Research Article | Open Access

Ping Zhou, Meihua Ke, "A New 3D Autonomous Continuous System with Two Isolated Chaotic Attractors and Its Topological Horseshoes", *Complexity*, vol. 2017, Article ID 4037682, 7 pages, 2017. https://doi.org/10.1155/2017/4037682

# A New 3D Autonomous Continuous System with Two Isolated Chaotic Attractors and Its Topological Horseshoes

**Academic Editor:**Dimitri Volchenkov

#### Abstract

Based on the 3D autonomous continuous Lü chaotic system, a new 3D autonomous continuous chaotic system is proposed in this paper, and there are coexisting chaotic attractors in the 3D autonomous continuous chaotic system. Moreover, there are no overlaps between the coexisting chaotic attractors; that is, there are two isolated chaotic attractors (in this paper, named “positive attractor” and “negative attractor,” resp.). The “positive attractor” and “negative attractor” depend on the distance between the initial points (initial conditions) and the unstable equilibrium points. Furthermore, by means of topological horseshoes theory and numerical computation, the topological horseshoes in this 3D autonomous continuous system is found, and the topological entropy is obtained. These results indicate that the chaotic attractor emerges in the new 3D autonomous continuous system.

#### 1. Introduction

A very interesting phenomenon in nonlinear systems is the possibility of chaos. Chaotic systems have some typical characteristics including high irregularity, unpredictability, and complexity [1, 2]. In 1963, the first chaotic attractor in a smooth 3D autonomous continuous system was found by Lorenz, which is called Lorenz chaotic system [3]. As the first chaotic model, the Lorenz system reveals the complex and fundamental behaviors of the nonlinear dynamical systems. In 1999, Chen and Ueta reported another chaotic attractor in a smooth 3D autonomous continuous system named Chen chaotic system [4], which nevertheless is not topologically equivalent to Lorenz’s. Afterwards, Lü and Chen carefully discussed the 3D Lorenz chaotic system and the 3D Chen chaotic system and discovered another chaotic attractor in 2002, which is called 3D Lü chaotic system [5]. The 3D Lü chaotic attractor connects the 3D Lorenz attractor and 3D Chen attractor and represents the transition from one to the other. Moreover, research on chaotic systems has attracted more and more attention in the last few decades because of its great applications in many fields like secure communication [6], data encryption [7], power system protection [8], DC motor control [8–10], flow dynamics [11], and so on [12–18].

On the other hand, coexisting chaotic attractors have been reported in many nonlinear systems in the recent years [19–23]. In [20, 21], the coexisting chaotic attractors were found in some 4D smooth systems, and there are overlaps between the coexisting chaotic attractors. In [22], Kengne et al. reported a simple 3D autonomous jerk system with multiple attractors; the chaotic system in [22] belongs to the generalized Lü chaotic system family. In [23], Pham et al. found the coexisting chaotic attractors in a novel 3D autonomous no-equilibrium chaotic system, and there are overlaps between the coexisting chaotic attractors. The chaotic system in [23] belongs to the generalized Chen chaotic system family. However, there are few results on the relationship between the coexisting chaotic attractor and the initial conditions.

Motivated by the above discussions, a new 3D autonomous continuous chaotic system that has two isolated chaotic attractors (two disconnected chaotic attractors) is reported in this paper. Some basic dynamics behaviors of the new chaotic system such as dissipative, Lyapunov exponents spectrum, bifurcation diagram, and phase diagram are obtained. It can be found that this new chaotic system has two isolated chaotic attractors or two disconnected chaotic attractors (named “positive attractor” and “negative attractor” in this paper), which depend on the distance between the initial points (initial conditions) and the unstable equilibrium points. The necessary condition for “positive attractor” or “negative attractor” is obtained. Furthermore, the horseshoes and entropy in this 3D chaotic system are also discussed by means of topological horseshoes theory and numerical computation.

The outline of our paper is organized as follows. In Section 2, a new 3D autonomous continuous chaotic system is addressed, and some basic dynamics behaviors of the new chaotic system are yielded. In Section 3, the horseshoes and entropy for the 3D chaotic system are investigated. In Section 4, the conclusion is given.

#### 2. A New 3D Autonomous Continuous Chaotic System

Normally, the 3D autonomous continuous chaotic systems can be described by . Here, is the state vector, is the nonlinear term of the 3D autonomous continuous chaotic system, and the constant matrix is determined by the linear part of the 3D autonomous chaotic system. According to the results [24] reported by Vanecek and Celikovsk, the 3D autonomous continuous Lorenz chaotic system satisfies , the 3D autonomous continuous Chen chaotic system satisfies , and the 3D autonomous continuous Lü chaotic system satisfies . One can obtain that the chaotic system in [22] satisfies , and the chaotic system in [23] satisfies . In this section, a new 3D autonomous continuous chaotic system that satisfies will be discussed.

The 3D Lü chaotic system [5] is described as follows:where , , , and .

Now, based on the 3D Lü chaotic system (1), a new 3D autonomous continuous system that satisfies is presented, and it is shown as follows:where . The second and third equations in system (2) are similar to the second and third equations in system (1), respectively. But, the first equation in system (2) is different from the first equation in system (1). Obviously, in system (2). So, system (2) is different from the 3D Lü chaotic system (1).

It is easily yielded that . So, the new system (2) is a dissipative system, and it can experience or develop attractors.

First, the Lyapunov exponents spectrum of system (2) with respect to parameter can be obtained by numerical calculation, which is displayed in Figure 1.

According to Figure 1, the maximum Lyapunov exponent is positive for , , , , and . Therefore, the chaotic attractor emerges in system (2) for suitable system parameter .

Now, setting the parameter , the five unstable equilibrium points in system (2) are , , , , and , respectively. The Lyapunov exponents are , , and , respectively. The Lyapunov dimension is ; this result means that system (2) is fractal. Therefore, the chaotic attractor emerges in system (2) for parameter . By numerical calculation, it can be found that there are two isolated chaotic attractors, which depend on the initial conditions. After a large number of numerical calculations, one has that the chaotic attractor depends on the distance between the initial points and the unstable equilibrium points (, , , and ). Some results are shown as follows:

(1) When the initial point is closed to the unstable equilibrium point or , the new system (2) has the same chaotic attractor. This attractor is named “positive attractor” in this paper, which refers to . A necessary condition for a “positive attractor” is .

(2) When the initial point is closed to the unstable equilibrium point or , the new system (2) has the same attractor. This attractor is named “negative attractor” in this paper, which refers to . A necessary condition for a “negative attractor” is .

Next, choose some initial conditions, for example.

*Case 1 (the initial point is closed to unstable equilibrium point ). *Let the initial conditions be (2, 2, 2). The distance between this initial point and unstable equilibrium points , , , and is 1.8464, 6.7420, 6.9944, and 7.0215, respectively. Therefore, the initial point is closed to unstable equilibrium point . So, the new system (2) has the “positive attractor,” which is shown in Figure 2.

*Case 2 (the initial point is closed to unstable equilibrium point ). *Let the initial conditions be (−2, −2, 2). The distance between this initial point and unstable equilibrium points , , , and is 6.7420, 1.8464, 7.0215, and 6.9944, respectively. Therefore, the initial point is closed to unstable equilibrium point . So, the new system (2) has the “negative attractor,” which is displayed in Figure 3.

*Case 3 (the initial point is closed to unstable equilibrium point ). *Let the initial conditions be (3, −3, −2). The distance between this initial point and unstable equilibrium points , , , and is 5.6257, 7.3097, 0.7266, and 9.2092, respectively. Therefore, the initial point is closed to unstable equilibrium point . So, the new system (2) has the “positive attractor,” which is shown in Figure 4.

*Case 4 (the initial point is closed to unstable equilibrium point ). *Let the initial conditions be (−3, 3, −2). The distance between this initial point and unstable equilibrium points , , , and is 7.3097, 5.6257, 9.2092, and 0.7266, respectively. Therefore, the initial point is closed to unstable equilibrium point . So, the new system (2) has the “negative attractor,” which is displayed in Figure 5.

According to Figures 2, 3, 4, and 5, we can obtain that the new system (2) has two isolated chaotic regions: one is named “positive attractor” and other one is named “negative attractor” in this paper. It is worth mentioning that there are also two isolated chaotic attractors for any other parameter . For example, let ; the Lyapunov exponents of system (2) are , , and , respectively. Two isolated chaotic attractors in the new system (2) are shown as Figure 6, where the initial conditions of “positive attractor” and “negative attractor” are (3, −3, −2) and (−3, 3, −2), respectively.

In addition, let ; the Lyapunov exponents of system (2) are , , and , respectively. So, there is no chaotic attractor, and there is periodic orbit which is shown in Figure 7.

Finally, the bifurcation diagram of variables and with respect to parameter is displayed in Figure 8. It can be observed that the bifurcation diagram coincides well with the Lyapunov exponents spectrum.

*Remark 1. *Obviously, the Lü chaotic system (1) and system (2) in this paper are invariant under the transformation →. However, the geometries of chaotic attractors of the Lü chaotic system (1) and system (2) are quite different. Firstly, for a given initial condition, the state variable in the Lü chaotic system (1) can be greater than zero or less than zero. Conversely, the state variable in system (2) can only be greater than zero or can only be less than zero. Secondly, for arbitrary initial conditions, the state variable in the Lü chaotic system (1) can only be greater than zero. Conversely, the state variable in system (2) can be greater than zero or can be less than zero.

#### 3. Horseshoes and Entropy in New Chaotic System (2)

First, some theoretical criteria of topological horseshoes are recalled.

Let be a metric space, is a compact subset of , and : is a map satisfying the assumption that there exist mutually disjoint compact subsets of ; the restriction of to each , that is, , is continuous.

*Definition 2 (see [25]). *For each , let and be two fixed disjoint compact subsets of . A connected subset of is said to connect and , if and , and we denote this by *↔*.

*Definition 3 (see [25]). *Let be a connected subset; we say that is suitably across with respect to and , if contains a connected subset such that , , and; that is, . In this case, we denote it by . In case that holds true for every connected subset with , we say that is suitably across with respect to two pairs and , or in case of no confusion.

Theorem 4 (see [26]). *Suppose that the map satisfies the following assumptions:**(1) There exist mutually disjoint compact subsets of ; is continuous.**(2) The relation holds for every pair with taken from . Then there exists a compact invariant set , such that is semiconjugate to the full -shift dynamics , and the topological entropy is .*

*Remark 5. *The -shift is also called the Bernoulli -shift. The symbolic series space is the collection of all bi-infinite sequences:where . The shift map is defined asIt is well known that is a Cantor set, which is compact, totally disconnected, and perfect. As a dynamical system defined on , has a countable infinity of periodic orbits consisting of orbits of all periods, an uncountable infinity of periodic orbits, and a dense orbit. A direct consequence of these three properties is that the dynamics generated by the shift map are sensitive to initial conditions. Mathematically, the topological entropy measures its complexity, which roughly means the exponential growth rate of the number of distinguishable orbits as time advances. When , ; therefore the system is chaotic. For more details of the above symbolic dynamics and horseshoes theory, we refer the reader to [25–28].

Corollary 6 (see [27]). *If , , , and , then there exists a compact invariant set , such that is semiconjugate to 2-shift dynamics, and .*

In order to find a horseshoes in system (2) with parameter and initial conditions (−2, −2, 2), we will first utilize the technique of cross section and the corresponding Poincaré map. By taking the setas a Poincaré section plane, we chose the corresponding Poincaré map as follows: for each , is taken to be the first return point in under the flow with the initial condition . Then, we use a MATLAB GUI program called “A toolbox for finding horseshoes in 2D map” [27]. After many attempts, we find a topological horseshoes by a similar method proposed in [27], as shown in Figure 9.

As shown in Figure 10, we find two subsets and , where the coordinates of four vertices of are and the coordinates of four vertices of are

**(a)**

**(b)**

Numerical computation shows that the two subsets under are continuous, and their images are illustrated in Figures 10(a) and 10(b), respectively.

It is easy to see from Figure 10(a) that passes through and between their top and bottom sides and transversely intersects with and and intersects with and . So each connected subset , if it is connection of and , then its images under must be across with respect to and and across with respect to and . Then we have and . Similarly, we have from Figure 10(b) too.

According to the topological horseshoes Corollary 6, there exists a compact invariant set , such that is semiconjugate to 2-shift dynamics and the topological entropy of is , which indicates that the map is chaotic indeed.

By the same way, a horseshoes in system (2) with parameter and initial conditions (2, 2, 2) can be obtained. Therefore, the chaotic attractor emerges in system (2) for parameter .

#### 4. Conclusions

In this paper, a 3D chaotic system satisfying is suggested. Some basic dynamics behaviors such as dissipative, Lyapunov exponents spectrum, bifurcation diagram, and phase diagram are obtained. The coexisting chaotic attractors are found in this 3D chaotic system, and there are two isolated chaotic attractors (named “positive attractor” and “negative attractor,” resp.) that depend on the distance between the initial points and the unstable equilibrium points. There are no overlaps between the “positive attractor” and “negative attractor.”

Furthermore, by means of topological horseshoes theory and numerical computation, a horseshoes in system (2) with parameter is obtained. Meanwhile, we obtained that the topological entropy is . These results indicate that the chaotic attractor emerges in system (2) for parameter .

#### Conflicts of Interest

The authors declare that there are no conflicts of interest regarding the publication of this paper.

#### References

- G. R. Chen and X. Dong,
*From Chaos to order Perspectives, Methodologies and Applications*, World Scientific, Singapore, 1998. - J. C. Sprott,
*Chaos and Time-Series Analysis*, Oxford University Press, New York, NY, USA, 2003. View at: MathSciNet - E. N. Lorenz, “Deterministic nonperiodic flow,”
*Journal of the Atmospheric Sciences*, vol. 20, no. 2, pp. 130–141, 1963. View at: Publisher Site | Google Scholar - G. Chen and T. Ueta, “Yet another chaotic attractor,”
*International Journal of Bifurcation and Chaos*, vol. 9, no. 7, pp. 1465-1466, 1999. View at: Publisher Site | Google Scholar | MathSciNet - J. Lü and G. Chen, “A new chaotic attractor coined,”
*International Journal of Bifurcation and Chaos*, vol. 12, no. 3, pp. 659–661, 2002. View at: Publisher Site | Google Scholar | MathSciNet - A. N. Miliou, I. P. Antoniades, S. G. Stavrinides, and A. N. Anagnostopoulos, “Secure communication by chaotic synchronization: robustness under noisy conditions,”
*Nonlinear Analysis: Real World Applications*, vol. 8, no. 3, pp. 1003–1012, 2007. View at: Publisher Site | Google Scholar | MathSciNet - P. Muthukumar, P. Balasubramaniam, and K. Ratnavelu, “Synchronization of a novel fractional order stretch-twist-fold (STF) flow chaotic system and its application to a new authenticated encryption scheme (AES),”
*Nonlinear Dynamics*, vol. 77, p. 1547, 2014. View at: Publisher Site | Google Scholar - J. Ni, C. Liu, K. Liu, and X. Pang, “Variable speed synergetic control for chaotic oscillation in power system,”
*Nonlinear Dynamics*, vol. 78, no. 1, pp. 681–690, 2014. View at: Publisher Site | Google Scholar - D. Q. Wei, L. Wan, X. S. Luo, S. Y. Zeng, and B. Zhang, “Global exponential stabilization for chaotic brushless DC motors with a single input,”
*Nonlinear Dynamics*, vol. 77, no. 1-2, pp. 209–212, 2014. View at: Publisher Site | Google Scholar - P. Zhou, R. J. Bai, and J. M. Zheng, “Stabilization of a fractional-order chaotic brushless DC motor via a single input,”
*Nonlinear Dynamics*, vol. 82, no. 1-2, pp. 519–525, 2015. View at: Publisher Site | Google Scholar - J. M. Ottino, F. J. Muzzio, M. Tjahjadi, J. G. Franjione, S. C. Jana, and H. A. Kusch, “Chaos, symmetry, and self-similarity: exploiting order and disorder in mixing processes,”
*Science*, vol. 257, no. 5071, pp. 754–760, 1992. View at: Publisher Site | Google Scholar - T. Yang and L. O. Chua, “Impulsive stabilization for control and synchronization of chaotic systems: theory and application to secure communication,”
*IEEE Transactions on Circuits and Systems I: Fundamental Theory and Applications*, vol. 44, no. 10, pp. 976–988, 1997. View at: Publisher Site | Google Scholar | MathSciNet - E. Montbrió, J. Kurths, and B. Blasius, “Synchronization of two interacting populations of oscillators,”
*Physical Review E: Statistical, Nonlinear, and Soft Matter Physics*, vol. 70, Article ID 056125, 2004. View at: Publisher Site | Google Scholar - Y. Feng, Z. Wei, U. E. Kocamaz, A. Akgül, and I. Moroz, “Synchronization and electronic circuit application of hidden hyperchaos in a four-dimensional self-exciting homopolar disc dynamo without equilibria,”
*Complexity*, vol. 2017, Article ID 7101927, 11 pages, 2017. View at: Publisher Site | Google Scholar | MathSciNet - J. Ma, F. Wu, G. Ren, and J. Tang, “A class of initials-dependent dynamical systems,”
*Applied Mathematics and Computation*, vol. 298, pp. 65–76, 2017. View at: Publisher Site | Google Scholar | MathSciNet - C. Wang, R. Chu, and J. Ma, “Controlling a chaotic resonator by means of dynamic track control,”
*Complexity*, vol. 21, no. 1, pp. 370–378, 2015. View at: Publisher Site | Google Scholar | MathSciNet - M. Lv, C. Wang, G. Ren, J. Ma, and X. Song, “Model of electrical activity in a neuron under magnetic flow effect,”
*Nonlinear Dynamics*, vol. 85, no. 3, pp. 1479–1490, 2016. View at: Publisher Site | Google Scholar - M. Lv and J. Ma, “Multiple modes of electrical activities in a new neuron model under electromagnetic radiation,”
*Neurocomputing*, vol. 205, pp. 375–381, 2016. View at: Publisher Site | Google Scholar - J. Argyris and I. Andreadis, “On the influence of noise on the coexistence of chaotic attractors,”
*Chaos, Solitons & Fractals*, vol. 11, no. 6, pp. 941–946, 2000. View at: Publisher Site | Google Scholar - F. Yuan, G. Wang, Y. Shen, and X. Wang, “Coexisting attractors in a memcapacitor-based chaotic oscillator,”
*Nonlinear Dynamics*, vol. 86, no. 1, pp. 37–50, 2016. View at: Publisher Site | Google Scholar - Q. Lai and S. Chen, “Coexisting attractors generated from a new 4D smooth chaotic system,”
*International Journal of Control, Automation, and Systems*, vol. 14, no. 4, pp. 1124–1131, 2016. View at: Publisher Site | Google Scholar - J. Kengne, Z. T. Njitacke, and H. B. Fotsin, “Dynamical analysis of a simple autonomous jerk system with multiple attractors,”
*Nonlinear Dynamics*, vol. 83, p. 751, 2016. View at: Google Scholar - V.-T. Pham, C. Volos, S. Jafari, and T. Kapitaniak, “Coexistence of hidden chaotic attractors in a novel no-equilibrium system,”
*Nonlinear Dynamics*, vol. 87, no. 3, pp. 2001–2010, 2017. View at: Publisher Site | Google Scholar - A. Vanecek and S. Celikovsk,
*Control Systems: From Linear Analysis to Synthesis of Chaos*, Pretice-Hall, London, UK, 1996. - X.-S. Yang, “Topological horseshoes and computer assisted verification of chaotic dynamics,”
*International Journal of Bifurcation and Chaos*, vol. 19, no. 4, pp. 1127–1145, 2009. View at: Publisher Site | Google Scholar | MathSciNet - X.-S. Yang, H. Li, and Y. Huang, “A planar topological horseshoe theory with applications to computer verifications of chaos,”
*Journal of Physics A: Mathematical and General*, vol. 38, no. 19, pp. 4175–4185, 2005. View at: Publisher Site | Google Scholar | MathSciNet - Q. Li and X.-S. Yang, “A simple method for finding topological horseshoes,”
*International Journal of Bifurcation and Chaos*, vol. 20, no. 2, pp. 467–478, 2010. View at: Publisher Site | Google Scholar | MathSciNet - X.-S. Yang and Y. Tang, “Horseshoes in piecewise continuous maps,”
*Chaos, Solitons & Fractals*, vol. 19, no. 4, pp. 841–845, 2004. View at: Publisher Site | Google Scholar

#### Copyright

Copyright © 2017 Ping Zhou and Meihua Ke. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.