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**Research article**
26 Apr 2019

**Research article** | 26 Apr 2019

Buckling of elastically restrained nonlocal carbon nanotubes

^{1}Department of Physics, University of Dschang, Dschang, Cameroon^{2}Discipline of Mechanical Engineering, University of KwaZulu-Natal, Durban, South Africa

^{1}Department of Physics, University of Dschang, Dschang, Cameroon^{2}Discipline of Mechanical Engineering, University of KwaZulu-Natal, Durban, South Africa

Abstract

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Buckling of elastically restrained carbon nanotubes is studied subject to a combination of uniformly distributed and concentrated compressive loads. Governing equations are based on the nonlocal model of carbon nanotubes. Weak formulation of the problem is formulated and the Rayleigh quotients are obtained for distributed and concentrated axial loads. Numerical solutions are obtained by Rayleigh–Ritz method using orthogonal Chebyshev polynomials. The method of solution is verified by checking against results available in the literature. The effect of the elastic restraints on the buckling load is studied by counter plots in term of small-scale parameter and the spring constants.

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Robinson, M. T. A. and Adali, S.: Buckling of elastically restrained nonlocal carbon nanotubes under concentrated and uniformly distributed axial loads, Mech. Sci., 10, 145-152, https://doi.org/10.5194/ms-10-145-2019, 2019.

1 Introduction

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Presently nanoscale components are being used extensively in a variety of nanotechnology applications (Morris and Iniewski, 2013; Tserpes and Silvestre, 2014). In particular, carbon nanotubes (CTN) are used in diverse fields due their superior properties (Endo et al., 2008; Zhang, 2012; Tserpes and Silvestre, 2014) which include high stiffness and low density. To exploit their properties in specific applications, their mechanical behaviour under loading needs to be investigated by mathematical modelling and/or molecular dynamic simulations. The modelling employed in the present study is nonlocal continuum mechanics. Continuum approach in the study of the mechanical behaviour of nano scale structures has been implemented extensively as can be judged from the review articles and the books on the subject (Wang et al., 2010; Eltaher et al., 2016; Kaushik and Majumder, 2015; Rafiei, 2015; Rafii-Tabar et al., 2016). In particular, buckling of carbon nanotubes has been studied extensively by continuum modelling and the recent work on this subject can be found in Reddy (2007), Reddy and Pang (2008), Zhang et al. (2010), Xu et al. (2012), Arash and Wang (2012) and Askari et al. (2017).

Previous studies on the buckling of nanotubes mostly involved rigid boundary conditions such as clamped, hinged and free boundaries. Recent studies on the buckling of nanotubes under a tip load and subject to classical boundary conditions include Ansari et al. (2011), Sahmani and Ansari (2011), Kumar (2016), Kumar and Deol (2016) and Taghizadeh and Ovesy (2016). In these studies the buckling loads for carbon nanotubes were obtained subject to classical boundary conditions. However, elastically restrained boundaries can be observed in a number of applications of nano-scale components. One such application area is nanomechanical sensors (Kiani, 2015) and for sensing nanosized objects (Kiani et al., 2013). Restraints such as rotational springs affect the buckling load that can be carried by a nanotube. Study of the buckling of CTNs subject to elastically restrained end conditions extends the previous results to the cases when the CTN boundaries cannot be modelled simply as hinged, clamped or free boundaries. Previous work on this subject involved the buckling of a nanotube with rotational springs on the boundaries and subject to a concentrated axial load (Wang et al., 2015; Yayli, 2015, 2016).

Present study is directed to determining the stability of carbon nanotubes under compressive axial loads when the nanotube is subject to elastically restrained boundary conditions. Such end conditions arise in situations when the nanotube cannot be attached to the boundaries in a rigid manner. Axial loads are taken as a concentrated tip load and a uniformly distributed axial load which corresponds to buckling under self-weight. Buckling of nanotubes under self-weight has been the subject of studies in Wang et al. (2004), Mustapha and Zhong (2012), Wang et al. (2016). Buckling of nanotubes subject to uniformly and triangularly distributed axial loads has been studied for uniform nanotubes in Robinson and Adali (2016), Robinson et al. (2018) and for non-uniform nanotubes in Robinson and Adali (2017, 2018).

In the present study, the numerical solution of the problem is based on a variational approach involving the weak formulation of the problem incorporating the differential equation and the elastic boundary conditions in a single expression. Rayleigh quotients for the tip load and the distributed axial loads are derived using the weak formulation framework. Rayleigh–Ritz method of solution is implemented via orthogonal Chebyshev polynomials. Solution method is validated by comparing the accuracy of the results with results available in the literature. There have been a number of studies applying Rayleigh–Ritz method to the buckling and vibration of nanotubes (Behera and Chakraverty, 2014; Ghannadpour et al., 2013; Ghannadpour and Mohammadi, 2010, 2011) and the method has been covered extensively in the book by Reddy (2002). Variational formulations for the buckling of nonlocal CTNs have been given in a number of cases (Adali, 2008, 2012).

2 Nonlocal problem formulation

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We consider an elastically restrained single-walled carbon nanotube subject
to concentrated and uniformly distributed axial loads. The nanotube has
length *L* and the axial load is expressed as

$$\begin{array}{}\text{(1)}& N\left(x\right)=P+Q(L-x),\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\mathrm{0}\le x\le L\end{array}$$

where *P* is the concentrated axial load applied at the end point *x*=*L* and
*Q* is the magnitude of the uniformly distributed axial load as shown in
Fig. 1.

The support at *x*=0 is elastically restrained by a rotational spring with a
torsional constant *K*_{r0}. The support at *x*=*L* is elastically
restrained by a rotational spring with a torsional constant *K*_{r1} and a translational spring of constant *K*_{t}. The clamped end
boundary conditions correspond to *K*_{r0}→∞ at *x*=0 and
*K*_{r1}→∞ and *K*_{t}→∞ at *x*=*L*.
Simply supported boundary conditions correspond to *K*_{r0}=0 at
*x*=0, and *K*_{r1}=0 and *K*_{t}→∞ at *x*=*L*.
Free end boundary condition at *x*=*L* is given by *K*_{r1}=0 and
*K*_{t}=0. The equation governing the buckling of the elastically
restrained column can be expressed in terms of moment *M*(*x*) and deflection
*w*(*x*) as

$$\begin{array}{ll}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}M}{\mathrm{d}{x}^{\mathrm{2}}}}& {\displaystyle}-{\displaystyle \frac{\mathrm{d}}{\mathrm{d}x}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)+\sum _{i=\mathrm{0}}^{i=\mathrm{1}}{K}_{{\mathrm{r}}_{i}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\mathit{\delta}(x-{x}_{i})\\ \text{(2)}& {\displaystyle}& {\displaystyle}-{K}_{\mathrm{t}}w\left(x\right)\mathit{\delta}(x-L)=\mathrm{0}\end{array}$$

where *x*_{0}=0, *x*_{1}=*L* and *δ*(*x*−*x*_{i}) is Dirac delta function.
The constitutive relation based on the nonlocal theory of elasticity can be
expressed as

$$\begin{array}{}\text{(3)}& M-{\mathit{\eta}}^{\mathrm{2}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}M}{\mathrm{d}{x}^{\mathrm{2}}}}=-EI{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\end{array}$$

where *η*=*e*_{0}*a* is the small scale parameter, *E* is the Young's
modulus and *I* is the moment of inertia. In the expression *η*=*e*_{0}*a*,
*e*_{0} stands for a constant which is specific to each material. It can be
determined either experimentally by using vibration or buckling load
measurements or by the use of atomic dispersion relations. The constant *a*
represents an internal characteristics length such as granular distance or
lattice parameter. The nonlocal parameter *η* is also called a
small-scale parameter and can be determined by conducting experiments and a
comparison of dispersion curves obtained from nonlocal continuum mechanics
and molecular dynamics simulations. Generally *η*≤2 nm for SWCNT and
its value depends on many parameters such as boundary conditions, chirality,
mode shape, number of walls and type of motion. Further information on the
computation and the meaning of *η* can be found in Challamel et
al. (2014) and Wang et al. (2017).

The expression for *M*(*x*) is obtained from Eqs. (2) and (3) as

$$\begin{array}{ll}{\displaystyle}M\left(x\right)& {\displaystyle}=-EI{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}+{\mathit{\eta}}^{\mathrm{2}}[{\displaystyle \frac{\mathrm{d}}{\mathrm{d}x}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)\\ \text{(4)}& {\displaystyle}& {\displaystyle}-\sum _{i=\mathrm{0}}^{i=\mathrm{1}}{K}_{{\mathrm{r}}_{i}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\mathit{\delta}(x-{x}_{i})+{K}_{\mathrm{t}}w\left(x\right)\mathit{\delta}(x-L)]\end{array}$$

From Eqs. (2) and (4), the differential equation governing the buckling of an
elastically restrained nanotube subject to the buckling load *N*(*x*) given by
Eq. (1) is obtained as

$$\begin{array}{ll}{\displaystyle}D\left(w\right)& {\displaystyle}=EI{\displaystyle \frac{{\mathrm{d}}^{\mathrm{4}}w}{\mathrm{d}{x}^{\mathrm{4}}}}+{\displaystyle \frac{\mathrm{d}}{\mathrm{d}x}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)-K\left(w\left({x}_{i}\right)\right)\\ \text{(5)}& {\displaystyle}& {\displaystyle}-{\mathit{\eta}}^{\mathrm{2}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}}{\mathrm{d}{x}^{\mathrm{2}}}}\left[{\displaystyle \frac{\mathrm{d}}{\mathrm{d}x}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)-K\left(w\left({x}_{i}\right)\right)\right]=\mathrm{0}\end{array}$$

where

$$\begin{array}{}\text{(6)}& K\left(w\left({x}_{i}\right)\right)=\sum _{i=\mathrm{0}}^{i=\mathrm{1}}{K}_{{\mathrm{r}}_{i}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\mathit{\delta}(x-{x}_{i})-{K}_{\mathrm{t}}w\left(x\right)\mathit{\delta}(x-L)\end{array}$$

3 Weak formulation

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Next the weak formulation for Eq. (5) is derived by noting that

$$\begin{array}{}\text{(7)}& \underset{\mathrm{0}}{\overset{L}{\int}}D\left(w\right)w\mathrm{d}x=\mathrm{0}\end{array}$$

The weak formulation of Eq. (5) is a weighted-integral form that incorporates both the governing differential equation and the associated natural boundary conditions. The use of equation Eq. (7) facilitates the derivation of the variational form of the problem as well as the derivation of the boundary conditions as shown below. This approach has been employed in Robinson and Adali (2016, 2017, 2018) for a number of nonlocal buckling problems. Using integration by parts, the following equation can be obtained from Eqs. (5) and (7):

$$\begin{array}{ll}{\displaystyle}& {\displaystyle}\underset{\mathrm{0}}{\overset{L}{\int}}\mathit{\{}EI{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}-N{\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)}^{\mathrm{2}}-{\mathit{\eta}}^{\mathrm{2}}[{\displaystyle \frac{\mathrm{d}N}{\mathrm{d}x}}{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\\ \text{(8)}& {\displaystyle}& {\displaystyle}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}+N{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\left]\mathit{\right\}}\mathrm{d}x+{B}_{\mathrm{1}}\left(w\left({x}_{i}\right)\right)+{B}_{\mathrm{2}}\left(w\left({x}_{i}\right)\right)=\mathrm{0}\end{array}$$

where the boundary terms are given by

$$\begin{array}{ll}{\displaystyle}& {\displaystyle}{B}_{\mathrm{1}}\left(w\left({x}_{i}\right)\right)={\left.\sum _{i=\mathrm{0}}^{i=\mathrm{1}}{K}_{{\mathrm{r}}_{i}}{\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)}^{\mathrm{2}}\right|}_{x={x}_{i}}+{\left.{K}_{\mathrm{t}}{w}^{\mathrm{2}}\right|}_{x=L}\\ \text{(9)}& {\displaystyle}& {\displaystyle}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}-{\mathit{\eta}}^{\mathrm{2}}\left(-{\left.\sum _{i=\mathrm{0}}^{i=\mathrm{1}}{K}_{{\mathrm{r}}_{i}}{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\right|}_{x={x}_{i}}+{\left.{K}_{t}w{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right|}_{x=L}\right)\text{(10)}& {\displaystyle}& {\displaystyle}{B}_{\mathrm{2}}\left(w\left({x}_{i}\right)\right)={\left.\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}m+wV\right)\right|}_{x=\mathrm{0}}^{x=L}\end{array}$$

with *m*(*x*_{i}) and *V*(*x*_{i}) denoting the expressions

$$\begin{array}{ll}{\displaystyle}& {\displaystyle}m\left({x}_{i}\right)=-EI{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}+{\mathit{\eta}}^{\mathrm{2}}{\displaystyle \frac{\mathrm{d}}{\mathrm{d}x}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right),\\ \text{(11)}& {\displaystyle}& {\displaystyle}V\left({x}_{i}\right)=EI{\displaystyle \frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}}-{\mathit{\eta}}^{\mathrm{2}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}}{\mathrm{d}{x}^{\mathrm{2}}}}\left(N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)+N{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\end{array}$$

4 Rayleigh quotients

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First the Rayleigh quotient for the concentrated load is derived for the case
*P*>0 and *Q*=0 (no distributed load). For this case the following relation
can be obtained from Eqs. (8), (10) and (11)

$$\begin{array}{ll}{\displaystyle}& {\displaystyle}\underset{\mathrm{0}}{\overset{L}{\int}}EI{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}x-P\underset{\mathrm{0}}{\overset{L}{\int}}{\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)}^{\mathrm{2}}\mathrm{d}x-{\mathit{\eta}}^{\mathrm{2}}P\underset{\mathrm{0}}{\overset{L}{\int}}{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}x\\ {\displaystyle}& {\displaystyle}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}+{B}_{\mathrm{1}}\left(w\left({x}_{i}\right)\right)-EI{\left.\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)\right|}_{x=\mathrm{0}}^{x=L}\\ {\displaystyle}& {\displaystyle}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}+{\mathit{\eta}}^{\mathrm{2}}P{\left.\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)\right|}_{x=\mathrm{0}}^{x=L}+EI{\left.\left(w{\displaystyle \frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}}\right)\right|}_{x=\mathrm{0}}^{x=L}\\ \text{(12)}& {\displaystyle}& {\displaystyle}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}-{\mathit{\eta}}^{\mathrm{2}}P{\left.\left(w{\displaystyle \frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}}\right)\right|}_{x=\mathrm{0}}^{x=L}+P{\left.\left(w{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)\right|}_{x=\mathrm{0}}^{x=L}=\mathrm{0}\end{array}$$

The Rayleigh quotient for *P* (*Q*=0) follows from Eq. (12) as

$$\begin{array}{}\text{(13)}& P={\displaystyle \frac{{\displaystyle \begin{array}{c}{\int}_{\mathrm{0}}^{L}EI{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}x+{B}_{\mathrm{1}}\left(w\left({x}_{i}\right)\right)\\ -EI{\left.\left(\frac{\mathrm{d}w}{\mathrm{d}x}\frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}\right)\right|}_{x=\mathrm{0}}^{x=L}+EI{\left.\left(w\frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}\right)\right|}_{x=\mathrm{0}}^{x=L}\end{array}}}{{\scriptscriptstyle \begin{array}{c}{\int}_{\mathrm{0}}^{L}{\left(\frac{\mathrm{d}w}{\mathrm{d}x}\right)}^{\mathrm{2}}\mathrm{d}x+{\mathit{\eta}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{L}{\left(\frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}\right)}^{\mathrm{2}}\mathrm{d}x-{\mathit{\eta}}^{\mathrm{2}}{\left.\left(\frac{\mathrm{d}w}{\mathrm{d}x}\frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}\right)\right|}_{x=\mathrm{0}}^{x=L}\\ +{\mathit{\eta}}^{\mathrm{2}}{\left.\left(w{\scriptscriptstyle \frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}}\right)\right|}_{x=\mathrm{0}}^{x=L}-{\left.\left(w{\scriptscriptstyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)\right|}_{x=\mathrm{0}}^{x=L}\end{array}}}}\end{array}$$

Rayleigh quotient for the distributed load *Q* with no concentrated load
applied (*P*=0) is obtained by a similar computation and the Rayleigh
quotient for the case is given by

$$\begin{array}{}\text{(14)}& Q={\displaystyle \frac{{\displaystyle \begin{array}{c}{\int}_{\mathrm{0}}^{L}EI{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}x+{B}_{\mathrm{1}}\left(w\left({x}_{i}\right)\right)\\ -EI{\left.\left(\frac{\mathrm{d}w}{\mathrm{d}x}\frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}\right)\right|}_{x=\mathrm{0}}^{x=L}+EI{\left.\left(w\frac{{\mathrm{d}}^{\mathrm{3}}w}{\mathrm{d}{x}^{\mathrm{3}}}\right)\right|}_{x=\mathrm{0}}^{x=L}\end{array}}}{{\scriptscriptstyle \begin{array}{c}{\int}_{\mathrm{0}}^{L}(L-x){\left(\frac{\mathrm{d}w}{\mathrm{d}x}\right)}^{\mathrm{2}}\mathrm{d}x-{\mathit{\eta}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{L}\frac{\mathrm{d}w}{\mathrm{d}x}\frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}\mathrm{d}x\\ +{\mathit{\eta}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{L}(L-x){\left({\scriptscriptstyle \frac{{\mathrm{d}}^{\mathrm{2}}w}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}x+b\left({x}_{i}\right)\end{array}}}}\end{array}$$

where

$$\begin{array}{ll}{\displaystyle}b\left({x}_{i}\right)& {\displaystyle}={\left.{\mathit{\eta}}^{\mathrm{2}}{\left({\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)}^{\mathrm{2}}\right|}_{x=\mathrm{0}}^{x=L}-{\left.{\mathit{\eta}}^{\mathrm{2}}(L-x){\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}{\displaystyle \frac{{d}^{\mathrm{2}}w}{d{x}^{\mathrm{2}}}}\right|}_{x=\mathrm{0}}^{x=L}\\ {\displaystyle}& {\displaystyle}+{\mathit{\eta}}^{\mathrm{2}}w{\displaystyle \frac{{d}^{\mathrm{2}}}{\mathrm{d}{x}^{\mathrm{2}}}}{\left.\left((L-x){\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)\right|}_{x=\mathrm{0}}^{x=L}-(L-x){\left.\left(w{\displaystyle \frac{\mathrm{d}w}{\mathrm{d}x}}\right)\right|}_{x=\mathrm{0}}^{x=L}\end{array}$$

Following dimensionless variables are introduced:

$$\begin{array}{ll}{\displaystyle}& {\displaystyle}X={\displaystyle \frac{x}{L}},\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}W={\displaystyle \frac{w}{L}},\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}\mathit{\mu}={\displaystyle \frac{\mathit{\eta}}{L}},\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}p={\displaystyle \frac{P{L}^{\mathrm{2}}}{EI}},\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}q={\displaystyle \frac{Q{L}^{\mathrm{3}}}{EI}},\\ \text{(15)}& {\displaystyle}& {\displaystyle}{k}_{{\mathrm{r}}_{i}}={\displaystyle \frac{{K}_{{\mathrm{r}}_{i}}L}{EI}},\phantom{\rule{0.25em}{0ex}}\phantom{\rule{0.25em}{0ex}}{k}_{\mathrm{t}}={\displaystyle \frac{{K}_{\mathrm{t}}{L}^{\mathrm{3}}}{EI}}\end{array}$$

Dimensionless Rayleigh quotient for the case *p*>0, *q*=0 can be expressed as

$$\begin{array}{}\text{(16)}& {\displaystyle}p={\displaystyle \frac{{\displaystyle \begin{array}{c}{\int}_{\mathrm{0}}^{\mathrm{1}}{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}X+{\displaystyle \frac{L}{EI}}{b}_{\mathrm{1}}\left(W\left({X}_{i}\right)\right)\\ -{\left.\left(\frac{\mathrm{d}W}{\mathrm{d}X}\frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}+{\left.\left(W\frac{{\mathrm{d}}^{\mathrm{3}}W}{\mathrm{d}{X}^{\mathrm{3}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\end{array}}}{{\scriptscriptstyle \begin{array}{c}{\int}_{\mathrm{0}}^{\mathrm{1}}{\left(\frac{\mathrm{d}W}{\mathrm{d}X}\right)}^{\mathrm{2}}\mathrm{d}X+{\mathit{\mu}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{\mathrm{1}}{\left(\frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}\right)}^{\mathrm{2}}\mathrm{d}X-{\mathit{\mu}}^{\mathrm{2}}{\left.\left(\frac{\mathrm{d}W}{\mathrm{d}X}\frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\\ +{\mathit{\mu}}^{\mathrm{2}}{\left.\left(W{\scriptscriptstyle \frac{{\mathrm{d}}^{\mathrm{3}}W}{\mathrm{d}{X}^{\mathrm{3}}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}-{\left.\left(W{\scriptscriptstyle \frac{\mathrm{d}W}{\mathrm{d}X}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\end{array}}}}\end{array}$$

Dimensionless Rayleigh quotient for *q*>0, *p*=0 is given by

$$\begin{array}{}\text{(17)}& q={\displaystyle \frac{{\displaystyle \begin{array}{c}{\int}_{\mathrm{0}}^{\mathrm{1}}{\left({\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{x}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}X+{\displaystyle \frac{L}{EI}}{B}_{\mathrm{1}}\left(w\left({X}_{i}\right)\right)\\ -{\left.\left(\frac{\mathrm{d}W}{\mathrm{d}X}\frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}+{\left.\left(W\frac{{\mathrm{d}}^{\mathrm{3}}W}{\mathrm{d}{X}^{\mathrm{3}}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\end{array}}}{{\scriptscriptstyle \begin{array}{c}{\int}_{\mathrm{0}}^{\mathrm{1}}(\mathrm{1}-X){\left(\frac{\mathrm{d}W}{\mathrm{d}X}\right)}^{\mathrm{2}}\mathrm{d}X-{\mathit{\mu}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{\mathrm{1}}\frac{\mathrm{d}W}{\mathrm{d}X}\frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}\mathrm{d}X\\ +{\mathit{\mu}}^{\mathrm{2}}{\int}_{\mathrm{0}}^{\mathrm{1}}(\mathrm{1}-X){\left({\scriptscriptstyle \frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}}\right)}^{\mathrm{2}}\mathrm{d}X+b\left({X}_{i}\right)\end{array}}}}\end{array}$$

where

$$\begin{array}{ll}{\displaystyle}b\left({X}_{i}\right)& {\displaystyle}={\left.{\mathit{\mu}}^{\mathrm{2}}{\left({\displaystyle \frac{\mathrm{d}W}{\mathrm{d}X}}\right)}^{\mathrm{2}}\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}-{\left.{\mathit{\mu}}^{\mathrm{2}}(\mathrm{1}-X){\displaystyle \frac{\mathrm{d}W}{\mathrm{d}X}}{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}W}{\mathrm{d}{X}^{\mathrm{2}}}}\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\\ {\displaystyle}& {\displaystyle}+{\mathit{\mu}}^{\mathrm{2}}W{\displaystyle \frac{{\mathrm{d}}^{\mathrm{2}}}{\mathrm{d}{X}^{\mathrm{2}}}}{\left.\left((\mathrm{1}-X){\displaystyle \frac{\mathrm{d}W}{\mathrm{d}X}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\\ {\displaystyle}& {\displaystyle}-(\mathrm{1}-X){\left.\left(W{\displaystyle \frac{\mathrm{d}W}{\mathrm{d}X}}\right)\right|}_{X=\mathrm{0}}^{X=\mathrm{1}}\end{array}$$

5 Method of solution

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Numerical results are obtained by Rayleigh–Ritz method based on the weak formulation of the problem given in Sect. 3 and the Rayleigh quotients given in Sect. 4. Variational methods of solution of differential equations have been outlined in a number of books (Reddy, 2002; Wunderlich and Pilkey, 2003; Cassel, 2013) and are not detailed here. The essence of the method involves approximating the solution of a differential equation by polynomials using the weak formulation of the problem given by Eq. (8). In the present study, Chebyshev polynomials are employed as the approximating functions expressed as

$$\begin{array}{}\text{(18)}& W\left(X\right)={X}^{r}(\mathrm{1}-X{)}^{s}\sum _{j=\mathrm{1}}^{N}{c}_{j}{f}_{j-\mathrm{1}}(X)\end{array}$$

where *r* and *s* take the values 0, 1 or 2 for free, simply supported and
clamped boundaries, respectively. Parameters *c*_{j} are determined as part
of the solution of an eigenvalue problem which yields the buckling load as
the minimum of the eigenvalues. In Eq. (18), *f*_{j}(*X*) is the *j*th
Chebyshev polynomial with *f*_{0}(*X*)=1 and *f*_{1}(*X*)=*X*. The remaining
terms are obtained from

$$\begin{array}{}\text{(19)}& {f}_{j+\mathrm{1}}\left(X\right)=\mathrm{2}X{f}_{j}\left(X\right)-{f}_{j-\mathrm{1}}\left(X\right)\end{array}$$

As noted in Ghannadpour et al. (2013), Chebyshev polynomials provide a set of complete and orthogonal series which leads to rapid convergence as compared to other polynomial series. Furthermore they can be expressed in a relatively simple and uniform form making the coding easier. Fourier series method can also be used effectively as shown in Kadıoglu and Yaylı (2017) where the buckling problem for a nonlocal Timoshenko beam was solved using Fourier series approach.

The polynomial approximation method implemented in the present study to solve
the buckling problem for elastically restrained nanotubes is applied to the
buckling of elastically restrained columns in order to assess and verify its
accuracy. The specific problem involves an elastically restrained column
subject to a tip load only, i.e., *p*>0 and *q*=0. Numerical results for this
problem are given in Wang et al. (2005). Comparative results are given in
Table 1 involving a column with a rotational spring constant *k*_{r0} at *x*=0 and a rotational spring constant *k*_{r1} at *x*=*L* with
no translation of the boundary at *x*=*L*, i.e., *k*_{t}=∞.
Corresponding results for a column with free end at *x*=*L* (*k*_{t}=0)
are given in Table 2. Solutions obtained with the present method are observed
to be quite accurate judging from the comparison of the present results with
the ones given in Wang et al. (2005) as shown in Tables 1 and 2.

6 Numerical results

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In this section the effect of the elastic restraints on the buckling loads of
nonlocal nanotubes is investigated by means of contour plots. Furthermore the
buckling loads of nanotubes under a tip load and a distributed load are
compared. The numerical results are given in terms of the small scale
parameter *μ* with the range taken as $\mathrm{0}\le \mathit{\mu}\le \mathrm{0.4}$. The contour
plots of the buckling load *p* with respect to *μ* and *k*_{r0}
are shown in Fig. 2 for the case *k*_{r1}=0, *k*_{t}=10^{8}, i.e., the end point *x*=*L* is simply supported. It is observed that
the buckling load increases as the rotational spring at *x*=0 becomes stiffer
as expected. However this increase becomes minor after a certain value of
*k*_{r0} depending on the small scale parameter *μ*. The
buckling load increases most as *k*_{r0} increases at low values of
*μ*. Increase in the buckling load with increasing *k*_{r0} is
much less as *μ* approaches *μ*=0.4. The corresponding results for
uniformly distributed axial load *q* are shown in Fig. 3. The trends are the
same as the concentrated load case shown in Fig. 2. However, the decrease in
the buckling load as *μ* increases is more pronounced.

Next contour plot of the buckling load under the concentrated load *p* is
shown with respect to *μ* and *k*_{r1} in Fig. 4 for a
nanocolumn clamped at *x*=*L*. A comparison of Figs. 2 and 4 shows that in this
case increase in the buckling load as *k*_{r1} increases is more
pronounced, but the increase tapers of quickly as *μ* increases. The
corresponding results for uniformly distributed axial load *q* are shown in
Fig. 5 where the increase in the buckling load as *k*_{r1}
increases is mostly observed for the low values of *μ*. This increase in
the buckling load as *k*_{r1} increases is observed to be of minor
magnitude. Figure 6 shows the contour plot for the concentrated load *p* for
a clamped-pinned nanocolumn with respect to *μ* and *k*_{t}
which is the translational spring at *x*=*L*. As *k*_{t} increases,
the buckling load *p* increases substantially for low values of *μ* with
this increase tapering off quickly as *μ* increases. The corresponding
results for uniformly distributed axial load *q* are shown in Fig. 7 where
the increase in *q* as *k*_{t} increases is observed to be less
pronounced as compared to *p*. At high values of *μ* the increase in *q*
is considerably less as *k*_{t} increases.

Stability boundaries with respect to *q* and *p* are shown in Fig. 8 for a
simply supported nanocolumn for several values of *μ*. As expected
stability boundary approaches the origin as *μ* increases.

7 Conclusions

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Buckling of elastically restrained nanotubes subject to concentrated and
uniformly distributed axial loads was studied. The elastic restraint at *x*=0
is specified as a rotational spring and its value changes between a simply
supported column (*k*_{r0}=0) and clamped column (*k*_{r0}→0). The elastic restraints at *x*=*L* are specified as a rotational spring
$\mathrm{0}\le {k}_{\mathrm{r}\mathrm{1}}<\mathrm{\infty}$ and a translational spring $\mathrm{0}\le {k}_{\mathrm{t}}<\mathrm{\infty}$. The value of *k*_{r1} changes between a
simply supported column (*k*_{r1}=0) and a clamped column
(*k*_{r1}→∞). Thus the boundary conditions at *x*=*L* can
vary between a simple support and a clamped support. Numerical results are
obtained by Rayleigh–Ritz method employing Chebyshev polynomials of the
first kind as the approximating functions. The accuracy of the present method
of solution is verified by comparing the numerical results with available
results on local columns available in the literature.

The numerical results are given mostly in the form of contour plots to study
the effect of the small scale parameter *μ* and elastic restraints on the
buckling loads. It is observed that the effect of the elastic restraints on
the buckling load decreases as the small scale parameter increases. Buckling
loads are observed to be more sensitive to the changes in the values of the
elastic constants when the small-scale parameter is *μ*≥0.1.

Data availability

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Data availability.

The data was used to generate the graphs in Figs. 2 to 8. Thus these figures contain the data of the present research. The numerical data can be made available upon request from the authors.

Author contributions

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Author contributions.

MTAR and SA worked on the model jointly and have chosen the Rayleigh-Ritz method and Chebyshev polynomials to obtain the numerical results. MTAR prepared the Figs. 1–8. MTAR and SA contributed to the writing of the article and agreed on the final form of the manuscript.

Competing interests

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Competing interests.

The authors declare that they have no conflict of interest.

Acknowledgements

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Acknowledgements.

The research reported in this paper was supported by research grants from the University of KwaZulu-Natal (UKZN) and from National Research Foundation (NRF) of South Africa. The authors gratefully acknowledge the supports provided by UKZN and NRF.

Review statement

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Review statement.

This paper was edited by Anders Eriksson and reviewed by Stefan Kaczmarczyk and two anonymous referees.

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Short summary

Nanoscale components are used extensively in a variety of nanotechnology applications. In particular, carbon nanotubes (CNTs) are used in diverse fields due their superior properties. For specific applications, their mechanical behaviour under loading needs to be investigated. Buckling of CNTs is a critical failure mode and in the present study, nonlocal continuum mechanics is employed to investigate their buckling behaviour subject to elastically restrained boundary conditions.

Nanoscale components are used extensively in a variety of nanotechnology applications. In...

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