Negative Mass in the Systems Driven by Entropic Forces

1. Introduction

Entropic forces are emergent forces that arise from the statistical tendency of a system to increase its entropy [1,2]. Unlike other fundamental forces (like gravity or electromagnetism), entropic forces originate from the system’s tendency to maximize the number of accessible microstates [3]. Entropic origin of these forces represents the tendency of a system to evolve into a more probable state, rather than simply into one of lower potential energy [1]. Elasticity of polymers is driven to a much extent by entropy [4,5,6,7]. Maximizing entropy of a polymer chain implies reducing the distance between its two free ends. Consequently, an entropic elastic force emerges, that tends to collapse the chain. Elasticity of the muscles arises from entropy in a way very similar to the entropy-driven elasticity of polymer chains [8]. Entropic forces drive contraction of cytoskeletal networks [9]. Verlinde suggested that gravity is actually the entropic force [10]. According to Verlinde, gravity emerges from fundamental principles of statistical mechanics and information theory rather than being a fundamental interaction like electromagnetism. His idea is rooted in holographic principle and thermodynamics [10]. Verlinde showed that if information about matter is stored on a holographic screen (a surface encoding information about space), then the tendency of entropy to maximize leads to an effect that mimics Newton’s law of gravity [10]. In a similar way the Coulomb interaction was treated as an entropic force [11].

Usually, entropic forces grow with temperature, however, the exceptions to this rule were reported, when the system of elementary magnets supposed to be in the thermal equilibrium with the thermal bath is exposed to external magnetic field [12].

Our paper addresses the situation when the entropic/polymer spring gives rise to the effect of the negative mass). The effect of the negative mass is a resonance effect, emerging in core-shell mechanical systems. This effect occurs when the frequency of the harmonic external force acting on core-shell system connected by a Hookean massless spring, approaches from above to the eigen-frequency of the system [13,14,15,16,17]. Negative-inertia converters for both translational and rotational motion were introduced [18].

The energy of the vibrated core-shell system is not conserved, due to the fact that it is exposed to the external harmonic force, as it occurs, for example, in the famous Kapitza pendulum, in which the pivot point vibrates in a vertical direction, up and down [19,20]. 2020). Unlike the Kapitza pendulum, the effect of “negative effective mass” arises in the linear approximation to the analysis of the motion [13,14,15,21]. The effect of the negative effective mass/negative effective density may be achieved with the plasma oscillations of the free electron gas in metals [22,23,24].

The effects of negative mass and negative density gave rise to the novel mechanic and thermal metamaterials [25,26,27]. The negative effective mass materials were manufactured by dispersion of soft silicon rubber coated heavy spheres in epoxy, acting as the mechanical resonators [13]. The negative density metamaterial was manufactured in an aluminum plate, comprising the resonant structure [28]. Soft 3D acoustic metamaterials polymer materials demonstrating negative effective density were reported [29]. Our paper is devoted to the possibility of realization of negative mass/density metamaterials exploiting entropic elastic forces.

2. Materials and Methods

Numerical calculations were performed with the Wolfram Mathematica software

3. Results

3.1. Negative Mass in the Core-Shell System Driven by Entropic Elastic Force

Consider the core-shell mechanical system, depicted in Figure 1. The core mass m is connected to the shell M with two polymer stripes/springs. The entire system is subjected to the external sinusoidal force $Im\left(\widehat{F}\left(t\right)\right)=F_{0x}sin\omega t$, as shown in Figure 1. We assume that the masses of the polymer stripes are much smaller than both masses of the core and shell; thus, the masses of polymer springs are negligible. The core-shell system may be replaced with a single effective mass $m_{eff}$ expressed with Eq. 1 (for the rigorous derivation of Eq. 1, see: [14,15,16,21,22].

$$m_{eff}=M+{\displaystyle \frac{m{\omega }_0^2}{{\omega }_0^2-{\omega }^2}},$$

(1)

where ${\omega }_0=\sqrt{{\displaystyle \frac{2k}{m}}}$, and k is the elastic constant of the polymer stripe (the core mass is driven by the pair of polymer springs).

.

It is easily seen from Eq. 1 that, when the frequency ω approaches ${\omega }_0$ from above, the effective mass $m_{eff}$ will be negative [14,15,16,21,22]. For the sake of simplicity we assume that the polymer stripe/spring is built of ξ identical polymer chains, each of which may be represented by the ideal Kuhn equivalent freely jointed chain, built of N Kuhn monomers, the Kuhn length of the monomer is b [5]. The elastic constant k of the polymer spring is given by Eq. 2:

$$k=3\xi {\displaystyle \frac{k_{B}T}{N{b}^2}},$$

(2)

where $k_B$ is the Boltzmann constant, and T is the temperature; we assume that the temperature is constant along the addressed core-shell system [5]. Substitution of Eq. 2 into Eq. 1 yields for the effective mass of the entire core-shell system (the masses of the polymer springs are neglected):

$$m_{eff}\left(\omega ,T\right)=M+{\displaystyle \frac{\frac{6\xi k_{B}T}{N{b}^2}}{\frac{6\xi }{m}\frac{k_{B}T}{N{b}^2}-{\omega }^2}}$$

(3)

Now we fix the frequency of the external force ω, and vary the temperature of the core-shell system T. It is easily seen, that the effective mass $m_{eff}\left(\omega ,T\right)$ becomes negative when the temperature of the core-shell system approaches the critical temperature $T^{*}$ from below, where $T^{*}$ is given by Eq. 4:

$$T^{*}={\displaystyle \frac{mN{\left(b\omega \right)}^2}{6\xi k_B}}$$

(4)

The dependence $m_{eff}\left(T\right)$ is presented in Figure 2 (the value of ω is fixed). It is instructive to calculate the asymptotic values of $m_{eff}\left(T\right)$. When, $T\gg T^{*}$ we derive from Eq 3.

$$\underset{T\gg T^{*}}{\lim }{m}_{eff}\left(T\right)=M+m$$

(6)

which is intuitively clear for an infinitively stiff spring. The low-temperature limit of the effective mass is also easily calculated.

$$\underset{T\ll T^{*}}{\lim }{m}_{eff}\left(T\right)=M$$

(7)

Eq. 7 is also intuitively clear; indeed, the influence of the “weak” polymer spring (the temperatures are low) becomes negligible.

3.2. Negative Density of the Chain of Core-Shell Systems Driven by Elastic Forces

The concept of negative resonant density emerging in the chain of core-shell units, depicted in Figure 3, was introduced [22]. The effective density of the chain depicted in Figure 3; ${\rho }_{eff}\left(\omega \right)$, was calculated in [22]; and it is given by Eq. 8:

$${{\rho }_{eff}\left(\omega \right)=\rho }_{st }{\displaystyle \frac{\theta }{\delta \left(1+\theta \right){\left(\frac{\omega }{{\omega }_0}\right)}^2}} {\left\{{cos}^{-1}\left\{1-{\displaystyle \frac{\delta }{2\theta }}{\displaystyle \frac{{\left(\frac{\omega }{{\omega }_0}\right)}^2\left[{\left(\frac{\omega }{{\omega }_0}\right)}^2-\left(1+\theta \right)\right]}{{\left(\frac{\omega }{{\omega }_0}\right)}^2-1}}\right\}\right\}}^2$$

(8)

where $m_1$ and $m_2$ are the masses of the shell and core correspondingly, the static linear density of the chain ${\rho }_{st}$ is given by: ${\rho }_{st}={\displaystyle \frac{m_1+m_2}{a}}$; $\left[{\rho }_{st}\right]={\displaystyle \frac{kg}{m}}$ and $\theta ={\displaystyle \frac{m_2}{m_1}}$; $\delta ={\displaystyle \frac{k_2}{k_1}}$; and a is the lattice constant (see Figure 3), ${\omega }_0=\sqrt{{\displaystyle \frac{k_2}{m_2}}}$. It was demonstrated that the effective density becomes negative, when the frequency of external force ω approaches ${\omega }_0$ from above [22].

Now we assume that both of the springs are polymer stripes. The elasticity of the stripes is given by Eqs. 9-10 [5]:

$$k_1=3{\xi }_1{\displaystyle \frac{k_{B}T}{N_1{b}_1^2}}={\alpha }_{1}T,$$

(9)

$$k_2=3{\xi }_2{\displaystyle \frac{k_{B}T}{N_2{b}_2^2}}={\alpha }_{2}T,$$

(10)

where ${\xi }_i,N_i,b_i, i=\mathrm{1,2}$ are the numbers and parameters of the Kuhn chains, constituting the strings, ${\alpha }_i=3{\xi }_i{\displaystyle \frac{k_{B}T}{N_i{b}_i^2}}, i=\mathrm{1,2}$. It is noteworthy that the parameter; $\delta ={\displaystyle \frac{k_2}{k_1}}$ is temperature-independent. Thus, the squared resonant frequency ${\omega }_0^2$ is given by Eq. 11:

$${\omega }_0^2=3{\xi }_2{\displaystyle \frac{k_{B}T}{{m_{2}N}_2{b}_2^2}}={\alpha }_{2}T$$

(11)

where ${\alpha }_2=3{\xi }_2{\displaystyle \frac{k_B}{{m_{2}N}_2{b}_2^2}}$. Hence, the effective density of the chain appears as follows:

$${{\rho }_{eff}\left(\omega ,T\right)=\rho }_{st }{\displaystyle \frac{\theta }{\delta \left(1+\theta \right)\frac{{\omega }^2}{{\alpha }_{2}T}}} {\left\{{cos}^{-1}\left\{1-{\displaystyle \frac{\delta }{2\theta }}{\displaystyle \frac{\frac{{\omega }^2}{{\alpha }_{2}T}\left[\frac{{\omega }^2}{{\alpha }_{2}T}-\left(1+\theta \right)\right]}{\frac{{\omega }^2}{{\alpha }_{2}T}-1}}\right\}\right\}}^2$$

(12)

Now we fix the frequency of the external force ω. The plot ${\rho }_{eff}\left(T\right)$ is depicted in Figure 4. The graph is numerically built with Wolfram Mathematica software. The blue curve depicts the dependence ${\rho }_{eff}\left(\omega ,T\right)$ for the dimensionless parameters: $k_1=k_2=1\times T; m_1=1; \delta =1; \theta ={\displaystyle \frac{1}{{\alpha }_2}}; a=1; \omega =2.3; {\alpha }_2=0.05$.

It is recognized that ${\rho }_{eff}\left(T\right)$ becomes negative, when the temperature of the core-shell system approaches to the critical temperature $T^{*}$ from below, where $T^{*}$ is given by Eq. 13:

$$T^{*}={\displaystyle \frac{{\omega }^2}{{\alpha }_2}},$$

(13)

where ${\alpha }_2=3{\xi }_2{\displaystyle \frac{k_B}{{m_{2}N}_2{b}_2^2}}$. Set of the brown curves, appearing in Figure 4, depicts the temperature dependencies of the effective density ${\rho }_{eff}\left(T\right)$ calculated for the different values of ${0.04<\alpha }_2<0.08$. It is easily demonstrated that the high-temperature limit of the effective density is given by Eq. 14:

$$\underset{T\to \infty }{\lim }{\rho }_{eff}\left(\omega ,T\right)={\rho }_{st}={\displaystyle \frac{m_1+m_2}{a}},$$

(14)

which is well-expected for the massless, infinitely stiff springs.

Let’s vary the parameter $\delta$ in Eq. 12 from values close to zero to $\delta =2,$ namely $0.001<\delta <2$. Parameter $\delta ={\displaystyle \frac{k_2}{k_1}}$ quantifies relative stiffness of spring $k_2$ referred to the string $k_1.$ The variation of parameters ${\alpha }_2$ and $\delta$ is illustrated with Figure 5. Brown curves are built for the fixed $\delta =1$ and demonstrates change of ${\rho }_{eff}$ with $\omega$ for ${0.04<\alpha }_2<0.08$. Magenta curves, in turn, illustrate are built for fixed ${\alpha }_2=0.05$ and $0.001<\delta <2$.

Brown curves are built for the fixed $\delta =1$ and demonstrates change of ${\rho }_{eff}$ with $\omega$ for ${0.04<\alpha }_2<0.08$. The blue curve demonstrates ${\rho }_{eff}\left(T;\omega =2.3,{\alpha }_2=\mathrm{0,05}, \delta =1\right).$ The magenta curves illustrate variation in $0.001<\delta <2$ and depict ${\rho }_{eff}\left(T;\omega =2.3,{\alpha }_2=0.05, \delta \in \{0.001, 0.5, 1.1, 1.5, 2\}\right).$ Brown arrow depicts increase in ${\alpha }_2$; magenta arrow illustrates increase in $\delta .$

Figure 5 illustrates the very important result, decrease in $\delta ={\displaystyle \frac{k_2}{k_1}}$ leads to the sharpening of the resonance behavior of ${\rho }_{eff}\left(T\right)$ dependence. This result is intuitively quite understandable; indeed, increase in stiffness of the outer spring $k_1$ results in the sharpening of the resonance.

Let us explore the limit $\underset{\delta \to 0}{\lim }\left({\rho }_{eff}\left(T, \omega ,\delta \right)\right)$ in more detail. The limit of ${\rho }_{eff}\left(T, \omega \right)$ (see Eq. 12) as $\delta$ tends to zero is:

$$\underset{\delta \to 0}{\lim }\left({\rho }_{eff}\left(T, \omega ,\delta \right)\right)=1+{\displaystyle \frac{T}{{T\alpha }_2-{\omega }^2}}.$$

(15)

The dependence ${\rho }_{eff}\left(\delta \right)$ as calculated for different temperatures is depicted in Figure 6A. In the low temperature limit, when $T\ll {\displaystyle \frac{{\omega }^2}{{\alpha }_2}}$ and, $\delta \ll 1$ the effective density ${\rho }_{eff}\left(T, \omega \right)$ almost doesn’t change with $\delta ={\displaystyle \frac{k_2}{k_1}}$, as it is illustrated with Figure 6B.

Figure 6. A. The dependence ${\rho }_{eff}\left(\delta \right)$ is depicted for various temperatures T. curves ${\rho }_{eff}\left(\delta ;\omega =2.3,{\alpha }_2=\mathrm{0,05}, T\in [0.2, 190]\right)$ are depicted. B. As $\delta$ and T tend to zero ${\rho }_{eff}$ (for the dimensionless parameters) tends to 1, as it is expected from Eq. 15.

Figure 6. A. The dependence ${\rho }_{eff}\left(\delta \right)$ is depicted for various temperatures T. curves ${\rho }_{eff}\left(\delta ;\omega =2.3,{\alpha }_2=\mathrm{0,05}, T\in [0.2, 190]\right)$ are depicted. B. As $\delta$ and T tend to zero ${\rho }_{eff}$ (for the dimensionless parameters) tends to 1, as it is expected from Eq. 15.

Now we address a situation, when we remove the temperature dependence of the elasticity of the stripes (Eqs 9-10) one by one. The first case: $k_1\left(T\right)=T,$ $k_2=const\left(T\right)=1$. Then Eq. 12 with dimensionless parameters will transform to Eq. 16:

$${\rho }_{eff}\left(T;\omega ,{\alpha }_2\right)={\displaystyle \frac{T}{{\omega }^2}}{{cos}^{-1}[1-{\displaystyle \frac{{\omega }^2(-1-\frac{1}{{\alpha }_2}+\frac{{\omega }^2}{{\alpha }_2})}{2T(-1+\frac{{\omega }^2}{{\alpha }_2})}}]}^2$$

(16)

The dependence ${\rho }_{eff}\left(T\right)$ calculated for the different values of parameter ${\alpha }_2$ is illustrated with Figure 7.

Figure 7. Curves ${\rho }_{eff}\left({T;\alpha }_2\in \left\{0.04,0.05\left(Bluecurve\right),0.06,0.07,0.08\right\},\omega =2.3\right)$ are depicted. Black arrow depicts the increase in ${\alpha }_2$. $\underset{T\to \mathrm{\infty }}{\mathrm{Lim}}\left({\rho }_{eff}\left(T,\omega \right)\right)=1+{\displaystyle \frac{1}{{\alpha }_2-{\omega }^2}}.$

Figure 7. Curves ${\rho }_{eff}\left({T;\alpha }_2\in \left\{0.04,0.05\left(Bluecurve\right),0.06,0.07,0.08\right\},\omega =2.3\right)$ are depicted. Black arrow depicts the increase in ${\alpha }_2$. $\underset{T\to \mathrm{\infty }}{\mathrm{Lim}}\left({\rho }_{eff}\left(T,\omega \right)\right)=1+{\displaystyle \frac{1}{{\alpha }_2-{\omega }^2}}.$

The second case corresponds to $k_1=const\left(T\right)=1,$ $k_2\left(T\right)=T$. Then Eq. 12 with dimensionless parameters will transform to Eq. 17:

$${\rho }_{eff}\left(T, \omega \right)={\displaystyle \frac{1}{{\omega }^2}}{{cos}^{-1}[1-{\displaystyle \frac{{\omega }^2(-1-\frac{1}{\alpha 2}+\frac{{\omega }^2}{T\alpha 2})}{2(-1+\frac{{\omega }^2}{T\alpha 2})}}]}^2$$

(17)

The dependence ${\rho }_{eff}\left(T\right)$ calculated for the different values of parameter ${\alpha }_2$ is illustrated with Figure 8.

Figure 8. Here are curves ${\rho }_{eff}\left({T; \alpha }_2\in \left\{0.04, 0.05 \left(Blue\right), 0.06, 0.07, 0.08\right\}, \omega =2.3\right)$. The asymptotic behavior corresponds to $T={\displaystyle \frac{{\omega }^2}{{\alpha }_2}}$. Black arrow depicts the increase in ${\alpha }_2.$

Figure 8. Here are curves ${\rho }_{eff}\left({T; \alpha }_2\in \left\{0.04, 0.05 \left(Blue\right), 0.06, 0.07, 0.08\right\}, \omega =2.3\right)$. The asymptotic behavior corresponds to $T={\displaystyle \frac{{\omega }^2}{{\alpha }_2}}$. Black arrow depicts the increase in ${\alpha }_2.$

The field of negative densities is clearly recognized in Figure 8.

4. Discussion

Resonances are ubiquitous in nature and engineering [30,31,32]. It is well known, that the resonant phenomena may be temperature dependent. The temperature dependence of the resonance frequency of the fundamental and four higher order modes of a silicon dioxide micro-cantilever was established [33]. Temperature effects in resonant Raman spectroscopy were registered [34]. Temperature dependent Raman resonant response in $U{O}_2$ was reported [35]. The temperature dependence of the Fano resonance discovered in infrared spectra of nano-diamonds was discussed [36]. We address the temperature dependent resonant effects giving rise the phenomenon of the “negative effective mass effect”, exerted to the intensive research in the last decade.

It is unnecessary to say that actually there is no negative mass [22,37]. The phenomenon of the “negative effective mass” arises when we substitute the core-shell mechanical systems comprising a pair of masses (M and m) and the massless Hookean spring k by a single effective mass $m_{eff}$, that is to say that the internal mass m is hidden and its influence is expressed by the introduction of the mass $m_{eff}$ [14,15,16,22,37]. The negative effective mass represents the contra-intuitive situation of “anti-vibrations”, when the harmonic acceleration of the system is in an opposite direction to the sinusoidal applied force [14,15,16,21,22]. We considered the situation when the vibrations are driven by temperature-dependent entropic forces, inherent for natural and biological polymer systems [39]. The stiffness of the polymer spring is temperature-dependent, and the physical situation resembling the parametric resonance emerges, when the temperature is varied [38]. Thus, the temperature-dependent effective mass emerges. The effect may be exemplified with polymer acoustic meta-materials [29,40]. The temperature dependent effective mass is not a novel concept; it is broadly used in semiconductors [41]. However, in our analysis the effect of temperature dependent mass emerges from the entropic origin of the elastic force in resonant systems.

5. Conclusions

We conclude that the effect of the temperature-dependent effective mass becomes possible in the core-shell systems in which the spring connecting the core mass to the shell is driven by the temperature-dependent entropic elasticity, such as that inherent for polymer materials. The core-shell system may be replaced with a single effective mass $m_{eff}\left(\omega ,T\right)$ exposed to the external harmonic force. When the frequency of the external force ω is fixed and the temperature of the core-shell system T is varied, the resonance becomes possible, and the harmonic acceleration of the shell may move in an opposite direction to the applied force. We demonstrate that the effective mass $m_{eff}\left(T\right)$ becomes negative when the temperature of the core-shell system approaches to the critical temperature $T^{*}$ from below.

We also considered the chain/lattice built of core-shell units, in which entropic forces are acting. In this case, the effect of “negative density” is attainable under variation the temperature of the system. Again, the negative density ${\rho }_{eff}\left(T,\omega \right)$ becomes negative when the temperature of the core-shell system approaches the critical temperature $T^{*}$ from below. The critical temperature is defined by the parameters of polymer chain and frequency of the external force ω. We varied the parameters of the lattice built of the core-shell elements and connected with the elastic springs. Increase in the stiffness of the springs connecting the core-shell units, leads to the sharpening of the resonance behavior of ${\rho }_{eff}\left(T\right)$ dependence. We also addressed a situation, and calculated the resonance curves, when we removed the temperature dependence of the elasticity of the “inner” and “outer” elastic elements one by one. In the low temperature limit, the effective density ${\rho }_{eff}\left(T, \omega \right)$ almost doesn’t change with the ratio of the elastic constants of the “internal” and “external springs” appearing in the lattice. The effect may be demonstrated experimentally with polymer meta-materials.