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Effects of the slip boundary condition on dynamics and pull-in instability of carbon nanotubes conveying fluid

Abstract

This paper addresses the effects of the slip boundary condition on dynamics and pull-in instability of carbon nanotubes (CNTs) containing internal fluid flow. Both the clamped–clamped and the cantilever boundary conditions are considered. The structure of CNTs is modelled using the size-dependent strain gradient theory (SGT) of continuum mechanics. It is shown that the Knudsen number (Kn) has a significant effect on the static and dynamic CNT response due to pull-in voltage loading and the existence of the instability region.

Introduction

CNTs attract much attention nowadays due to their superior mechanical, thermal and electrical properties and also their numerous applications (Iijima 1991; Yamamoto et al. 2012; Umeda et al. 2012; Xu et al. 2012; Che et al. 1998; Evans et al. 1996). A remarkable number of studies in this field have been conducted, especially concerning the fluid–structure interaction. For instance, Yoon et al. (2005) studied free vibration and instability of CNTs with internal fluid. Wang et al. (2008) investigated buckling instability considering the effect of the Van der Waals force, and Zhang and Fang (Zhen and Fang 2010) presented the thermal and nonlocal effects on vibration for both CNT and the conveyed fluid. The aspect ratio, the viscosity effect and elastic medium parameters, as well as the nonlocal effect, were considered by Chang and Lee (2009). Kaviani and Mirdamadi (2013) studied the wave propagation phenomena in CNTs with internal fluid, using the strain/inertia gradient theory and considering the slip boundary condition and Knudsen number in the solid–fluid interaction. Furthermore, in Kaviani and Mirdamadi (2012), they presented the effect of Kn and the slip boundary condition coupling on the viscosity of the nanofluid which passes through a CNT.

Generally, we can distinguish the following regimes of flow (Kaviani and Mirdamadi 2012; Mirramezani and; Mirdamadi 2012; Kucaba-Piętal 2004): (1) 0 < Kn < 10− 2 for the continuum flow regime; (2) 10− 2<Kn < 10− 1for the slip flow regime; (3) 10− 1 < Kn < 10 for the transition flow regime; and (4) Kn > 10 for the free molecular flow regime. In this paper, we consider the interval 0 < Kn < 10− 1. It contains both the continuum and the slip flow regimes. From the point of view of modelling, the commonly known governing equations for the conventional fluid–structure interaction problems result from the assumption of no-slip boundary conditions. However, if we consider the influence of Kn on the CNT behaviour, this condition is no longer valid. Therefore, we have to use the conventional Navier–Stokes equations satisfying the slip boundary conditions on the tube walls and then find out an average velocity correction factor that relates the average velocity of the no-slip and the slip boundary conditions to each other.

The effects of the slip and no-slip boundary conditions, and Kn can be found in the literature. Kaviani et al. (Kaviani and Mirdamadi 2012) studied the effects of Kn and the slip boundary condition for a nanoflow passing through a nanotube. Mirramezani et al. (Mirramezani and Mirdamadi 2012a, b) studied vibrational behaviour of CNTs considering small-size effects for both the slip boundary condition on fluid flow and the solid structure using the Euler–Bernoulli plug flow theory. Wave propagation of CNTs conveying fluid was studied by Kaviani et al. (Kaviani and Mirdamadi 2013) in which the slip boundary condition was considered based on the gradient theory of continuum mechanics. Mirramezani et al. (2013) proposed a new model for 1D coupled vibrations of CNTs conveying fluid in which they took into account the slip boundary condition using Kn and the size-dependent continuum theories.

Research in nanotechnology is often multidisciplinary. For instance, the study of micro/nanoelectromechanical systems (MEMS and NEMS) is an important research area which includes the concepts of basic sciences as well as mechanical and electrical engineering. The most effective and applicable technique to actuate NEMS is the electrostatic actuation method (Fakhrabadi et al. 2013). Dequesnes et al. (2002, 2004) investigated the deflection and the static pull-in of CNTs under electrostatic actuation considering the Van der Waals force. Rasekh and Khadem (Rasekh et al. 2010) studied the static and dynamic behaviour of CNTs under the electrostatic and Van der Waals force. Ouakad and Younis (2010) studied the nonlinear dynamics of CNTs with the clamped–clamped and the cantilever boundary conditions under DC and AC electrical excitations. Hajnayeb et al. (Hajnayeb and Khadem 2012) presented forced vibration of a double-wall CNT under the axial force and AC–DC complex electrostatic actuations. Fakhrabadi et al. (2013) investigated the influence of the fluid flow on static and dynamic behaviour of electrostatically actuated CNTs with cantilever and doubly clamped boundary conditions, using SGT. More recently, some researchers have studied the vibration and instability of nano- and micro-tubes conveying fluid (Ghazavi and Molki 2018; Guo et al. 2018; Zhang et al. 2017, 2016; Wang et al. 2016).

The main purpose of this paper is to study the effects of the slip and no-slip boundary conditions on the pull-in instability and dynamics of the clamped–clamped and the cantilever CNTs conveying fluid, utilizing the SGT, to consider the small-scale effect of the nano-structure. The value of Kn is in the interval 0 < Kn < 10− 1 ,which includes the slip boundary conditions on the CNT wall. We show the effect of the fluid velocity on the static and dynamic pull-in instability in the presence of different values of Kn. Finally, we study the effects of the slip and no-slip boundary conditions on the flutter (dynamic instability) and the buckling (static instability) of the CNTs under the electrostatic force.

System description and mathematical formulation

We consider a fluid conveying CNT (Fig. 1). The CNT is clamped over a metal plate with an initial gap (G0). A potential difference (V) is applied to the CNT (the positive electrode) and the metal plate (the negative electrode). Thus, the CNT is subjected to an electrostatic distributed load. Generally, the value of this electrostatic force is associated with the deflections of the CNT. The deflection corresponds to the applied voltage as long as the elastic force of the CNT can balance the attractive force resulting from the applied voltage. However, at some point the tip of the cantilevered CNT or the centre of the doubly clamped CNT suddenly drops on the metal plate. This phenomenon is called pull-in instability and the corresponding voltage is called the pull-in voltage.

Fig. 1
figure1

A schematic diagram of electrostatically actuated CNTs conveying fluid

Since the classical elasticity theory often fails to predict the mechanical behaviour of the micro/nanostructures precisely, some researchers have tried to develop non-classical elasticity theories to enhance the accuracy and capability of numerical modelling techniques to predict of desired behaviour. According to the SGT, the strain energy U of an isotropic linear elastic material with volume Ω under an infinitesimal deformation can be formulated as follows (Kahrobaiyan et al. 2011):

$${U_{\text{s}}}=\frac{1}{2}\int {\int {\int_{\Omega } {\left( {{\sigma _{ij}}{\varepsilon _{ij}}+{P_i}{\gamma _j}+\tau _{{ijk}}^{{(1)}}\eta _{{ijk}}^{{(1)}}+{m^s}_{{ij}}{\chi ^s}_{{ij}}} \right){\text{d}}V} } } ,$$
(1)

where \({\varepsilon _{ij}},{\gamma _j},\eta _{{ijk}}^{{(1)}},\chi _{{ij}}^{s}\) denote components of the strain tensor, P is the dilatation gradient vector, γ is the deviatoric stretch, \({\eta _1}\) the gradient tensor, and \({\chi ^s}\) is the symmetric part of the rotation gradient tensor. They are defined by the following relations:

$${\varepsilon _{ij}}=\frac{1}{2}\left( {{\partial _i}u{}_{j}+{\partial _j}{u_i}} \right),$$
(2)
$$\begin{aligned} {\eta ^{(1)}}_{{ijk}} & =\frac{1}{3}\left( {{\partial _i}{\varepsilon _{jk}}+{\partial _j}{\varepsilon _{ki}}+{\partial _k}{\varepsilon _{ij}}} \right) - \frac{1}{{15}}\left[ {{\delta _{ij}}\left( {{\partial _k}{\varepsilon _{mm}}+2{\partial _j}{\varepsilon _{mk}}} \right)} \right. \\ & \left. {\quad +{\delta _{jk}}\left( {{\partial _i}{\varepsilon _{mm}}+2{\partial _m}{\varepsilon _{mi}}} \right)+{\delta _{ki}}\left( {{\partial _j}{\varepsilon _{mm}}+2{\partial _m}{\varepsilon _{mj}}} \right)} \right], \\ \end{aligned}$$
(3)
$${\gamma _i}={\partial _i}{\varepsilon _{mm}},$$
(4)
$${\chi ^s}_{{ij}}=\frac{1}{2}\left( {{e_{ipq}}{\partial _p}{\varepsilon _{qj}}+{e_{jpq}}{\partial _p}{\varepsilon _{qi}}} \right),$$
(5)
$${\theta _i}=\frac{1}{2}{[{\text{curl}}(u)]_i},$$
(6)

where \(u{}_{i},{\theta _i}\) denote the components of the displacement vector and infinitesimal rotation vector, respectively. The conjugated force parameters for \(\varepsilon ,\gamma ,{\eta ^{(1)}}\) and\({\chi ^s}\) are denoted by \(\sigma ,P,{\tau ^{(1)}}\) and \({m^s}\), respectively, where the first one is the classical stress tensor and the next ones are the higher order stresses. They are defined as follows (Kahrobaiyan et al. 2011):

$${\sigma _{ij}}=\lambda tr(\varepsilon ){\delta _{ij}}+2G{\varepsilon _{ij}},$$
(7)
$${p_i}=2l_{0}^{2}G{\gamma _j},$$
(8)
$$\tau _{{ijk}}^{{(1)}}=2l_{0}^{2}G\eta _{{ijk}}^{{(1)}},$$
(9)
$${m_{ij}}=2l_{2}^{2}G{\chi _{ij}},$$
(10)

where \(\lambda\) and \(\mu\) are Lame’s constants and \({l_0},{l_1},{l_2}\) are the material length scale parameters corresponding to the dilatation gradient, the deviatoric stretch gradient and the rotation gradient, respectively. Substituting Eqs. (710) into Eq. (1), applying the Hamilton principle and using some mathematical calculations, we obtain the equation of motion of the CNT (Fakhrabadi et al. 2014):

$$S\frac{{{\partial ^4}w}}{{\partial {x^4}}} - K\frac{{{\partial ^6}w}}{{\partial {x^6}}} - N\frac{{{\partial ^2}w}}{{\partial {x^2}}}+m\frac{{{\partial ^2}w}}{{\partial {t^2}}}+c\frac{{\partial w}}{{\partial t}}=q(x,t),$$
(11)

where

$$S={\text{EI}}+{\text{GA}}\left( {2l_{0}^{2}+\frac{{120}}{{225}}l_{1}^{2}+l_{2}^{2}} \right),$$
(12)
$$K={\text{GI}}\left( {2l_{0}^{2}+\frac{4}{5}l_{1}^{2}} \right),\quad m=\rho A,$$
(13)
$$N={N_0}+\frac{{EA}}{{2L}}\int\limits_{0}^{L} {{{\left( {\frac{{\partial w}}{{\partial x}}} \right)}^2}{\text{d}}x} ,$$
(14)
$$q(x,t)={q_{{\text{fluid}}}}+{q_{{\text{elec}}}},$$
(15)

and \(E,I,G,A,w,x,N,c,L\), and t are elastic modulus, moment of inertia, shear modulus, cross-sectional area, deflection, axial coordinate, axial force, damping coefficient, length of the CNT, and time, respectively.

Next, we define the boundary conditions for cantilever and doubly clamped CNTs with Eqs. (16) and (17), respectively:

$$\begin{aligned} w(0,t) & =\frac{{\partial w(0,t)}}{{\partial x}}=\frac{{{\partial ^2}w(0,t)}}{{\partial {x^2}}}=0, \\ & \quad - K\frac{{{\partial ^5}w(L,t)}}{{\partial {x^5}}}+S\frac{{{\partial ^3}w(L,t)}}{{\partial {x^3}}}=0, \\ & \quad - K\frac{{{\partial ^4}{w_i}(L,t)}}{{\partial {x^4}}}+S\frac{{{\partial ^2}w(L,t)}}{{\partial {x^2}}}=0, \\ K\frac{{{\partial ^3}w(L,t)}}{{\partial {x^3}}} & =0, \\ \end{aligned}$$
(16)
$$\begin{aligned} w(0,t) & =\frac{{\partial w(0,t)}}{{\partial x}}=\frac{{{\partial ^2}w(0,t)}}{{\partial {x^2}}}=0, \\ w(L,t) & =\frac{{\partial w(L,t)}}{{\partial x}}=\frac{{{\partial ^2}w(L,t)}}{{\partial {x^2}}}=0. \\ \end{aligned}$$
(17)

The distributed external force in Eq. (11) comprises the electrostatic force and the force which results from the fluid flow through the CNT.

The electrostatic force can be written as (Dequesnes et al. 2002)

$${q_{{\text{elec}}}}=\frac{{\pi {\varepsilon _0}{V^2}}}{{\sqrt {({G_0} - w)({G_0} - w+2R)} \arccos {h^2}\left( {1+\frac{{{G_0} - w}}{R}} \right)}},$$
(18)

where \({\varepsilon _0},V,R\) and \({G_0}\) represent the electrical permittivity of the vacuum (= 8.854 PF), voltage, the radius of the CNT and the initial gap, respectively.

The force resulting from the fluid flow including the slip boundary condition can be obtained as follows:

We follow the considerations by Beskok and Karniadakis (1999). Within this model, the equation based on experimental data is postulated in the following form:

$${U_s} - {U_w}=\left( {\frac{{2 - {\sigma _v}}}{{{\sigma _v}}}} \right)\left( {\frac{{Kn}}{{1 - bKn}}} \right){\left( {\frac{{\partial U}}{{\partial n}}} \right)_{r=R}},$$
(19)

where b is a general slip coefficient. Choosing b = − 1, Us is the slip velocity of the fluid near the CNT wall surface, Uw is the axial rigid body solid wall velocity, and n is the outward unit vector normal to the CNT wall surface. The parameter σv is the tangential momentum accommodation coefficient and is assumed to be 0.7 for practical purposes (Shokouhmand et al. 2010).

In this paper, Eq. (19) is used to model the slip velocity boundary condition in the Navier–Stokes equations. Up to now, for conventional FSI problems, no-slip boundary conditions were considered, in which the influence of Kn on CNTs was not included. Thus, the conventional Navier–Stokes equations are used but the slip boundary conditions on the tube walls are satisfied and an average velocity correction factor is established, which relates to the average velocity of the no-slip and slip boundary conditions.

Therefore, a fully developed, incompressible, viscous fluid flow of constant density and viscosity is considered. Since the Newtonian fluid with a constant pressure gradient and negligible effect of gravitational body force is taken into account, the Navier–Stokes equations are  (Shames 1962):

$$\rho \frac{{D\overrightarrow U }}{{Dt}}= - \nabla \overrightarrow P +\mu {\nabla ^2}\overrightarrow U +{\overrightarrow F _{{\text{body}}}},$$
(20)

where ρ is the mass fluid density, P is pressure, and \(\frac{D}{{Dt}}\) is the material derivative. In the slip regime, the effective viscosity of the fluid is considered, which, according to Beskok and Karniadakis model (Beskok and Karniadakis 1999) is:

$$\begin{aligned} {\mu _e} & =\mu Cr(Kn), \\ Cr & =\left( {\frac{1}{{1+\alpha Kn}}} \right), \\ \end{aligned}$$
(21)

where the coefficient α can vary from zero to a constant value, according to the formula (Karniadakis et al. 2006):

$$\alpha ={\alpha _0}\frac{2}{\pi }\left[ {{{\tan }^{ - 1}}\left( {{\alpha _1}K{n^B}} \right)} \right],$$
(22)

where \({\alpha _1}=4\) and \(B=0.04\) are experimental data and \({\alpha _0}\) can be obtained from the free molecular regime:

$$\mathop {\lim }\limits_{{Kn \to \infty }} \alpha ={\alpha _0}=\frac{{64}}{{3\pi \left( {1 - \frac{4}{b}} \right)}}.$$
(23)

The solution of Eq. (20) in the axial direction of cylindrical orthogonal coordinates is  (Shames 1962):

$$U=\frac{1}{{4{\mu _e}}}\left( {\frac{{\partial p}}{{\partial x}}} \right){r^2}+C.$$
(24)

Hence, to obtain C, we use Eq. (19):

$${U_{r=R}}= - R\left( {\frac{{2 - {\sigma _v}}}{{{\sigma _v}}}} \right)\left( {\frac{{Kn}}{{1 - bKn}}} \right){\left( {\frac{{\partial U}}{{\partial n}}} \right)_{r=R}},$$
(25)

where R is the inner radius of the CNT. Substituting Eq. (25) into Eq. (26) leads to the slip and no-slip velocities:

$$\begin{aligned} {U_{{\text{slip}}}} & =\frac{1}{{4{\mu _0}Cr(Kn)}}\left( {\frac{{\partial p}}{{\partial x}}} \right)\left[ {{r^2} - {R^2} - 2{R^2}\left( {\frac{{2 - {\sigma _v}}}{{{\sigma _v}}}} \right)\left( {\frac{{Kn}}{{1 - bKn}}} \right)} \right], \\ {U_{{\text{no-slip}}}} & =\frac{1}{{4{\mu _0}}}\left( {\frac{{\partial p}}{{\partial x}}} \right)\left( {{r^2} - {R^2}} \right). \\ \end{aligned}$$
(26)

The VCF coefficients are defined as follows:

$${\text{VCF}}=\frac{{{U_{{\text{avg-slip}}}}}}{{{U_{{\text{avg-noslip}}}}}}=\frac{1}{{Cr(Kn)}}\left( {4\left( {\frac{{2 - {\sigma _v}}}{{{\sigma _v}}}} \right)\left( {\frac{{Kn}}{{1 - bKn}}} \right)+1} \right).$$
(27)

Finally, the following equation for external force due to the fluid flow is obtained  (Wang and Ni 2009):

$$\begin{aligned} {q_{{\text{fluid}}}} & =\left[ {{m_f}{{({\text{VCF}})}^2}U_{{{\text{avg-noslip}}}}^{2}+{P^*}A} \right]\frac{{{\partial ^2}w}}{{\partial {x^2}}} - 2{m_f}({\text{VCF}}){U_{{\text{avg-noslip}}}}\frac{{{\partial ^2}w}}{{\partial x\partial t}} \\ & \quad - {m_f}\frac{{{\partial ^2}w}}{{\partial {t^2}}}+\mu (Cr){A_i}\frac{{{\partial ^3}w}}{{\partial {x^2}\partial t}}+\mu (Cr)({\text{VCF}}){U_{{\text{avg-noslip}}}}{A_i}\frac{{{\partial ^3}w}}{{\partial {x^3}}}, \\ \end{aligned}$$
(28)

where \({m_f},{P^*},{m_c},\mu\) and \({A_i}\) represent the fluid mass, fluid pressure, mass of the CNT per unit length, fluid viscosity and fluid cross-section, respectively. Substituting Eqs. (28) and (18) into Eq. (11) leads to the equation of motion of a CNT conveying fluid:

$$\begin{aligned} & S\frac{{{\partial ^4}w}}{{\partial {x^4}}} - K\frac{{{\partial ^6}w}}{{\partial {x^6}}}+\left( {{m_f}{{({\text{VCF}})}^2}U_{{{\text{avg-noslip}}}}^{2}+{P^*}A - N} \right)\frac{{{\partial ^2}w}}{{\partial {x^2}}} \\ & \quad +2{m_f}({\text{VCF}}){U_{{\text{avg-noslip}}}}\frac{{{\partial ^2}w}}{{\partial x\partial t}}+\left( {{m_c}+{m_f}} \right)\frac{{{\partial ^2}w}}{{\partial {t^2}}} - \mu (Cr)A\frac{{{\partial ^3}w}}{{\partial {x^2}\partial t}} \\ & \quad - \mu (Cr)A({\text{VCF}}){U_{{\text{avg-noslip}}}}\frac{{{\partial ^3}w}}{{\partial {x^3}}}+c\frac{{\partial w}}{{\partial t}}={q_{{\text{elec}}}}, \\ \end{aligned}$$
(29)

where \(\left( {{P^*}A - N} \right)\frac{{{\partial ^2}w}}{{\partial {x^2}}}\) is equal to zero for the CNTs.

Solution

We define the following non-dimensional parameters:

$$\hat {w}=\frac{w}{{{G_0}}},\;\;\hat {x}=\frac{x}{{{G_0}}},\;\;\overset{\lower0.5em\hbox{$\smash{\scriptscriptstyle\frown}$}}{R} =\frac{R}{{{G_0}}},\;\;\hat {t}=\frac{t}{{{t^*}}},\;\;{t^*}=\sqrt {\frac{{({m_c}+{m_f}){L^4}}}{{EI}}} ,\;\;{u_{{\text{avg}}}}={\left( {\frac{{{m_f}}}{{EI}}} \right)^{\frac{1}{2}}}L{U_{{\text{avg}}}}.$$
(30)

Substituting the above non-dimensional parameters into Eq. (30), we have:

$$\begin{aligned} & \frac{{{\partial ^4}\hat {w}}}{{\partial {{\hat {x}}^4}}} - {\alpha _1}\frac{{{\partial ^6}\hat {w}}}{{\partial {{\hat {x}}^6}}}+{\alpha _2}\frac{{{\partial ^2}\hat {w}}}{{\partial {{\hat {x}}^2}}}+\beta \frac{{{\partial ^2}\hat {w}}}{{\partial \hat {x}\partial \hat {t}}}+\gamma \frac{{{\partial ^2}\hat {w}}}{{\partial {{\hat {t}}^2}}} - \delta \frac{{{\partial ^3}\hat {w}}}{{\partial {{\hat {x}}^2}\partial \hat {t}}} \\ & \quad - \xi \frac{{{\partial ^3}\hat {w}}}{{\partial {{\hat {x}}^3}}}+\zeta \frac{{\partial \hat {w}}}{{\partial \hat {t}}}=\alpha {{\hat {q}}_{{\text{elec}}}}, \\ \end{aligned}$$
(31)

where the lateral displacement \(w(\hat {x},\hat {t})\) consists of a static part and a dynamic part:

$$\hat {w}(\hat {x},\hat {t})={\hat {w}_s}(\hat {x})+{\hat {w}_d}(\hat {x},\hat {t}).$$
(32)

Static analysis

Ignoring the inertia terms in Eq. (31), the static equation is represented by the relation:

$$\frac{{{\partial ^4}{{\hat {w}}_s}}}{{\partial {{\hat {x}}^4}}} - {\alpha _1}\frac{{{\partial ^6}{{\hat {w}}_s}}}{{\partial {{\hat {x}}^6}}}+{\alpha _2}\frac{{{\partial ^2}{{\hat {w}}_s}}}{{\partial {{\hat {x}}^2}}} - \xi \frac{{{\partial ^3}{{\hat {w}}_s}}}{{\partial {{\hat {x}}^3}}}=\alpha {\hat {q}_{elec}}(V,\hat {w}).$$
(33)

To solve the above equation, we use the step-by-step linearization method (SSLM) (Talebian et al. 2010), where the voltage and the deflection in the Kth step are VK and \({\hat {w}_K}\), and in the (K + 1)th step \({V_{K+1}}\) and \({\hat {w}_{K+1}}\). The resultant deflections in the (K + 1)th step can be written as

$$\begin{aligned} {V^{i+1}} & ={V^i}+\delta V, \\ {{\hat {w}}_s}^{{i+1}} & ={{\hat {w}}_s}^{i}+\delta \hat {w}~={{\hat {w}}_s}^{i}+\psi {\text{ }}(\hat {x})~. \\ \end{aligned}$$
(34)

Hence, for the (K + 1)th step, Eq. (33) can be rewritten as

$$\frac{{{\partial ^4}{{\hat {w}}^{K+1}}_{s}}}{{\partial {{\hat {x}}^4}}} - {\alpha _1}\frac{{{\partial ^6}{{\hat {w}}^{K+1}}_{s}}}{{\partial {{\hat {x}}^6}}}+{\alpha _2}\frac{{{\partial ^2}{{\hat {w}}^{K+1}}_{s}}}{{\partial {{\hat {x}}^2}}} - \xi \frac{{{\partial ^3}{{\hat {w}}^{K+1}}_{s}}}{{\partial {{\hat {x}}^3}}}=\alpha {\hat {q}_{{\text{elec}}}}\left( {{V^{K+1}},{{\hat {w}}^{K+1}}} \right).$$
(35)

Now, for the investigation of a small value of \(\delta V\), \(\psi (\hat {x})\)should be small enough; therefore, using the calculus of variation theory and Taylor’s series expansion about \({\hat {w}^K}\), and applying the truncation to its first order for a suitable value of \(\delta V\), it is possible to obtain desired accuracy. So, the linearized equations to calculate \(\psi (\hat {x})\) are:

$$\frac{{{\partial ^4}\psi }}{{\partial {{\hat {x}}^4}}} - {\alpha _1}\frac{{{\partial ^6}\psi }}{{\partial {{\hat {x}}^6}}}+{\alpha _2}\frac{{{\partial ^2}\psi }}{{\partial {{\hat {x}}^2}}} - \xi \frac{{{\partial ^3}\psi }}{{\partial {{\hat {x}}^3}}} - \alpha \frac{{\partial {{\hat {q}}_{{\text{elec}}}}}}{{\partial {{\hat {w}}^K}_{s}}}\psi - \alpha \frac{{\partial {{\hat {q}}_{{\text{elec}}}}}}{{\partial V}}\delta V=0.$$
(36)

The expansion theory is used to solve the above equation (Younis and Nayfeh 2003):

$$\psi (\hat {x})=\sum\limits_{{j=1}}^{N} {{a_j}{\varphi _j}(\hat {x})} ,$$
(37)

where \({\varphi _j}\) is the jth free vibration mode shape of the CNT. Substituting Eq. (37) into Eq. (36), multiplying both sides by \({\varphi _i}\) and applying the Galerkin method, we have:

$$\sum\limits_{{j=1}}^{N} {{K_{ij}}{a_j}={F_i}} ,\quad i=1, \ldots ,n,$$
(38)

where \({K_{ij}}=K_{{ij}}^{m}+K_{{ij}}^{f} - K_{{ij}}^{e}\) and \({F_i}\) are:

$$\begin{aligned} K_{{ij}}^{m} & =\int\limits_{0}^{1} {{\varphi _i}\varphi _{j}^{{i\upsilon }}} {\text{d}}\hat {x} - {\alpha _1}\int\limits_{0}^{1} {{\varphi _i}\varphi _{j}^{{\upsilon i}}} {\text{d}}\hat {x}, \\ K_{{ij}}^{f} & ={\alpha _2}\int\limits_{0}^{1} {{\varphi _i}\varphi _{j}^{\prime \prime }{\text{d}}\hat {x}} - \xi \int\limits_{0}^{1} {{\varphi _i}\varphi _{j}^{{\prime \prime \prime }}} {\text{d}}\hat {x}, \\ K_{{ij}}^{e} & =\alpha \frac{{\partial {{\hat {q}}_{{\text{elec}}}}}}{{\partial {{\hat {w}}^K}_{s}}}\int\limits_{0}^{1} {{\varphi _i}{\text{d}}\hat {x}} , \\ {F_i} & =\alpha \frac{{\partial {{\hat {q}}_{{\text{elec}}}}}}{{\partial V}}\delta V\int\limits_{0}^{1} {{\varphi _i}{\text{d}}\hat {x}} . \\ \end{aligned}$$
(39)

Dynamic analysis

To solve the dynamic behaviour of the CNTs conveying fluid under DC voltage, the expansion theory is applied to Eq. (31) as follows (Karniadakis et al. 2006):

$${w_d}(\hat {x},\hat {t})=\sum\limits_{{j=1}}^{N} {{\varphi _j}(\hat {x}){q_j}(\hat {t})} .$$
(40)

Next, substituting Eq. (40) into Eq. (31), multiplying both sides by \({\varphi _i}\) and applying the Galerkin method lead to:

$$\sum\limits_{{j=1}}^{N} {{M_{ij}}{{\ddot {q}}_j}(\hat {t})} +\sum\limits_{{j=1}}^{N} {{C_{ij}}{{\dot {q}}_j}(\hat {t})} +\sum\limits_{{j=1}}^{N} {{K_{ij}}{q_j}(\hat {t})} ={F_i},$$
(41)

where M, K, C and F are mass, stiffness, damping matrices and the force vector, respectively, and are defined as follows:

$$\begin{aligned} {M_{ij}} & =\gamma \int\limits_{0}^{1} {{\varphi _i}{\varphi _j}{\text{d}}\hat {x}} , \\ {K_{ij}} & =\int\limits_{0}^{1} {\varphi _{i}^{{\prime \prime \prime }}{\varphi _j}{\text{d}}\hat {x}} +{\alpha _2}\int\limits_{0}^{1} {\varphi _{i}^{{\prime \prime \prime }}{\varphi _j}{\text{d}}\hat {x}} - {\alpha _1}\int\limits_{0}^{1} {\varphi _{i}^{{\upsilon i}}{\varphi _j}{\text{d}}\hat {x}} - \xi \int\limits_{0}^{1} {\varphi _{i}^{{\prime \prime \prime }}{\varphi _j}{\text{d}}\hat {x},} \\ {C_{ij}} & =\beta \int\limits_{0}^{1} {\varphi _{i}^{\prime }{\varphi _j}{\text{d}}\hat {x}} +\zeta \int\limits_{0}^{1} {{\varphi _i}{\varphi _j}{\text{d}}\hat {x}} - \delta \int\limits_{0}^{1} {\varphi _{i}^{{\prime \prime }}{\varphi _j}{\text{d}}\hat {x}} , \\ {F_i} & =\alpha \int\limits_{0}^{1} {{\varphi _i}{{\hat {q}}_{{\text{elec}}}}(V,\hat {w}){\text{d}}\hat {x}} . \\ \end{aligned}$$
(41)

Due to the complexity of the self-excited nonlinear Eq. (41), this equation is solved step by step in the time domain. In other words, at each discrete time step, the nonlinear forcing vectors are calculated based on the results of the previous step. In this method, if the time steps are sufficiently small, acceptable results can be obtained.

Numerical results

This section presents the results obtained from Eq. (41).

Validation

To validate our results, two verification procedures have been performed. In Table 1, static pull-in voltage is compared with the results of Seyyed Fakhrabadi et al. (2013) and in Table 2 dynamic behaviour is compared with the results of Dai et al. (2015). Our results are in good agreement with those in the literature.

Table 1 The comparison of the static pull-in voltage of CNTs
Table 2 Comparison of the dynamic behaviour of CNTs (E = 7.56 GPa, G = 2.9 GPa, l = 0 µm, ρ = 1000 kg/m3, ρm = 970 kg/m3, b = 150 µm, h = 50 µm, bi = 67.9 µm, hi = 22.6, L = 30 nm)

In the next sections, we discuss the effects of Kn and the slip boundary condition on the dynamic and pull-in instability of the CNTs for C–F and C–C boundary conditions using the SGT. The material and geometrical properties of CNTs are as follows (Fakhrabadi et al. 2013): CNT Young’s modulus E = 1 TPa; shear modulus G = 0.4 TPa and mass density of CNT \({\rho _c}=2300\;{\text{kg}}\,{{\text{m}}^{ - 3}}\); gap distance G0 = 4 nm; radius R = 0.6785 nm; thickness h = 0.34 nm; length L = 50 nm and length scale parameters of SGT \({l_0}={l_1}={l_2}=0.2\;{\text{nm}}\); fluid mass density and viscous fluid are \({\rho _f}=1.169\;{\text{kg}}\;{{\text{m}}^{ - 3}}\) and \(\mu =3\, \times \,{10^{ - 7}}\;{\text{Pa}}\;{\text{s}}\), respectively (Kaviani and Mirdamadi 2012; Cengel 2007). 

Pull-in instability

The static pull-in voltage of cantilever and doubly clamped CNTs for no flow condition (u = 0), under continuum flow and with slip flow regimes, is shown in Figs. 2 and 3, respectively. As it was expected for no flow condition, the static pull-in voltage of the C–C CNT is higher than for the C–F CNT due to the stiffer structure of C–C CNT. It follows from Fig. 2 that the fluid flow increases the static pull-in voltage of the C–F CNT and decreases in the C–C CNT. This opposite effect of the fluid versus the axial force results from the fluid flow through the CNTs. For the cantilever boundary conditions, the axial force remains tensile because of the free end. The tensile force increases the stiffness of the CNT. However, for doubly clamped CNTs, the clamped ends transform the axial force to the compressive force and thus reduce the stiffness (Fakhrabadi et al. 2014). When the flow regime passes from its continuum condition to the slip flow regime, the axial force produced by the fluid flow increases, therefore, the static pull-in voltage in the slip flow regime decreases more and increases more compared to continuum flow regime in C–C and C–F CNTs, respectively.

Fig. 2
figure2

The effect of Knudsen number on the static pull-in behaviours of C–C CNTs using the SGT

Fig. 3
figure3

The effect of the Knudsen number on the static pull-in behaviour of C–F CNTs using the SGT

The effects of Kn on the dynamic pull-in voltage for three values of the flow speed (u = 1, 2 and 3) are shown for both C–C and C–F CNTs in Figs. 4 and 5, respectively. From Fig. 4, it can be concluded that increasing Kn causes a decrease of the pull-in voltage for different values of u and this decrease is more significant for larger values of u. Figure 5 shows that for the C–F CNT the Kn parameter has an opposite effect. Furthermore, these illustrations demonstrate that the effect of Kn on the dynamic pull-in voltage of the C–F CNT for different values of u is almost stable, whereas for the C–C CNT and larger values of u it is greater.

Fig. 4
figure4

The effect of the Knudsen number on the static pull-in of C–C CNTs for different values of flow speed

Fig. 5
figure5

The effect of the Knudsen number on the static pull-in behaviour of C–F CNTs for different values of flow speed

The instability regions

The stability boundaries for C–C and C–F CNTs are shown in Figs. 6 and 7, respectively. The diagrams are divided into two sub-regions (stable and unstable). As it can be seen from Fig. 6 for the C–C CNT case, when V < 8.6, buckling instability occurs due to the internal flow as u crosses the boundary from the left side. When 8.6 < V < 41.2, pull-in instability occurs when u crosses the boundaries from the left side, and finally for V > 41.2 the system is totally unstable for all values of the flow speed. Next, we conclude that when Kn increases the stable region decreases—this means that for the slip regime for constant voltage the system is unstable for smaller u than in the continuum regime and that the value of u which will make the system unstable is smaller as Kn increases. Note that for the C–C CNT the increase of Kn has almost no effect on the buckling instability boundary but decreases the pull-in instability boundary.

Fig. 6
figure6

The instability region in the (u, V) plane for a C–C CNT in different regimes

Fig. 7
figure7

Instability region in the (u, V) plane for a C–F CNT in different regimes

The instability and stability region diagram for the C–F CNT has a different shape compared to the diagram for the C–C CNT, as illustrated in Fig. 7. For the C–F CNT we have pull-in and flutter instabilities. Figure 7 shows that for a small value of V (V < 7.1) when u increases and crosses the boundary, it causes flutter instability in the system. Furthermore, for relatively large values of the applied voltage (7.1 < V < 21.8) the CNT is unstable when u is small (when u increases, the system will be stable and then unstable again). The effect of Kn is the same for the C–C CNT in which increasing Kn decreases the stable region. This means that the stable region for the slip regime is smaller than for continuum regime. Finally, when   V > 21.8, for the slip regime pull-in instability of the system occurs for smaller u versus the continuum regime, and u becomes smaller as Kn increases. On the other hand, flutter instability occurs for smaller u, too.

As a closing remark, notice that in the slip regime the effect of the flow speed on the stability and the instability of the system is greater than for continuum regime, and this effect is more pronounced as Kn increases. This means that for smaller change of u one can control stability of the system in the slip regime.

Conclusions

In this study, we investigated the static pull-in instability and the dynamics of CNTs conveying fluid assuming both the continuum and the slip flow regimes based on the SGT. Furthermore, we considered different boundary conditions on CNT, i.e. doubly clamped and cantilever boundary conditions. We studied the effect of the Kn parameter on the static pull-in voltage and we observed that the fluid flow increases and decreases the stiffness of the C–F and C–C CNTs, respectively, which results in greater and smaller static pull-in voltage. Moreover, the slip flow regime decreases more the pull-in voltage for C–C CNTs and increases it more for C–F CNTs compared to the continuum flow regime. In the slip flow regime these effects were magnified as Kn increased.

We studied the effects of Kn on the dynamic and stability regions of CNTs and we obtained the following results:

  • In the case of C–C CNT, the dynamic pull-in voltage of the slip flow regime is greater than in the continuum regime.

  • The increase of Kn results in higher increase of the pull-in voltage, especially for greater speed of the flow regime.

  • As Kn increases, the stability region becomes smaller, which means that the instability of the system will occur for smaller u compared to the continuum flow regime.

For C–F CNTs, the dynamic pull-in voltage decreases as the flow regime changes from continuum to slip. Similar to C–C CNTs, Kn has the same effect on the stability region in which for the slip flow regime smaller changes of speed could result in instable or stable versus continuum flow, and as Kn increases this interval is smaller.

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Acknowledgements

The third author acknowledges the support of the National Science Centre, Poland, under Grant No. 2017/27/B/ST8/00351.

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Rashidi, H., Rahimi, Z. & Sumelka, W. Effects of the slip boundary condition on dynamics and pull-in instability of carbon nanotubes conveying fluid. Microfluid Nanofluid 22, 131 (2018). https://doi.org/10.1007/s10404-018-2156-z

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Keywords

  • Cantilever Boundary Conditions
  • Carbon Nanotubes (CNT)
  • Slip Flow Regime
  • Continuous Regime
  • Kaviani