Abstract
The excess lowfrequency vibrational spectrum, called boson peak, and nonaffine elastic response are the most important particularities of glasses. Herein, the vibrational and mechanical properties of polymeric glasses are examined by using coarsegrained molecular dynamics simulations, with particular attention to the effects of the bending rigidity of the polymer chains. As the rigidity increases, the system undergoes a glass transition at a higher temperature (under a constant pressure), which decreases the density of the glass phase. The elastic moduli, which are controlled by the decrease of the density and the increase of the rigidity, show a nonmonotonic dependence on the rigidity of the polymer chain that arises from the nonaffine component. Moreover, a clear boson peak is observed in the vibrational density of states, which depends on the macroscopic shear modulus G. In particular, the boson peak frequency ω_{BP} is proportional to \(\sqrt{G}\). These results provide a positive correlation between the boson peak, shear elasticity, and the glass transition temperature.
Introduction
Glasses show vibrational and mechanical properties that are markedly different from other crystalline materials^{1,2}. Thermal measurements and scattering experiments have been performed to study the properties of various glassy systems, such as covalentbonding^{3,4,5,6,7,8}, molecular^{9,10,11,12,13}, metallic^{14,15,16,17}, and polymeric^{18,19,20,21,22,23} glasses. For instance, the excess vibrational modes at low frequencies and the excess heat capacity at low temperatures exceeding the Debye predictions, which describe the corresponding crystalline values, have been observed universally in various glassy materials. This phenomenon, which is referred to as the boson peak (BP), has been widely studied.
The ideas of elastic heterogeneities^{24,25,26} and criticality near isostatic state and marginally stable state^{27,28,29,30} have been introduced, following the recent theoretical advances for understanding the origin of anomalies in glasses. Based on these theories, the meanfield formulations have been developed by using the effective medium technique^{24,25,26,29,30}. In addition, more recent studies^{31,32} have focused on the local inversionsymmetry breaking, which can explain the microscopic origin of the BP. The anomalous vibrational properties in both crystals and glasses have also been investigated within the framework of the phonon Green's function^{33}.
Molecular dynamics (MD) simulations play an essential role for studying the vibrational and mechanical properties of glasses. Firstly, MD simulations enable to assess the theoretical predictions. In fact, various MD simulations have been performed on simple atomic glasses, e.g., LennardJones (LJ) systems^{34,35,36,37,38,39,40}. Concerning the isostaticity and marginal stability^{27,28,29,30}, the systems with a finiteranged, purely repulsive potential have also been studied^{41,42,43,44}, and are considered as the simplest model of glasses. In particular, it is crucial for MD simulations to solve finitedimensional effects that are not captured by the meanfield treatments^{45,46,47}. Secondly, MD simulations perform quasiexperiments on welldefined systems and access data that cannot be examined experimentally. Relevant systems to experiments and applications have been simulated, including covalentbonding^{48,49,50,51,52,53}, metallic^{54,55,56,57}, polymeric^{58,59,60,61,62} glasses. These simulation studies complete theoretical understandings based on simple systems and experimental observations of more complex systems.
The vibrational properties and the BP of polymeric glasses have been studied by both of experiments^{18,19,20,21,22,23} and MD simulations^{58,59,60,61,62}. The effects caused by noncovalent bonds including bending forces and chain length represent an important feature of polymer glasses. Previous experiments^{18,19} have investigated the effects of the pressure or densification on the frequency and intensity of the BP in polymeric glasses. It was demonstrated that the evolution of the BP with pressure cannot be scaled by the Debye values (i.e., the Debye frequency and the Debye level). Therefore, the pressure effects cannot be explained only by the variation of macroscopic elasticity. In contrast, another experiment^{20} has shown that the polymerization effects on the BP is explained by the change in macroscopic elasticity as the frequency and intensity variations of the BP are both scaled by the Debye values.
In addition, Zaccone et al. have recently performed MD simulations to calculate the vibrational density of states (vDOS) in polymeric glasses by changing the chain length and the rigidity of the chain bending^{61}. This work studied the vibrational eigenstates in a wide range of frequencies and the effects of the chain length and bending rigidity on the highfrequency spectra. Furthermore, Giuntoli and Leporini studied the BP of polymeric glasses having chains with highly rigid bonds^{62}. It was demonstrated that the BP decouples with macroscopic elasticity and arises from nonbonding interactions only. Although these studies^{61,62} have helped understand polymeric glass properties, the effects of bending rigidity and chain length on the lowfrequency spectra and BP need to be further studied.
Herein, the vDOS and the elastic moduli of polymeric glasses are analyzed through coarsegrained MD simulations (see Methods). In particular, the connection between the BP and elasticity as well as the glass transition temperature is explored by systematically changing the bending stiffness of short and long polymer chains. The contributions of the present study are given as follows. We demonstrate that polymeric glasses can exhibit extremelylarge nonaffine elastic response (compared to atomic glasses), whereas the BP is simply scaled by the behavior of macroscopic shear modulus. This behavior of the BP can be explained by the theory of elastic heterogeneities^{24,25,26}. Our results indicate that effects of the bending rigidity on the BP are encompassed in change of macroscopic elasticity, which is in contrast to effects of pressure^{18,19}, but instead is similar to effects of polymerization^{20}. Furthermore, we show the positive correlation among the BP, elasticity, and the glass transition temperature. Finally, we will discuss the relaxation dynamics in the liquid state, in relation to our results of lowfrequency vibrational spectra.
Results
Glass transition temperature
When the polymeric system is cooled down from the liquid state under a constant pressure, the volume of the system monotonically decreases with decreasing the temperature. Figure 1a shows the specific volume \(v\) as a function of the temperature \(T\) for several different bending rigidities \({\varepsilon }_{{\rm{bend}}}\) and the chain length \(L=50\). For each value of \({\varepsilon }_{{\rm{bend}}}\), the slope of the \(v\)\(T\) curve clearly presents a discontinuous change at a certain temperature, which is defined as the glass transition temperature \({T}_{g}\). Figure 1b (triangles) presents the value of \({T}_{g}\) as a function of \({\varepsilon }_{{\rm{bend}}}\). As the rigidity increases from \({\varepsilon }_{{\rm{bend}}}=1\) to \(1{0}^{3}\), \({T}_{g}\) progressively increases from \({T}_{g}\simeq 0.45\) to 0.75. Below \(\varepsilon =1\) and above \(\varepsilon =1{0}^{3}\), the variation of \({T}_{g}\) is low or even negligible. In addition, Fig. 1b (circles) plots the density \(\rho (=1/v)\) of the system that is quenched down to \(T=0\). The density decreases from \(\rho \simeq 1.09\) to 0.97 as the rigidity increases from \({\varepsilon }_{{\rm{bend}}}=1\) to \(1{0}^{3}\). As the chain bending becomes rigid, the glass transition occurs at a higher temperature, and as a result, the density in the glass state becomes lower. The similar observation was obtained by Milkus et al.^{61}.
These behaviors of \({T}_{g}\) and \(\rho \) can be understood by studying the microscopic conformation of the polymeric chains. Figure 2a presents the probability distribution of the angle formed by three consecutive beads along the chain, \(P(\theta )\), when changing the rigidity \({\varepsilon }_{{\rm{bend}}}\). Two peaks are observed at approximately \(\theta \simeq 7{0}^{\circ }\) and \(\theta \simeq 12{0}^{\circ }\) for a low rigidity (\({\varepsilon }_{{\rm{bend}}}\le 1\)). A similar distribution \(P(\theta )\) was also reported in ref. ^{61}. As the rigidity increases, the peak position in \(P(\theta )\) shifts towards \({\theta }_{0}=109.{5}^{\circ }\). It is noted that the bending potential \({U}_{{\rm{bend}}}(\theta )\) in Eq. 5 tends to stabilize the angle \(\theta \) at \({\theta }_{0}=109.{5}^{\circ }\). In addition, Fig. 2b presents the radius of gyration \({R}_{g}\) as a function of \({\varepsilon }_{{\rm{bend}}}\). It can be observed that \({R}_{g}\) increases from \({R}_{g}\simeq 11.5\) to 16.5 with an increasing \({\varepsilon }_{{\rm{bend}}}\). Importantly, these variations of conformation are induced intensively when the rigidity increases from \({\varepsilon }_{{\rm{bend}}}=1\) to \(1{0}^{3}\), which exactly matches the region where variations of \({T}_{g}\) and \(\rho \) are observed in Fig. 1b. Therefore, it can be concluded that the conformation changes of the polymeric chains control the glass transition temperature and the density. In fact, as the rigidity of the chain bending increases, the angle \(\theta \) of the polymer chains tends to be stabilized at \({\theta }_{0}=109.{5}^{\circ }\) and the radius of inertia increases. As a result, the glass transition occurs at a higher temperature and the lower density (larger volume). At \({\varepsilon }_{{\rm{bend}}}\lesssim 1\), the effect of the bending interaction of Eq. 5 is weak compared to those of the LJ and finitely extensible nonlinear elastic (FENE) components of Eqs. 3 and 4 (see Methods). However, at \({\varepsilon }_{{\rm{bend}}}\gtrsim 1{0}^{3}\), the opposite phenomenon occurs.
It is noted that the glass transition occurs at a lower temperature for \(L=3\) than for \(L=50\), which is consistent with a previous report^{64}. Correspondingly, the values of \(\rho \) for \(L=3\) becomes larger than that of \(L=50\). However, common results were observed between \(L=3\) and 50 with respect to the dependences on the rigidity \({\varepsilon }_{{\rm{bend}}}\). Specifically, \({T}_{g}\) and \(\rho \), as well as the conformation of the polymeric chains progressively change when the rigidity increases from \({\varepsilon }_{{\rm{bend}}}=1\) to \(1{0}^{3}\), which also occurs for \(L=50\).
Elastic properties
The elastic properties of polymer glasses are studied by changing the strength of bending rigidity. An external strain is applied to the system at \(T=0\), which enables to measure the corresponding elastic moduli. Specifically, the volumechanging bulk deformation and the volumeconserving shear deformation are applied, which provide the bulk modulus \(K\) and the shear modulus \(G\), respectively^{63}. Figure 3 presents the values of \(K\) and \(G\) as functions of \({\varepsilon }_{{\rm{bend}}}\). Disordered systems exhibit large nonaffine elastic responses^{2}. The elastic moduli, \(M=K\) and \(G\), are decomposed into affine moduli \({M}_{{\rm{A}}}\) and nonaffine moduli \({M}_{{\rm{NA}}}\), i.e., \(M={M}_{{\rm{A}}}{M}_{{\rm{NA}}}\)^{65,66,67}. In Fig. 3, these affine and nonaffine components are also presented.
First, the bulk modulus \(K\) is analyzed for \(L=50\) and presented Fig. 3a. The affine component \({K}_{{\rm{A}}}\) decreases from \({K}_{{\rm{A}}}\simeq 155\) to 130 as \({\varepsilon }_{{\rm{bend}}}\) changes from 1 to \(1{0}^{3}\). The reduction of \({K}_{{\rm{A}}}\) is caused by the decrease of the density \(\rho \) with the increasing \({\varepsilon }_{{\rm{bend}}}\) (see Fig. 1b). In contrast, the nonaffine component \({K}_{{\rm{NA}}}\) shows a nonmonotonic dependence on the \({\varepsilon }_{{\rm{bend}}}\). In particular, \({K}_{{\rm{NA}}}\) slightly increases from \({\varepsilon }_{{\rm{bend}}}=1\) to 30, which is induced by the decrease of the density \(\rho \). As \({\varepsilon }_{{\rm{bend}}}\) is further increased above \({\varepsilon }_{{\rm{bend}}}=30\), \({K}_{{\rm{NA}}}\) decreases. This is because the nonaffine relaxation process is constrained due to the large rigidity of \({\varepsilon }_{{\rm{bend}}}\). As a result, the total modulus of \(K={K}_{{\rm{A}}}{K}_{{\rm{NA}}}\) also presents a nonmonotonic behavior, which is demonstrated in Fig. 3a. From \({\varepsilon }_{{\rm{bend}}}=1\) to \(1{0}^{2}\), \(K\) decreases from \(K\simeq 80\) to 60, which is caused by the reduction of \({K}_{{\rm{A}}}\). Moreover, \(K\) increases from \(K\simeq 60\) to 65 above \({\varepsilon }_{{\rm{bend}}}=100\), which is caused by the reduction of \({K}_{{\rm{NA}}}\). Therefore, the \({\varepsilon }_{{\rm{bend}}}\) dependence of the bulk modulus \(K\) is determined by the competition between the density reduction and the increase in the bending rigidity.
Further, the shear modulus \(G\) is analyzed for \(L=50\) and presented Fig. 3c. We note that a nonmonotonic behavior of the shear modulus as a function of bending stiffness is observed in the previous study^{60}. Figure 3c demonstrates that the bending rigidity strongly affects the shear modulus compared to the bulk modulus. Particularly, above \({\varepsilon }_{{\rm{bend}}}=1{0}^{2}\), both of the affine \({G}_{{\rm{A}}}\) and nonaffine \({G}_{{\rm{NA}}}\) components considerably increase. As the shear deformation is anisotropic and causes deformations of the angles \(\theta \) of polymeric chains, its response is expected to be highly affected by the bending rigidity. Interestingly, contrary to the important increases of \({G}_{{\rm{A}}}\) and \({G}_{{\rm{NA}}}\), the total shear modulus \(G={G}_{{\rm{A}}}{G}_{{\rm{NA}}}\) shows a low variation (by comparing \({G}_{{\rm{A}}}\simeq {G}_{{\rm{NA}}}\simeq 900\) with \(G\simeq 24\) at \({\varepsilon }_{{\rm{b}}{\rm{e}}{\rm{n}}{\rm{d}}}=1{0}^{4}\)). The bending rigidity increases the affine shear modulus but, at the same time, the nonaffine component also increases to cancel the increase in \({G}_{{\rm{A}}}\), and as a result, the total shear modulus presents a low increase. The elasticity of the shear deformation is therefore different from that of the bulk deformation, which is obvious when the elastic moduli are decomposed into affine and nonaffine components.
Figure 3 also shows \(K\) in (b) and \(G\) in (d) for \(L=3\). The values of \(K\) and \(G\) of \(L=3\) are smaller than those of \(L=50\), due to the bonding energy, \({\varepsilon }_{{\rm{FENE}}}\), connecting the monomers along the polymeric chains. The responses of \(K\) and \(G\) to the variation of \({\varepsilon }_{{\rm{bend}}}\) are also weaker for \(L=3\). However, \(K\) and \(G\), as well as affine \({K}_{{\rm{A}}}\) and \({G}_{{\rm{A}}}\) and nonaffine \({K}_{{\rm{NA}}}\) and \({G}_{{\rm{NA}}}\), exhibit overall common dependences on \({\varepsilon }_{{\rm{bend}}}\) between \(L=3\) and 50. Therefore, the decrease in \(\rho \) and increase in \({\varepsilon }_{{\rm{bend}}}\) engenders similar effects on the elasticity for \(L=3\) and 50.
Finally, it is remarked that the polymer glasses present larger nonaffine elastic components than the atomic (LJ) glasses^{63,68}. Even under an isotropic bulk deformation, the nonaffine \({K}_{{\rm{NA}}}\) (\(\simeq 80\) for \(L=50\) and \(\simeq 50\) for \(L=3\), at \({\varepsilon }_{{\rm{bend}}}\le 1\)) is approximately half of the magnitude of the affine \({K}_{{\rm{A}}}\) (\(\simeq 155\) for \(L=50\) and \(\simeq 120\) for \(L=3\), at \({\varepsilon }_{{\rm{bend}}}\le 1\)). This result is different from that of the LJ glasses, where a negligible value of \({K}_{{\rm{NA}}}\simeq 0.5\) (whereas \({K}_{{\rm{A}}}\simeq 60.2\)) was obtained^{63}. Larger nonaffine moduli reflect various elastic responses due to the multiple degrees of conformations in polymeric chains. Therefore, the nonaffine deformation process must be considered to characterize the elastic property of polymeric systems. Interestingly, ref. ^{69} has reported that nonaffine displacements also play an important role on melting of amorphous polymers.
Lowfrequency vibrational spectra
Reduced vDOS
Finally, the spectra of vibrational eigenmodes in polymer glasses are studied. The vibrational mode analysis is performed on the configuration of the polymeric system at \(T=0\), which corresponds to the inherent structure^{71,72}. The Hessian matrix is diagonalized to obtain the eigenfrequencies \({\omega }^{k}\) that corresponds to the square root of the eigenvalues \({\lambda }^{k}\), i.e., \({\omega }^{k}=\sqrt{{\lambda }^{k}}\) (\(k=1,2,...,3{N}_{{\rm{p}}}\)). The specific expression of the Hessian matrix is given in Supplementary Material.
The statistics of the eigenfrequency provide the vDOS, \(g(\omega )\). Figure 4 presents the reduced version of the vDOS, \(g(\omega )/{\omega }^{2}\), when changing the rigidity \({\varepsilon }_{{\rm{bend}}}\) and for \(L=50\) in (a) and \(L=3\) in (b). The reduced vDOS, \(g(\omega )/{\omega }^{2}\), of the Debye theory is the socalled Debye level \({A}_{{\rm{D}}}\)^{71,72}. \({A}_{{\rm{D}}}\) is calculated from the elastic moduli, \(K\) and \(G\), as follows: \({A}_{{\rm{D}}}=3/{\omega }_{{\rm{D}}}^{3}\), where \({\omega }_{{\rm{D}}}\) is the Debye frequency defined as \({\omega }_{{\rm{D}}}={\left[18{\pi }^{2}\rho /(2{{c}_{{\rm{T}}}}^{3}+{{c}_{{\rm{L}}}}^{3})\right]}^{1/3}\), and \({c}_{{\rm{L}}}=\sqrt{(K+4G/3)/\rho }\) and \({c}_{{\rm{T}}}=\sqrt{G/\rho }\) are the longitudinal and transverse sound speeds, respectively. Figure 5 presents the values of \({\omega }_{{\rm{D}}}\) and \({A}_{{\rm{D}}}\) as functions of \({\varepsilon }_{{\rm{bend}}}\). As the bulk modulus is approximately four times larger than the shear modulus, \({\omega }_{{\rm{D}}}\) and \({A}_{{\rm{D}}}\) are mostly determined with the shear modulus, i.e, \({\omega }_{{\rm{D}}}\approx {(9{\pi }^{2}\rho )}^{1/3}{c}_{{\rm{T}}}\) and \({A}_{{\rm{D}}}\approx 1/(3{\pi }^{2}\rho {c}_{{\rm{T}}}^{3})\).
As shown in Fig. 4, the polymer glasses present clear excess peaks over the Debye level, i.e., the BP. The BP frequency, \({\omega }_{{\rm{BP}}}\), is defined as the frequency at which \(g(\omega )/{\omega }^{2}\) is maximal. As \({\varepsilon }_{{\rm{bend}}}\) increases, \({\omega }_{{\rm{BP}}}\) shifts to a higher frequency. In addition, the height of the reduced vDOS, \(g({\omega }_{{\rm{BP}}})/{\omega }_{{\rm{BP}}}^{2}\), becomes lower. These behaviors of BP are consistent with the previous observation^{61}. These shifts are observed in the region from \({\varepsilon }_{{\rm{bend}}}=10\) to \(1{0}^{3}\) for \(L=50\) and 3. Importantly, this region corresponds to the shear modulus \(G\) variations, as shown in Fig. 3c,d. As the bulk modulus is much larger than the shear modulus, the bulk modulus should only have minor effects on the lowfrequency spectra. Therefore, the BP of the proposed system should only be controlled by the shear elasticity.
To confirm this hypothesis, the scaled vDOS \(g(\omega )/({\omega }^{2}{A}_{{\rm{D}}})\) is plotted as a function of the scaled frequency \(\omega /{\omega }_{{\rm{D}}}\) and presented in Fig. 6. As discussed above, \({A}_{{\rm{D}}}\) and \({\omega }_{{\rm{D}}}\) are determined mostly by the shear modulus \(G\). Although deviations are observed, the scaled vDOSs collapse for different values of \({\varepsilon }_{{\rm{bend}}}\). This result indicates that the effects engendered by the bending rigidity on the lowfrequency spectra are comprised of the the shear modulus changes. A same collapse was observed in effects of pressure on the BP in the covalentbonding network glass (Na\({}_{2}\)FeSi\({}_{3}\)O\({}_{8}\))^{6}. In addition, a previous experiment^{20} demonstrated that the effects of the polymerization are also comprised by the macroscopic elasticity changes. The collapsed results for (a) \(L=50\) and (b) \(L=3\) are consistent with the experimental observation.
The collapses observed in Fig. 6 indicates that \({\omega }_{{\rm{BP}}}/{\omega }_{{\rm{D}}}\) does not depend on \({\varepsilon }_{{\rm{bend}}}\). As stated previously, when \({\varepsilon }_{{\rm{bend}}}\) varies, \({\omega }_{{\rm{D}}}\propto {\rho }^{1/3}{c}_{{\rm{T}}}\propto {\rho }^{1/6}\sqrt{G}\). As \(\rho \) varies in a range of 15%, as shown in Fig. 1, the effect of \(\rho \) on \({\omega }_{{\rm{D}}}\) is weak. Thus, \({\omega }_{{\rm{D}}}\) is approximately proportional to \(\sqrt{G}\), which leads to \({\omega }_{{\rm{BP}}}\propto \sqrt{G}\) in the variation of \({\varepsilon }_{{\rm{bend}}}\). The \({\varepsilon }_{{\rm{bend}}}\) dependence of the BP frequency is determined by the shear modulus, which is a macroscopic quantity describing the entire system in an averaged manner. According to the heterogeneous elasticity theory^{24,25,26}, the spatial fluctuations of the local shear modulus \(\delta G\) control nature of the BP. The value of \(\delta G\) is quantified by the standard deviation of probability distribution function of the local shear modulus^{63}. The collapse of \(g(\omega )/({\omega }^{2}{A}_{{\rm{D}}})\) as a function of \(\omega /{\omega }_{{\rm{D}}}\) indicates that the shear modulus fluctuations relative to the macroscopic value, \(\delta G/G\), are constant for all the cases of different bending rigidities. Therefore, the results of this study can be explained as follows. The increase in bending rigidity does not affect the shear modulus fluctuations (relative to the macroscopic moduli) but only affects the macroscopic shear modulus, which leads to the collapse of the scaled vDOS. Furthermore, it is also noted that the recent theoretical study explains the origin of BP in both crystals and glasses in terms of the competition between elastic phonon propagation and diffusive damping^{33}. The model based on the phonon Green's function leads to the result \({\omega }_{{\rm{BP}}}\propto \sqrt{G}\). This necessitates further investigations regarding the effects of \({\varepsilon }_{{\rm{bend}}}\) on phonon transport and the phonon's Green function.
Participation ratio
To further study the vibrational eigenstates, the participation ratio \({P}^{k}\) that measures the extent of localization of the eigenmodes \(k\) is calculated as follows^{34,35}:
where \({{\boldsymbol{e}}}_{i}^{k}\)\((i=1,2,\cdots ,{N}_{{\rm{p}}})\) are the eigenvectors associated with the eigenfrequencies \({\omega }^{k}\) (\(i\) is the index of the monomer particle and \({N}_{{\rm{p}}}\) is the number of monomer particles). The \({{\boldsymbol{e}}}_{i}^{k}\) represents the displacements of each monomer bead \(i\) in the eigenmode \(k\). It is noted that \({{\boldsymbol{e}}}_{i}^{k}\) is obtained from the diagonalization of the Hessian matrix and is orthonormalized as \({\sum }_{i=1}^{{N}_{{\rm{p}}}}{{\boldsymbol{e}}}_{i}^{k}\cdot {{\boldsymbol{e}}}_{i}^{l}={\delta }_{kl}\) (\({\delta }_{kl}\) is the Kronecker delta). The following extreme cases can occur: \({P}^{k}=2/3\) for an ideal sinusoidal plane wave, \({P}^{k}=1\) for an ideal mode in which all constituent particles vibrate equally, and \({P}^{k}=1/{N}_{{\rm{p}}}\ll 1\) for a perfect localization, which indicates that each vibrational state is associated only with a single atom and that \({e}_{i}^{k}\cdot {e}_{i}^{k}=1\) for a single \(i\), otherwise \({e}_{i}^{k}\cdot {e}_{i}^{k}=0\).
Figure 7 presents the value of \({P}^{k}\) as a function of the scaled frequency \(\omega /{\omega }_{{\rm{D}}}\), for different \({\varepsilon }_{{\rm{bend}}}\). It is noted that the presented data are the binned average values. Below the BP frequency \({\omega }_{{\rm{BP}}}\), \({P}^{k}\) progressively decreases when \(\omega \) decreases due to the spatially localized vibrations. The lowfrequency localization below \({\omega }_{{\rm{BP}}}\) has also been observed in multiple glasses^{34,35,48,49}. Importantly, \({P}^{k}\) below \({\omega }_{{\rm{BP}}}\) collapses between different values of \({\varepsilon }_{{\rm{bend}}}\). This result indicates that the variations of not only the vDOS and the vibrational states due to \({\varepsilon }_{{\rm{bend}}}\) can be characterized by the macroscopic shear modulus changes. However, \({P}^{k}\) does not collapse above \({\omega }_{{\rm{BP}}}\), as also shown in Fig. 7. This result is attributed to the fact that the highfrequency modes above \({\omega }_{{\rm{BP}}}\) reflect microscopic vibrations that cannot be captured by the macroscopic elasticity.
Comparison with LJ glasses
The lowfrequency spectra are comparable to that of atomic LJ glasses reported in ref. ^{70}. As observed in Fig. 4, the height of \(g({\omega }_{{\rm{BP}}})/{\omega }_{{\rm{BP}}}^{2}\) of LJ glasses is higher than that of polymer glasses, and \({\omega }_{{\rm{BP}}}\) is lower than that of polymer glasses. These observations are different from the study reported in ref. ^{62}, which demonstrated that the lowfrequency spectra of polymer glasses correspond to those atomic LJ glasses. In ref. ^{62}, the bonded monomers interact via a harmonic potential with a large bonding energy scale of \(k=2500\). This value is two orders of magnitude larger than \({\varepsilon }_{{\rm{FENE}}}=30\), investigated in this study. With respect to the large bonding energy, the rigidity of the polymeric chains has a smaller effect on the lowfrequency spectra. Therefore, the lowfrequency spectra are mainly determined by the nonbonding LJ interactions, whereas the elasticity is mainly determined mainly by the bonding rigidity. As a results, the BP decouples with the macroscopic elasticity, as demonstrated in the previous study^{62}.
In contrast to the the results presented in ref. ^{62}, the rigidity of the polymeric chains is necessary to determine the elasticity and the lowfrequency spectra with respect to the bonding energy scale of \({\varepsilon }_{{\rm{FENE}}}=30\). In fact, the \({\varepsilon }_{{\rm{bend}}}\) reduces the height of \(g({\omega }_{{\rm{BP}}})/{\omega }_{{\rm{BP}}}^{2}\), as shown in Fig 4. In this case, the BP couples with the macroscopic elasticity. However, the plot of the scaled \(g(\omega )/({\omega }^{2}{A}_{{\rm{D}}})\) as a function of \(\omega /{\omega }_{{\rm{D}}}\) does not collapse between the polymer glasses and LJ glass, as shown in Fig. 6. The height of \(g(\omega )/({\omega }^{2}{A}_{{\rm{D}}})\) is consistent between the polymer glasses and LJ glass, but \(\omega /{\omega }_{{\rm{D}}}\) of the LJ glass is lower than that of the polymer glasses. This result indicates that vibrational states differences between polymer glasses and LJ glasses cannot be described only by changes in macroscopic elasticity, changes in the local elastic properties should be considered as well^{6,18,19,38}.
Here we make a note on the finite system size effects. We consider that the present system size of \({N}_{p}\simeq 5000\) is not enough large to sample the low frequency modes below the BP. The previous work on the LJ glass^{70} employed the very large system size up to \(N=1000000\) to study the low frequency regime without any system size effect. In contrast, our results of polymer glass for the region below the BP are affected by finite system size effects. However, the system size of \({N}_{p}\simeq 5000\) is enough large to study the vibrational modes in the BP. Indeed, we confirm that our results in the BP regime are not contaminated by the size effects. Thus, as long as we discuss on the BP, we do not need to care for the system size effects.
In addition, the length scale of collective vibrational modes in the BP region is discussed. For atomic LJ glasses, the length scale was evaluated as \({\xi }_{{\rm{BP}}}=2\pi {c}_{{\rm{T}}}/{\omega }_{{\rm{BP}}}\), which corresponds to the size of approximately 23 particle^{68}. This length scale diverges near the isostatic point or the marginally stable point, theoretically^{27,28,29,30} as well as numerically^{41,46,47,73,74}. The present study evaluates the length scale of collective vibrational modes in polymeric glasses as \({\xi }_{{\rm{BP}}}=2\pi {c}_{{\rm{T}}}/{\omega }_{{\rm{BP}}}\approx 12\), which corresponds to half of that for LJ glasses. The vibrational modes in the BP region are more localized nature due to the polymerization. Moreover, the value of \({\xi }_{{\rm{BP}}}\) is independent of the bending rigidity \({\varepsilon }_{{\rm{bend}}}\) because of \({\omega }_{{\rm{BP}}}\propto {\omega }_{{\rm{D}}}\propto {c}_{{\rm{T}}}\). In other words, the bending rigidity does not affect the length scale of the collective vibrational motions in the BP region.
Discussion
The glass transition temperature, elastic properties, and the lowfrequency vibrational spectra were studied in polymeric glasses. In particular, the bending energy scale was highly varied for long chains (\(L=50\)) and short chains (\(L=3\)). As the system becomes rigid by increasing the bending rigidity, the glass transition occurs at a higher temperature, leading to a lower density in the glass phase. The lowering density directly affects the isotropic bulk deformation, but does not affect the shear elasticity. The shear elasticity is mainly controlled by the bending rigidity. The nonaffinity of polymeric glasses is much larger than that of atomic LJ glasses. This is due to the more complex conformational relaxations of the polymeric chains during nonaffine deformation. Even under an isotropic elastic deformation, the nonaffine relaxation process should be considered to describe the elastic response.
In addition, it is demonstrated that the BP frequency ω_{BP} and its intensity are simply scaled by the Debye frequency ω_{D} and the Debye level A_{D} which are mainly determined by the macroscopic shear modulus G. This result indicates that the BP is controlled by macroscopic shear modulus and that the bending rigidity has a small impact on heterogeneities of local elasticity properties. The effects of the bending rigidity on the BP is similar to that of the polymerization, which has also been explained by macroscopic elasticity changes^{20}.
The presented results provide a simple relationship between the BP and the elasticity as well as the glass transition temperature. As the system becomes more rigid by increasing the bending rigidity, the glass transition temperature T_{g} and the shear modulus G are increased. On the contrary, the bulk modulus \(K\) decreases due to the decrease in the density \(\rho \) caused by the increase in the glass transition temperature \({T}_{g}\). However, the BP is mainly determined by the shear modulus \(G\): \({\omega }_{{\rm{BP}}}\propto {\omega }_{{\rm{D}}}\propto \sqrt{G}\). Therefore, the glass transition temperature, the shear elasticity, and the BP frequency are positively correlated. A similar relationship between \({T}_{g}\) and \({\omega }_{{\rm{BP}}}\) was observed experimentally in ionic liquids systems^{75} and also numerically in LJ glasses^{76}. It is noted that the studies of refs. ^{75,76} provided the relationship of \({T}_{g}\propto {\omega }_{{\rm{BP}}}^{2}\), but a clear powerlaw like relationship between \({T}_{g}\) and \({\omega }_{{\rm{BP}}}\) was not observed in polymeric glasses.
Finally, it is worthwhile to discuss the relationship between structural relaxation above the glass transition temperature and the elastic properties. In fact, there have been proposed the shoving model, which characterizes the activation energy of the structural relaxation time \({\tau }_{\alpha }\) in terms of the shear modulus \(G\)^{77,78}. In the literature, a recent study^{79} has demonstrated the scaling relationship between the structural relaxation time \({\tau }_{\alpha }\) and the DebyeWaller factor \(\langle {u}^{2}\rangle \) as \({\tau }_{\alpha }\propto \exp (a{\langle {u}^{2}\rangle }^{1}+b{\langle {u}^{2}\rangle }^{2})\) (where \(a,b\) are constants) for multiple glassforming liquids including polymeric glasses. Here, the DebyeWaller factor in the harmonic approximation^{80} is estimated as \(\langle {u}^{2}\rangle =3T{\int }_{0}^{\infty }g(\omega )/{\omega }^{2}d\omega \propto T{\omega }_{{\rm{BP}}}^{2}\propto T{G}^{1}\). It is naturally expected that the relaxation dynamics become drastically slow by increasing the bending rigidity because of the following relationship:
where \(\alpha ,\beta ,\alpha ^{\prime} ,{\beta }^{^{\prime} }\) are constants. This simple relationship demonstrates that the BP below \({T}_{g}\) and the structural relaxation above \({T}_{g}\) are well correlated in the polymeric glasses with varying the bending rigidity. Further work is necessary to evaluate its validity by calculating \({\tau }_{\alpha }\), despite the equation analogous to Eq. (2) has empirically been proposed from MD simulations of polymeric glasses^{81}.
Methods
Coarsegrained MD simulations are performed by using the Kremer–Grest model^{82}, which treats polymer chains as linear series of monomer beads (particles) of mass \(m\). Each polymer chain is composed of \(L\) monomer beads, and two cases are considered in this study: long chain length with \(L=50\) and short chain length with \(L=3\). In a threedimensional cubic simulation box under periodic boundary conditions, \({N}_{{\rm{p}}}=5000\) and 4998 is defined as the total number of monomers for \(L=50\) and \(L=3\) respectively, which means that the number of polymeric chains is \({N}_{{\rm{p}}}/L=100\) for \(L=50\) and 1666 for \(L=3\).
The polymer chain is modeled by three types of interparticle potentials as follows. Firstly, all the monomer particles interact via the LJ potential:
where \(r\) is the distance between two monomers, \(\sigma \) is the diameter of monomer, and \({\varepsilon }_{{\rm{LJ}}}\) is the energy scale of the LJ potential. The LJ potential is truncated at the cutoff distance of \({r}_{c}=2.5\sigma \), where the potential and the force (first derivative of the potential) are shifted to zero continuously^{70}. Throughout this study, the mass, length, and energy scales are measured in units of \(m\), \(\sigma \), \({\varepsilon }_{{\rm{LJ}}}\), respectively. The temperature is measured by \({\varepsilon }_{{\rm{LJ}}}/{k}_{{\rm{B}}}\) (\({k}_{{\rm{B}}}\) is the Boltzmann constant). Secondly, sequential monomerbeads along the polymeric chain are connected by the FENE potential:
where \({\varepsilon }_{{\rm{FENE}}}\) is the energy scale of the FENE potential, and \({R}_{0}\) is the maximum length of the FENE bond. Their values are defined as \({\varepsilon }_{{\rm{FENE}}}=30\) and \({R}_{0}=1.5\), according to ref. ^{61}. Finally, three consecutive monomer beads along the chain interact via the bending potential defined as follows:
where \(\theta \) is the angle formed by three consecutive beads, and \({\varepsilon }_{{\rm{bend}}}\) is the associated energy scale. This potential intends to stabilize the angle \(\theta \) at \({\theta }_{0}\) that we set as \({\theta }_{0}=109.{5}^{\circ }\). Here, the value of \({\varepsilon }_{{\rm{bend}}}\) in a wide range from \({\varepsilon }_{{\rm{bend}}}=1{0}^{3}\) to \(1{0}^{4}\), and the effects of the bending rigidity on the vibrational and mechanical properties of the polymeric system are studied.
MD simulations are performed by using the Largescale Atomic/Molecular Massively Parallel Simulator (LAMMPS)^{83}. The polymeric system is first equilibrated in the melted, liquid state at a temperature \(T=1.0\). Further, the system is cooled down under a fixed pressure condition of \(p=0\) and with a cooling rate of \(dT/dt=1{0}^{4}\). During the cooling process, the glass transition occurs at a particular temperature, i.e., the glass transition temperature. After the glass transition, the system is quenched down towards the zero temperature, i.e., \(T=0\) state.
Data availability
The data supporting the findings of this study are available from the corresponding authors upon reasonable request.
References
 1.
Phillips, W.A. (ed.) Amorphous Solids: LowTemperature Properties, vol. 24 of Topics in Current Physics (Springer, Berlin, Heidelberg, 1981).
 2.
Alexander, S. Amorphous solids: their structure, lattice dynamics and elasticity. Phys. Rep 296, 65–236 (1998).
 3.
Zeller, R. C. & Pohl, R. O. Thermal Conductivity and Specific Heat of Noncrystalline Solids. Phys. Rev. B 4, 2029–2041 (1971).
 4.
Buchenau, U., Nucker, N. & Dianoux, A. J. Neutron Scattering Study of the LowFrequency Vibrations in Vitreous Silica. Phys. Rev. Lett. 53, 2316–2319 (1984).
 5.
Nakayama, T. Boson peak and terahertz frequency dynamics of vitreous silica. Rep. Prog. Phys. 65, 1195–1242 (2002).
 6.
Monaco, A. et al. Effect of Densification on the Density of Vibrational States of Glasses. Phys. Rev. Lett. 97, 135501 (2006).
 7.
Baldi, G., Giordano, V. M., Monaco, G. & Ruta, B. Sound Attenuation at Terahertz Frequencies and the Boson Peak of Vitreous Silica. Phys. Rev. Lett. 104, 195501 (2010).
 8.
Chumakov, A. I. et al. Equivalence of the Boson Peak in Glasses to the Transverse Acoustic van Hove Singularity in Crystals. Phys. Rev. Lett. 106, 225501 (2011).
 9.
Yamamuro, O. et al. Inelastic neutron scattering study of low energy excitations in glassy 1butene. J. Chem. Phys. 105, 732–737 (1996).
 10.
Ramos, M. A., Talón, C., JiménezRiobóo, R. J. & Vieira, S. Lowtemperature specific heat of structural and orientational glasses of simple alcohols. J. Phys.: Condens. Matter 15, S1007–S1018 (2003).
 11.
Monaco, G. & Giordano, V. M. Breakdown of the Debye approximation for the acoustic modes with nanometric wavelengths in glasses. Proc. Natl. Acad. Sci. U.S.A. 106, 3659–3663 (2009).
 12.
Shibata, T., Mori, T. & Kojima, S. Lowfrequency vibrational properties of crystalline and glassy indomethacin probed by terahertz timedomain spectroscopy and lowfrequency Raman scattering. Spectrochim. Acta A 150, 207–211 (2015).
 13.
Kabeya, M. et al. Boson peak dynamics of glassy glucose studied by integrated terahertzband spectroscopy. Phys. Rev. B 94, 224204 (2016).
 14.
van den Berg, R., Grondey, S., Kästner, J. & Löhneysen, H. V. Low temperature thermal properties of amorphous Mg_{0.7}Zn_{0.3}. Solid State Commun. 47, 137–140 (1983).
 15.
Li, Y., Yu, P. & Bai, H. Y. Study on the boson peak in bulk metallic glasses. J. Appl. Phys. 104, 013520 (2008).
 16.
Bruna, P. et al. Acoustic properties of metallic glasses in the mesoscopic regime by inelastic Xray scattering. J. Alloys Compd. 509, S95–S98 (2011).
 17.
Huang, B., Bai, H. Y. & Wang, W. H. Relationship between boson heat capacity peaks and evolution of heterogeneous structure in metallic glasses. J. Appl. Phys. 115, 153505 (2014).
 18.
Niss, K. et al. Influence of Pressure on the Boson Peak: Stronger than Elastic Medium Transformation. Phys. Rev. Lett. 99, 055502 (2007).
 19.
Hong, L. et al. Pressure and density dependence of the boson peak in polymers. Phys. Rev. B 78, 134201 (2008).
 20.
Caponi, S. et al. Effect of polymerization on the boson peak, from liquid to glass. J. NonCryst. Solids 357, 530–533 (2011).
 21.
PérezCastañeda, T., JiménezRiobóo, R. J. & Ramos, M. A. TwoLevel Systems and Boson Peak Remain Stable in 110MillionYearOld Amber Glass. Phys. Rev. Lett. 112, 165901 (2014).
 22.
Terao, W. et al. Boson peak dynamics of natural polymer starch investigated by terahertz timedomain spectroscopy and lowfrequency Raman scattering. Spectrochim. Acta A 192, 446–450 (2018).
 23.
Zorn, R. et al. Anomalies in the low frequency vibrational density of states for a polymer with intrinsic microporosity  the Boson peak of PIM1. Phys. Chem. Chem. Phys. 20, 1355–1363 (2018).
 24.
Schirmacher, W. Thermal conductivity of glassy materials and the “boson peak”. EPL 73, 892–898 (2006).
 25.
Schirmacher, W., Ruocco, G. & Scopigno, T. Acoustic Attenuation in Glasses and its Relation with the Boson Peak. Phys. Rev. Lett. 98, 025501 (2007).
 26.
Schirmacher, W., Scopigno, T. & Ruocco, G. Theory of vibrational anomalies in glasses. J. NonCryst. Solids 407, 133–140 (2015).
 27.
Wyart, M., Nagel, S. R. & Witten, T. A. Geometric origin of excess lowfrequency vibrational modes in weakly connected amorphous solids. EPL 72, 486–492 (2005).
 28.
Wyart, M., Silbert, L. E., Nagel, S. R. & Witten, T. A. Effects of compression on the vibrational modes of marginally jammed solids. Phys. Rev. E 72, 051306 (2005).
 29.
Wyart, M. Scaling of phononic transport with connectivity in amorphous solids. EPL 89, 64001 (2010).
 30.
DeGiuli, E., LaversanneFinot, A., Düring, G., Lerner, E. & Wyart, M. Effects of coordination and pressure on sound attenuation, boson peak and elasticity in amorphous solids. Soft Matter 10, 5628–5644 (2014).
 31.
Milkus, R. & Zaccone, A. Local inversionsymmetry breaking controls the boson peak in glasses and crystals. Phys. Rev. B 93, 094204 (2016).
 32.
Krausser, J., Milkus, R. & Zaccone, A. Nonaffine lattice dynamics of defective fcc crystals. Soft Matter 13, 6079–6089 (2017).
 33.
Baggioli, M. & Zaccone, A. Universal Origin of Boson Peak Vibrational Anomalies in Ordered Crystals and in Amorphous Materials. Phys. Rev. Lett. 122, 145501 (2019).
 34.
Schober, H. R. & Oligschleger, C. Lowfrequency vibrations in a model glass. Phys. Rev. B 53, 11469–11480 (1996).
 35.
Mazzacurati, V., Ruocco, G. & Sampoli, M. Lowfrequency atomic motion in a model glass. EPL 34, 681–686 (1996).
 36.
Shintani, H. & Tanaka, H. Universal link between the boson peak and transverse phonons in glass. Nat. Mater. 7, 870–877 (2008).
 37.
Monaco, G. & Mossa, S. Anomalous properties of the acoustic excitations in glasses on the mesoscopic length scale. Proc. Natl. Acad. Sci. U.S.A. 106, 16907–16912 (2009).
 38.
Mizuno, H., Mossa, S. & Barrat, J.L. Elastic heterogeneity, vibrational states, and thermal conductivity across an amorphisation transition. EPL 104, 56001 (2013).
 39.
Lerner, E., Düring, G. & Bouchbinder, E. Statistics and Properties of LowFrequency Vibrational Modes in Structural Glasses. Phys. Rev. Lett. 117, 035501 (2016).
 40.
Wang, L. et al. Lowfrequency vibrational modes of stable glasses. Nat. Commun. 10, 26 (2019).
 41.
Silbert, L. E., Liu, A. J. & Nagel, S. R. Vibrations and Diverging Length Scales Near the Unjamming Transition. Phys. Rev. Lett. 95, 098301 (2005).
 42.
Silbert, L. E., Liu, A. J. & Nagel, S. R. Normal modes in model jammed systems in three dimensions. Phys. Rev. E 79, 021308 (2009).
 43.
Vitelli, V., Xu, N., Wyart, M., Liu, A. J. & Nagel, S. R. Heat transport in model jammed solids. Phys. Rev. E 81, 021301 (2010).
 44.
Xu, N., Vitelli, V., Liu, A. J. & Nagel, S. R. Anharmonic and quasilocalized vibrations in jammed solids–Modes for mechanical failure. EPL 90, 56001 (2010).
 45.
Mizuno, H., Shiba, H. & Ikeda, A. Continuum limit of the vibrational properties of amorphous solids. Proc. Natl. Acad. Sci. U.S.A 114, E9767–E9774 (2017).
 46.
Shimada, M., Mizuno, H., Wyart, M. & Ikeda, A. Spatial structure of quasilocalized vibrations in nearly jammed amorphous solids. Phys. Rev. E 98, 060901(R) (2018).
 47.
Mizuno, H. & Ikeda, A. Phonon transport and vibrational excitations in amorphous solids. Phys. Rev. E 98, 062612 (2018).
 48.
Taraskin, S. & Elliott, S. Nature of vibrational excitations in vitreous silica. Phys. Rev. B 56, 8605–8622 (1997).
 49.
Taraskin, S. & Elliott, S. Anharmonicity and localization of atomic vibrations in vitreous silica. Phys. Rev. B 59, 8572–8585 (1999).
 50.
Horbach, J., Kob, W. & Binder, K. High frequency sound and the boson peak in amorphous silica. Eur. Phys. J. B 19, 531–543 (2001).
 51.
Léonforte, F., Tanguy, A., Wittmer, J. & Barrat, J. L. Inhomogeneous Elastic Response of Silica Glass. Phys. Rev. Lett. 97, 055501 (2006).
 52.
Beltukov, Y. M., Fusco, C., Parshin, D. A. & Tanguy, A. Boson peak and IoffeRegel criterion in amorphous siliconlike materials: The effect of bond directionality. Phys. Rev. E 93, 023006 (2016).
 53.
Beltukov, Y. M., Parshin, D. A., Giordano, V. M. & Tanguy, A. Propagative and diffusive regimes of acoustic damping in bulk amorphous material. Phys. Rev. E 98, 023005 (2018).
 54.
Derlet, P. M., Maaß, R. & Löffler, J. F. The Boson peak of model glass systems and its relation to atomic structure. Eur. Phys. J. B 85, 148 (2012).
 55.
Fan, Y., Iwashita, T. & Egami, T. Evolution of elastic heterogeneity during aging in metallic glasses. Phys. Rev. E 89, 062313 (2014).
 56.
Crespo, D., Bruna, P., Valles, A. & Pineda, E. Phonon dispersion relation of metallic glasses. Phys. Rev. B 94, 144205 (2016).
 57.
Brink, T., Koch, L. & Albe, K. Structural origins of the boson peak in metals: From highentropy alloys to metallic glasses. Phys. Rev. B 94, 224203 (2016).
 58.
Jain, T. S. & de Pablo, J. J. Influence of confinement on the vibrational density of states and the Boson peak in a polymer glass. J. Chem. Phys. 120, 9371–9375 (2004).
 59.
Schnell, B., Meyer, H., Fond, C., Wittmer, J. P. & Baschnagel, J. Simulated glassforming polymer melts: Glass transition temperature and elastic constants of the glassy state. Eur. Phys. J. E 34, 97 (2011).
 60.
Ness, C. et al. Nonmonotonic dependence of polymerglass mechanical response on chain bending stiffness. Phys. Rev. E 96, 030501(R) (2017).
 61.
Milkus, R. et al. Interpretation of the Vibrational Spectra of Glassy Polymers Using CoarseGrained Simulations. Macromolecules 51, 1559–1572 (2018).
 62.
Giuntoli, A. & Leporini, D. Boson Peak Decouples from Elasticity in Glasses with Low Connectivity. Phys. Rev. Lett. 121, 185502 (2018).
 63.
Mizuno, H., Mossa, S. & Barrat, J.L. Measuring spatial distribution of the local elastic modulus in glasses. Phys. Rev. E 87, 042306 (2013).
 64.
Durand, M., Meyer, H., Benzerara, O., Baschnagel, J. & Vitrac, O. Molecular dynamics simulations of the chain dynamics in monodisperse oligomer melts and of the oligomer tracer diffusion in an entangled polymer matrix. J. Chem. Phys. 132, 194902 (2010).
 65.
Tanguy, A., Wittmer, J., Leonforte, F. & Barrat, J. L. Continuum limit of amorphous elastic bodies: A finitesize study of lowfrequency harmonic vibrations. Phys. Rev. B 66, 174205 (2002).
 66.
Lemaître, A. & Maloney, C. Sum Rules for the QuasiStatic and ViscoElastic Response of Disordered Solids at Zero Temperature. J. Stat. Phys 123, 415–453 (2006).
 67.
Zaccone, A. & ScossaRomano, E. Approximate analytical description of the nonaffine response of amorphous solids. Phys. Rev. B 83, 184205 (2011).
 68.
Leonforte, F., Boissière, R., Tanguy, A., Wittmer, J. & Barrat, J. L. Continuum limit of amorphous elastic bodies. III. Threedimensional systems. Phys. Rev. B 72, 224206 (2005).
 69.
Zaccone, A. & Terentjev, E. M. DisorderAssisted Melting and the Glass Transition in Amorphous Solids. Phys. Rev. Lett. 110, 178002 (2013).
 70.
Shimada, M., Mizuno, H. & Ikeda, A. Anomalous vibrational properties in the continuum limit of glasses. Phys. Rev. E 97, 022609 (2018).
 71.
Kittel, C. Introduction to Solid State Physics (John Wiley and Sons, New York, 2004), edition 8th edn.
 72.
Ashcroft, N. W. & Mermin, N. D. Solid State Physics (Harcourt College Publishers, New York, 1976).
 73.
Lerner, E., DeGiuli, E., Düring, G. & Wyart, M. Breakdown of continuum elasticity in amorphous solids. Soft Matter 10, 5085–5092 (2014).
 74.
Karimi, K. & Maloney, C. E. Elasticity of frictionless particles near jamming. Phys. Rev. E 92, 022208 (2015).
 75.
Kofu, M. et al. Inelastic neutron scattering study on boson peaks of imidazoliumbased ionic liquids. J. Mol. Liq. 210, 164–168 (2015).
 76.
Wang, L. & Xu, N. Probing the Glass Transition from Structural and Vibrational Properties of ZeroTemperature Glasses. Phys. Rev. Lett. 112, 055701 (2014).
 77.
Dyre, J. C. Source of nonArrhenius average relaxation time in glassforming liquids. J. NonCryst. Solids 235237, 142–149 (1998).
 78.
Dyre, J. C. Colloquium: The glass transition and elastic models of glassforming liquids. Rev. Mod. Phys. 78, 953–972 (2006).
 79.
Larini, L., Ottochian, A., De Michele, C. & Leporini, D. Universal scaling between structural relaxation and vibrational dynamics in glassforming liquids and polymers. Nat. Phys 4, 42–45 (2008).
 80.
Shiba, H., Yamada, Y., Kawasaki, T. & Kim, K. Unveiling Dimensionality Dependence of Glassy Dynamics: 2D Infinite Fluctuation Eclipses Inherent Structural Relaxation. Phys. Rev. Lett. 117, 245701 (2016).
 81.
Puosi, F. & Leporini, D. Communication: Correlation of the instantaneous and the intermediatetime elasticity with the structural relaxation in glassforming systems. J. Chem. Phys. 136, 041104 (2012).
 82.
Kremer, K. & Grest, G. S. Dynamics of entangled linear polymer melts: A moleculardynamics simulation. J. Chem. Phys. 92, 5057–5086 (1990).
 83.
Plimpton, S. Fast parallel algorithms for shortrange molecular dynamics. J. Comput. Phys. 117, 1–19 (1995).
Acknowledgements
The authors thank Atsushi Ikeda for useful discussions and suggestions. This work was supported by JSPS KAKENHI Grant Numbers: JP19K14670 (H.M.), JP17K14318 (T.M.), JP18H04476 (T.M.), JP18H01188 (K.K.), JP15K13550 (N.M.), and JP19H04206 (N.M.). This work was also partially supported by the Asahi Glass Foundation and by the PostK Supercomputing Project and the Elements Strategy Initiative for Catalysts and Batteries from the Ministry of Education, Culture, Sports, Science, and Technology. The numerical calculations were performed at Research Center of Computational Science, Okazaki Research Facilities, National Institutes of Natural Sciences, Japan.
Author information
Affiliations
Contributions
H.M., K.K. and N.M. designed and supervised the project; T.N. performed numerical simulations; and all authors discussed the results and wrote the manuscript.
Corresponding authors
Ethics declarations
Competing interests
The authors declare no competing interests.
Additional information
Publisher’s note Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Supplementary information
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Tomoshige, N., Mizuno, H., Mori, T. et al. Boson peak, elasticity, and glass transition temperature in polymer glasses: Effects of the rigidity of chain bending. Sci Rep 9, 19514 (2019). https://doi.org/10.1038/s41598019555642
Received:
Accepted:
Published:
Further reading

Material properties particularly suited to be measured with helium scattering: selected examples from 2D materials, van der Waals heterostructures, glassy materials, catalytic substrates, topological insulators and superconducting radio frequency materials
Physical Chemistry Chemical Physics (2021)

Characteristic terahertz absorption spectra of paramylon and paramylonester compounds
Spectrochimica Acta Part A: Molecular and Biomolecular Spectroscopy (2021)

Formation and crystallization of lowdensity amorphous ice
Journal of Physics D: Applied Physics (2021)

Dynamics & Spectroscopy with Neutrons—Recent Developments & Emerging Opportunities
Polymers (2021)

In Situ Studies of Stress Environment in Amorphous Solids Using Negatively Charged Nitrogen Vacancy (NV–) Centers in Nanodiamond
ACS Applied Polymer Materials (2021)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.