency-amplitude curves of the system when the van der Pol oscillator is weakly coupled to the Duffing resonator. The parameters are, respectively,c1=c2=0.001, k3=0.003, kc=0.002, and fd=0.002.The van der Pol response curve reveals a new behaviour. Its resonance is sharpened and a shoulder has been introduced at the location of the antiresonance of the Duffing resonator, but more relevant is the appearance of additional multiple hysteresis branches, denoting new characteristics of the weakly-coupled van der Pol oscillator.Are these branches stable or not? To answer this, the eigenvalues of the system's Jacobian matrixJac were evaluated at a pair of equilibrium points (ae1,ae2) which correspond to a pair of points in the frequency response curves of Figure 1 for the Duffing resonator and van der Pol oscillator, respectively. The eigenvalues of Jac determine linear stability of the equilibrium, which is asymptotically stable if all eigenvalues have negative real parts whereas it is unstable if at least one eigenvalue has positive real part. Figure 2 shows the stable (solid lines) and unstable (dotted lines) branches of the coupled system. As can be expected, the middle branches of the hysteresis for the Duffing resonator and van der Pol oscillator, respectively, are unstable for the system parameters that have been chosen. The system also displays interesting phenomena such as an antiresonance at Ω≈1 and a shoulder in the curve which is due to a stagnant response of the van der Pol oscillator. The stability of the system is further investigated numerically in the next section where an analysis of the time series is carried out using tools to study chaos in nonlinear dynamical systems. The oscillating states of the system at specific points on the branches are shown in Figure 9.The stability of the frequency-amplitude curves shown in Figure1 with the parameters of c1=c2=0.001, k3=0.003, kc=0.002, and fd=0.002.
(a)(b)For the case of strong coupling, the van der Pol oscillator is synchronized to the Duffing resonator and the coupled system oscillates like a single unit, exhibiting Duffing behaviour. This can be illustrated in Figure3 where the frequency response curve of the system is plotted to first-order approximation.Figure 3
The frequency-amplitude curves of the system when the van der Pol oscillator is strongly coupled to the Duffing resonator. The parameters are, respectively,c1=0.1, c2=0.05, k3=0.3, kc=8, and fd=0.2.Similarly, the stability was checked by calculating the eigenvalues of the corresponding Jacobian matrix of (2.15). Choosing several fixed points on one of the branches shown in Figure 3, we found that as in the case of normal Duffing resonators, the top and bottom branches are stable, while the middle branch is unstable. This is further verified by the transient simulation given in Section 4, where transitions between branches are observed.


## 2.1. The Resonant Case of Weak Coupling

When the van der Pol oscillator is weakly connected to the Duffing resonator, we rewrite (1.1) as follows:
(2.1)ẍ1+ϵμ1ẋ1+x1+ϵαx13=ϵβ(x2-x1)+ϵFcos(Ωτ),ẍ2+ϵμ2(x22-1)ẋ2+x2=ϵβ(x1-x2),
where c1=ϵμ1, c2=ϵμ2, k3=ϵα, kc=ϵβ, fd=ϵF, Ω=ωd/ω1 and ϵ is a small parameter.The stable response of the system driven near the primary resonance can be calculated from (2.1) using the standard two-time scales method [14]. Briefly, we introduce a fast scale τ0 (τ0=τ) and a slow scale τ1 (τ1=ϵτ0) characterizing the modulation in amplitudes and phases and seek solutions of (2.1) that are expressed in the form of an asymptotic expansion as follows: (2.2)x1=x10(τ0,τ1)+ϵx11(τ0,τ1),x2=x20(τ0,τ1)+ϵx21(τ0,τ1).Substituting (2.2) into (2.1) and equating coefficients of like powers of ϵ, we obtain that(2.3a)D02x10+x10=0,(2.3b)D02x20+x20=0,(2.3c)D02x11+x11=-2D0D1x10-μ1D0x10-αx103+β(x20-x10)+Fcos(Ωτ0),(2.3d)D02x21+x21=-2D0D1x20-μ2D0x20(x202-1)+β(x10-x20),where D0=∂/∂τ0 and D1=∂/∂τ1.The general solution of (2.3a) and (2.3b) can be expressed as
(2.4)x10=A1(τ1)eiτ0+c.c,x20=A2(τ1)eiτ0+c.c,
where A1 and A2 are arbitrary constants and c.c denotes the complex conjugate.Substitutingx10 and x20 into the right-hand side of (2.3c) and (2.3d), we obtain the following set of equations by imposing secular conditions: (2.5)2A1′+μ1A1-3iα|A1|2A1+iβ(A2-A1)-i2Feiστ1=0,2A2′+μ2(|A2|2-1)A2+iβ(A1-A2)=0.
We have introduced the frequency detuning σ to characterize the closeness of driving frequency to the fundamental frequency, given by Ω=1+ϵσ.ExpressingA1 and A2 in polar form:
(2.6)A1=a1eiθ1,A2=a2eiθ2,
and substituting the polar expressions into (2.5) and separating real and imaginary parts, we obtain the following coupled first-order differential equations:
(2.7)2a1′=-μ1a1+βa2sinγ2-F2sinγ1,2a2′=-μ2(a22-1)a2-βa1sinγ2,2a1γ1′=-(β-2σ)a1+3αa13-βa2cosγ2-F2cosγ1,2a2γ2′=(β-2σ)a2-βa1cosγ2-2a2γ1′,
where γ1=θ1-στ1 and γ2=θ2-θ1.To determine the steady-state motion, we use the condition thata1′=a2′=0 and γ1′=γ2′=0. From (2.7), we obtain the following set of algebraic equations, (2.8a)(a1(β-2σ)+3a13α-a22(β-2σ)a1)2+(a1μ1-a22μ2a1(1-a22))2=14F2,(2.8b)(β-2σ)2a22+μ22a22(1-a22)2=a12β2.Equation (2.8b) shows Duffing-type behaviour of the van der Pol oscillator, provided that the coupling and damping coefficients are not zero. If the coupling effect diminishes, then (2.8a) will be reduced to the frequency-amplitude modulation of a normal Duffing resonator.


## 2.2. The Resonant Case of Strong Coupling

If the coupling stiffnesskc is not the same order of magnitude as the other parameters, the analysis in Section 2.1 does not hold, so a modified analysis considering strong coupling is given as follows. When kc is larger than 4.5 for example, 1/(2kc+1) is less than 0.1. Therefore, We choose ϵ=1/(2kc+1) and assume all other coefficients are small as defined in Section 2.1. Then (1.1) can be rewritten as (2.9)ẍ1+ẍ2+ϵμ1ẋ1+ϵμ2(x22-1)ẋ2+x1+x2+ϵαx13=ϵFcos(Ωτ),ϵ(ẍ1-ẍ2)+ϵ2μ1ẋ1-ϵ2μ2(x22-1)ẋ2+x1-x2+ϵ2αx13=ϵ2Fcos(Ωτ).Repeating the same analysis in Section2.1, we obtain the solutions of (2.9) for the zero-order approximation as (2.10)D02(x10+x20)+x10+x20=0,(2.11)x10-x20=0.
Equation (2.11) means that the Duffing resonator and the van der Pol oscillator are completely synchronised. As shown in Section 2.1, we can easily write down the solutions of (2.10) and (2.11) as follows:
(2.12)x10=x20=Aeiτ+c.c.The first-order approximation gives(2.13)D02(x11+x21)+x11+x21=-2D1D0(x10+x20)-μ1D0x10-μ2(x202-1)D0x20-αx103+Fcos(Ωτ),x11-x21=0.Apparently, the Duffing resonator and the van der Pol oscillator are still completely synchronised in the first-order approximation when they are strongly coupled. Substituting the expressions ofx10 and x20 into the right-hand side of (2.13), we obtain the following equation by imposing secular conditions:(2.14)4A′+(μ1-μ2)A+μ2A|A|2-3iαA|A|2+i12Feiστ1=0.ExpressingA in polar form as defined in Section 2.1 (note that a1=a2=a, θ1=θ2 as (2.12) holds), and substituting into (2.14), we obtain the following set of first-order differential equations for the amplitude and phase:
(2.15)4a′=(μ2-μ1)a-μ2a3-12Fsinγ1,4aγ1′=-4aσ+3αa3-12Fcosγ1.
For the steady state solutions, we obtain the following algebraic equation describing the amplitude response of the system:(2.16)a2(-4σ+3αa2)2+a2(μ1-μ2+μ2a2)2=14F2.After eliminating the secular terms in the two-time scales analysis, the second-order differential equation, (2.13) can be solved. Accordingly, x11 and x21 are obtained as follows:
(2.17)x11=x21=116(α-μ1i)A3e3iτ+cc.
Therefore, the general solution of the strongly coupled Duffing resonator and van der Pol oscillator in the first-order approximation is given by(2.18)x1=x2=ℜ(x10+ϵx11)=(aei(Ωτ+γ)+116ϵ(α-μ2i)a3e3i(Ωτ+γ)+cc),
which shows that in the case of strong coupling, the van der Pol oscillator is completely synchronized to the Duffing resonator and their oscillations are also locked to the external driving force by a phase lag.


## 2.3. Stability Analysis

The frequency-amplitude relation for weak coupling and strong coupling is, respectively, governed by (2.8a)-(2.8b) and (2.16). By varying the frequency detuning σ, the amplitudes (a1 and a2) are computed numerically with other parameters provided. Figure 1 shows a frequency response for a weakly coupled system. The amplitude of the Duffing resonator bends towards the higher frequency side like a normal Duffing resonator with a hardening cubic stiffness, but there is another antiresonance peak in addition to the hysteresis domain. Interestingly, even though the van der Pol oscillator is weakly connected to the Duffing resonator, its dynamic behaviour is strongly affected by the Duffing resonator as shown in Figure 1.Figure 1
The frequency-amplitude curves of the system when the van der Pol oscillator is weakly coupled to the Duffing resonator. The parameters are, respectively,c1=c2=0.001, k3=0.003, kc=0.002, and fd=0.002.The van der Pol response curve reveals a new behaviour. Its resonance is sharpened and a shoulder has been introduced at the location of the antiresonance of the Duffing resonator, but more relevant is the appearance of additional multiple hysteresis branches, denoting new characteristics of the weakly-coupled van der Pol oscillator.Are these branches stable or not? To answer this, the eigenvalues of the system's Jacobian matrixJac were evaluated at a pair of equilibrium points (ae1,ae2) which correspond to a pair of points in the frequency response curves of Figure 1 for the Duffing resonator and van der Pol oscillator, respectively. The eigenvalues of Jac determine linear stability of the equilibrium, which is asymptotically stable if all eigenvalues have negative real parts whereas it is unstable if at least one eigenvalue has positive real part. Figure 2 shows the stable (solid lines) and unstable (dotted lines) branches of the coupled system. As can be expected, the middle branches of the hysteresis for the Duffing resonator and van der Pol oscillator, respectively, are unstable for the system parameters that have been chosen. The system also displays interesting phenomena such as an antiresonance at Ω≈1 and a shoulder in the curve which is due to a stagnant response of the van der Pol oscillator. The stability of the system is further investigated numerically in the next section where an analysis of the time series is carried out using tools to study chaos in nonlinear dynamical systems. The oscillating states of the system at specific points on the branches are shown in Figure 9.The stability of the frequency-amplitude curves shown in Figure1 with the parameters of c1=c2=0.001, k3=0.003, kc=0.002, and fd=0.002.
(a)(b)For the case of strong coupling, the van der Pol oscillator is synchronized to the Duffing resonator and the coupled system oscillates like a single unit, exhibiting Duffing behaviour. This can be illustrated in Figure3 where the frequency response curve of the system is plotted to first-order approximation.Figure 3
The frequency-amplitude curves of the system when the van der Pol oscillator is strongly coupled to the Duffing resonator. The parameters are, respectively,c1=0.1, c2=0.05, k3=0.3, kc=8, and fd=0.2.Similarly, the stability was checked by calculating the eigenvalues of the corresponding Jacobian matrix of (2.15). Choosing several fixed points on one of the branches shown in Figure 3, we found that as in the case of normal Duffing resonators, the top and bottom branches are stable, while the middle branch is unstable. This is further verified by the transient simulation given in Section 4, where transitions between branches are observed.


## 3. Bifurcation Analysis

In the two-time scales analysis in Section2, most coefficients of (1.1) are assumed small and of the same order. However, it is very interesting to know the dynamics of the system when the parameters vary in different ranges. In this section, the dependence of the system dynamics on its parameters are studied using a bifurcation analysis. We transform (1.1) into a set of first-order differential equations as follows:
(3.1)ẋ1=y1,ẏ1=-c1y1-x1-k3x13+kc(x2-x1)+fdcos(z),ẋ2=y2,ẏ2=-c2(x22-1)y2-x2+kc(x1-x2),ż=Ω,
where z=Ωτ=(ωd/ω1)τ and the internal resonance condition ω1=ω2 is applied.Usually, it is easy to adjust the driving force to change the behaviour of the coupled system once it is designed and physically constructed. Therefore, the frequency and the amplitude of the driving force are used as main control parameters in the bifurcation. For better visualisation of the attractors and their bifurcations the dynamics is investigated in the Poincaré section defined by,(3.2)∑={(x1,y1,x2,y2,z)∈R4×S1:z=const.}.
In order to investigate the dependence of the system on a single control parameter, several bifurcation diagrams have been computed.Each bifurcation diagram is calculated by changing the value of the control parameter in small steps. The last computed values (for a particular control parameter value) are used as a new set of initial conditions for the next control parameter value. Equation (3.1) with different driving frequencies is integrated using a fourth-order Runge-Kutta method with the step size of (2π/Ω)/40, where 2π/Ω is the period of the driving force. Numerical solutions corresponding to the first 500 driving cycles are removed as transient. The given bifurcation diagrams show the projection of the attractors in the Poincaré section onto the x1 and x2 coordinates versus the control parameter.Figure4 shows the symmetry breaking bifurcation of the periodically driven Duffing resonator coupled to a van der Pol oscillator. When the driving frequency Ω varies from 0.6 to 0.85, the system undergoes a period-one to a period-two and then to a period-one behaviour again. If the frequency of the driving force varies from 1.2 to 1.45, the coupled system suddenly enters into a chaotic state after a short range of period-one motion as shown in Figure 5 and then the system transits into period-one motion. There is a narrow window in the chaotic regime showing multiple period motion. If the damping coefficients c1 and c2 are decreased, a few more enlarged windows open up as shown in Figure 6, where the system has undergone period-one, chaotic, and multiple-period motion when the frequency varies. The transition between these different dynamics is justified by examining the Lyapunov exponents of the system shown in Figure 7, which shows the weak degree of chaos in specific windows of the driving frequency.Bifurcation diagram showing the coordinatex1 (a) and x2 (b) of the Poincaré Section versus the driving frequency in the range of 0.6→0.85 with parameters of c1=c2=0.1, k3=1, kc=5,  and fd=4.5.
(a)(b)Bifurcation diagram showing the coordinatex1 and x2 of the Poincaré section versus the driving frequency in the range of 1.2→1.45 with parameters of c1=c2=0.1, k3=1, kc=5, and fd=4.5.
(a)(b)Bifurcation diagram showing the coordinatex1 and x2 of the Poincaré section versus the driving frequency in the range of 1.2→1.45 with parameters of c1=c2=0.01, k3=1, kc=5, and fd=4.5.
(a)(b)Figure 7
Largest Lyapunov Exponent (LLE) for Figure6.For a single Duffing resonator, there is a critical value of the driving force which can drive it from the simple regime to the chaotic regime. The external force will also influence the van der Pol oscillator through the elastic coupling. As shown in Figure6, the system experiences a multiple-periods motion at the frequency 1.325. Using the same parameters, we investigated the effect of the driving force by varying its amplitude from 0.1 to 10. As shown in Figure 8, the system exhibits complex behaviour when the force changes.Bifurcation diagram showing the coordinatex1 (a) and x2 (b) of the Poincaré section versus the amplitude of driving force. The frequency of driving force is 1.325 and the initial conditions are x1(0)=1, ẋ1(0)=0, x2(0)=0, ẋ2(0)=0 with other parameters are c1=c2=0.1, k3=1, and kc=5.
(a)(b)Poincaré section of the Duffing Resonator (a) and the van der Pol oscillator (b) with the parameters used in Figure1. The frequency Ω is equal to 1.01 where six branches of the frequency response curve are expected and the initial conditions for transient analysis are x1(0)=1.05703, ẋ1(0)=0, x2(0)=0.11727, ẋ2(0)=0 with other parameters are c1=c2=0.1, k3=1, and kc=5.
(a)(b)


## 4. Dynamics of the Coupled System

The dynamics of the coupled system was studied by integrating (1.1) directly using the fourth-order Runge-Kutta method. As indicated in Section 2.1, the weakly coupled Duffing-van der Pol system has complicated dynamics. Using the parameters in Figure 1 and choosing the frequency Ω at 1.01, where stable and unstable branches of the frequency response curves coexist, we computed the transient motion of the Duffing resonator and van der Pol oscillator. The Poincaré section in Figure 9 shows the system converges to an attractor after a long transient motion and the system shows weak chaos with the largest Lyapunov exponent being about 0.007.When the coupling stiffness becomes stronger, the van der Pol oscillator quickly synchronizes to, and behaves like the Duffing resonator. The numerical experiment of sweeping the frequency of the driving force clearly illustrates a jumping/hysteresis phenomenon as shown in Figure10, which is further confirmation of the two-times-scale analysis in Section 2.Van der Pol oscillator (b) is synchronized to the Duffing resonator (a) and behaves like a normal Duffing resonator showing a hysteresis curve and jumping phenomena whenΩ varies between 0.6 and 1.4 with the initial conditions of x1(0)=1, ẋ1(0)=0, x2(0)=0, ẋ2(0)=0 and the parameters of the system are, respectively, c1=0.1, c2=0.05, k3=0.3, kc=8, and fd=0.2.
(a)(b)


## 5. Conclusion

In this paper, we have studied the dynamics of a coupled nonlinear system consisting of a van der Pol oscillator coupled to a periodically driven Duffing resonator, both of which show different attractors individually. The competition between the two different attractors depends upon the coupling constant and the control parameters.In the strong coupling regime, dominating synchronization is observed, where the van der Pol oscillator is locked to the behaviour of the Duffing resonator.The weak coupling regime reveals a multitude of complex behaviours, including multiperiod transitions and weakly chaotic motion which was confirmed by an analysis of Lyapunov exponents of the system Jacobian. We have also observed, multistable branches in the asymptotic amplitude-frequency response curves, and also an antiresonance in the Duffing response leading to a sharpening and a shoulder in the van der Pol response curve.These unexpected characteristics will have profound consequences when we construct chains and arrays composed of repeated units of coupled Duffing and van der Pol systems. Arrays of such components could have practical use as compact and resilient sensor arrays, for example. However the response of a sensor array of such coupled subsystems is likely to have a complexity of response characteristics beyond normal expectations of current sensor arrays. The next challenge will be in designing sensor arrays based on these subsystems which utilise this vast spectrum of computational behaviours.



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*Source: 248328-2010-10-04.xml*