570 |
|
\dot x = J(x)\nabla _x H \label{introEquation:poissonHamiltonian} |
571 |
|
\end{equation} |
572 |
|
The most obvious change being that matrix $J$ now depends on $x$. |
573 |
– |
The free rigid body is an example of Poisson system (actually a |
574 |
– |
Lie-Poisson system) with Hamiltonian function of angular kinetic |
575 |
– |
energy. |
576 |
– |
\begin{equation} |
577 |
– |
J(\pi ) = \left( {\begin{array}{*{20}c} |
578 |
– |
0 & {\pi _3 } & { - \pi _2 } \\ |
579 |
– |
{ - \pi _3 } & 0 & {\pi _1 } \\ |
580 |
– |
{\pi _2 } & { - \pi _1 } & 0 \\ |
581 |
– |
\end{array}} \right) |
582 |
– |
\end{equation} |
583 |
– |
|
584 |
– |
\begin{equation} |
585 |
– |
H = \frac{1}{2}\left( {\frac{{\pi _1^2 }}{{I_1 }} + \frac{{\pi _2^2 |
586 |
– |
}}{{I_2 }} + \frac{{\pi _3^2 }}{{I_3 }}} \right) |
587 |
– |
\end{equation} |
573 |
|
|
574 |
|
\subsection{\label{introSection:exactFlow}Exact Flow} |
575 |
|
|
935 |
|
However, both of these methods are iterative and inefficient. In |
936 |
|
this section, we will present a symplectic Lie-Poisson integrator |
937 |
|
for rigid body developed by Dullweber and his |
938 |
< |
coworkers\cite{Dullweber1997}. |
954 |
< |
|
955 |
< |
\subsection{\label{introSection:lieAlgebra}Lie Algebra} |
938 |
> |
coworkers\cite{Dullweber1997} in depth. |
939 |
|
|
940 |
|
\subsection{\label{introSection:constrainedHamiltonianRB}Constrained Hamiltonian for Rigid Body} |
941 |
< |
|
941 |
> |
The motion of the rigid body is Hamiltonian with the Hamiltonian |
942 |
> |
function |
943 |
|
\begin{equation} |
944 |
|
H = \frac{1}{2}(p^T m^{ - 1} p) + \frac{1}{2}tr(PJ^{ - 1} P) + |
945 |
|
V(q,Q) + \frac{1}{2}tr[(QQ^T - 1)\Lambda ]. |
1011 |
|
\[ |
1012 |
|
V(q,Q) = V(Q X_0 + q). |
1013 |
|
\] |
1014 |
< |
Hence, |
1014 |
> |
Hence, the force and torque are given by |
1015 |
|
\[ |
1016 |
< |
\nabla _q V(q,Q) = F(q,Q) = \sum\limits_i {F_i (q,Q)} |
1016 |
> |
\nabla _q V(q,Q) = F(q,Q) = \sum\limits_i {F_i (q,Q)}, |
1017 |
|
\] |
1018 |
< |
|
1018 |
> |
and |
1019 |
|
\[ |
1020 |
|
\nabla _Q V(q,Q) = F(q,Q)X_i^t |
1021 |
|
\] |
1022 |
+ |
respectively. |
1023 |
|
|
1024 |
|
As a common choice to describe the rotation dynamics of the rigid |
1025 |
|
body, angular momentum on body frame $\Pi = Q^t P$ is introduced to |
1065 |
|
(\Lambda - \Lambda ^T ) . \label{introEquation:skewMatrixPI} |
1066 |
|
\end{equation} |
1067 |
|
Since $\Lambda$ is symmetric, the last term of Equation |
1068 |
< |
\ref{introEquation:skewMatrixPI}, which implies the Lagrange |
1069 |
< |
multiplier $\Lambda$ is ignored in the integration. |
1068 |
> |
\ref{introEquation:skewMatrixPI} is zero, which implies the Lagrange |
1069 |
> |
multiplier $\Lambda$ is absent from the equations of motion. This |
1070 |
> |
unique property eliminate the requirement of iterations which can |
1071 |
> |
not be avoided in other methods\cite{}. |
1072 |
|
|
1073 |
< |
Hence, applying hat-map isomorphism, we obtain the equation of |
1074 |
< |
motion for angular momentum on body frame |
1075 |
< |
\[ |
1076 |
< |
\dot \pi = \pi \times I^{ - 1} \pi + Q^T \sum\limits_i {F_i (r,Q) |
1077 |
< |
\times X_i } |
1078 |
< |
\] |
1073 |
> |
Applying hat-map isomorphism, we obtain the equation of motion for |
1074 |
> |
angular momentum on body frame |
1075 |
> |
\begin{equation} |
1076 |
> |
\dot \pi = \pi \times I^{ - 1} \pi + \sum\limits_i {\left( {Q^T |
1077 |
> |
F_i (r,Q)} \right) \times X_i }. |
1078 |
> |
\label{introEquation:bodyAngularMotion} |
1079 |
> |
\end{equation} |
1080 |
|
In the same manner, the equation of motion for rotation matrix is |
1081 |
|
given by |
1082 |
|
\[ |
1083 |
< |
\dot Q = Qskew(M^{ - 1} \pi ) |
1083 |
> |
\dot Q = Qskew(I^{ - 1} \pi ) |
1084 |
|
\] |
1085 |
|
|
1086 |
< |
The free rigid body equation is an example of a non-canonical |
1087 |
< |
Hamiltonian system. |
1086 |
> |
\subsection{\label{introSection:SymplecticFreeRB}Symplectic |
1087 |
> |
Lie-Poisson Integrator for Free Rigid Body} |
1088 |
|
|
1089 |
< |
\subsection{\label{introSection:symplecticDiscretizationRB}Symplectic Integration of Euler Equations} |
1090 |
< |
|
1091 |
< |
\[ |
1092 |
< |
\varphi _{\Delta t} = \varphi _{\Delta t/2,V} \circ \varphi |
1093 |
< |
_{\Delta t,T} \circ \varphi _{\Delta t/2,V} |
1094 |
< |
\] |
1089 |
> |
If there is not external forces exerted on the rigid body, the only |
1090 |
> |
contribution to the rotational is from the kinetic potential (the |
1091 |
> |
first term of \ref{ introEquation:bodyAngularMotion}). The free |
1092 |
> |
rigid body is an example of Lie-Poisson system with Hamiltonian |
1093 |
> |
function |
1094 |
> |
\begin{equation} |
1095 |
> |
T^r (\pi ) = T_1 ^r (\pi _1 ) + T_2^r (\pi _2 ) + T_3^r (\pi _3 ) |
1096 |
> |
\label{introEquation:rotationalKineticRB} |
1097 |
> |
\end{equation} |
1098 |
> |
where $T_i^r (\pi _i ) = \frac{{\pi _i ^2 }}{{2I_i }}$ and |
1099 |
> |
Lie-Poisson structure matrix, |
1100 |
> |
\begin{equation} |
1101 |
> |
J(\pi ) = \left( {\begin{array}{*{20}c} |
1102 |
> |
0 & {\pi _3 } & { - \pi _2 } \\ |
1103 |
> |
{ - \pi _3 } & 0 & {\pi _1 } \\ |
1104 |
> |
{\pi _2 } & { - \pi _1 } & 0 \\ |
1105 |
> |
\end{array}} \right) |
1106 |
> |
\end{equation} |
1107 |
> |
Thus, the dynamics of free rigid body is governed by |
1108 |
> |
\begin{equation} |
1109 |
> |
\frac{d}{{dt}}\pi = J(\pi )\nabla _\pi T^r (\pi ) |
1110 |
> |
\end{equation} |
1111 |
|
|
1112 |
+ |
One may notice that each $T_i^r$ in Equation |
1113 |
+ |
\ref{introEquation:rotationalKineticRB} can be solved exactly. For |
1114 |
+ |
instance, the equations of motion due to $T_1^r$ are given by |
1115 |
+ |
\begin{equation} |
1116 |
+ |
\frac{d}{{dt}}\pi = R_1 \pi ,\frac{d}{{dt}}Q = QR_1 |
1117 |
+ |
\label{introEqaution:RBMotionSingleTerm} |
1118 |
+ |
\end{equation} |
1119 |
+ |
where |
1120 |
+ |
\[ R_1 = \left( {\begin{array}{*{20}c} |
1121 |
+ |
0 & 0 & 0 \\ |
1122 |
+ |
0 & 0 & {\pi _1 } \\ |
1123 |
+ |
0 & { - \pi _1 } & 0 \\ |
1124 |
+ |
\end{array}} \right). |
1125 |
+ |
\] |
1126 |
+ |
The solutions of Equation \ref{introEqaution:RBMotionSingleTerm} is |
1127 |
|
\[ |
1128 |
< |
\varphi _{\Delta t,T} = \varphi _{\Delta t,R} \circ \varphi |
1129 |
< |
_{\Delta t,\pi } |
1128 |
> |
\pi (\Delta t) = e^{\Delta tR_1 } \pi (0),Q(\Delta t) = |
1129 |
> |
Q(0)e^{\Delta tR_1 } |
1130 |
|
\] |
1131 |
< |
|
1131 |
> |
with |
1132 |
|
\[ |
1133 |
< |
\varphi _{\Delta t,\pi } = \varphi _{\Delta t/2,\pi _1 } \circ |
1134 |
< |
\varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t,\pi _3 } |
1135 |
< |
\circ \varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t/2,\pi |
1136 |
< |
_1 } |
1133 |
> |
e^{\Delta tR_1 } = \left( {\begin{array}{*{20}c} |
1134 |
> |
0 & 0 & 0 \\ |
1135 |
> |
0 & {\cos \theta _1 } & {\sin \theta _1 } \\ |
1136 |
> |
0 & { - \sin \theta _1 } & {\cos \theta _1 } \\ |
1137 |
> |
\end{array}} \right),\theta _1 = \frac{{\pi _1 }}{{I_1 }}\Delta t. |
1138 |
|
\] |
1139 |
< |
|
1139 |
> |
To reduce the cost of computing expensive functions in e^{\Delta |
1140 |
> |
tR_1 }, we can use Cayley transformation, |
1141 |
|
\[ |
1142 |
< |
\varphi _{\Delta t/2,V} = \varphi _{\Delta t/2,F} \circ \varphi |
1143 |
< |
_{\Delta t/2,\tau } |
1142 |
> |
e^{\Delta tR_1 } \approx (1 - \Delta tR_1 )^{ - 1} (1 + \Delta tR_1 |
1143 |
> |
) |
1144 |
> |
\] |
1145 |
> |
|
1146 |
> |
The flow maps for $T_2^r$ and $T_2^r$ can be found in the same |
1147 |
> |
manner. |
1148 |
> |
|
1149 |
> |
In order to construct a second-order symplectic method, we split the |
1150 |
> |
angular kinetic Hamiltonian function can into five terms |
1151 |
> |
\[ |
1152 |
> |
T^r (\pi ) = \frac{1}{2}T_1 ^r (\pi _1 ) + \frac{1}{2}T_2^r (\pi _2 |
1153 |
> |
) + T_3^r (\pi _3 ) + \frac{1}{2}T_2^r (\pi _2 ) + \frac{1}{2}T_1 ^r |
1154 |
> |
(\pi _1 ) |
1155 |
> |
\]. |
1156 |
> |
Concatenating flows corresponding to these five terms, we can obtain |
1157 |
> |
an symplectic integrator, |
1158 |
> |
\[ |
1159 |
> |
\varphi _{\Delta t,T^r } = \varphi _{\Delta t/2,\pi _1 } \circ |
1160 |
> |
\varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t,\pi _3 } |
1161 |
> |
\circ \varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t/2,\pi |
1162 |
> |
_1 }. |
1163 |
|
\] |
1164 |
|
|
1165 |
+ |
The non-canonical Lie-Poisson bracket ${F, G}$ of two function |
1166 |
+ |
$F(\pi )$ and $G(\pi )$ is defined by |
1167 |
+ |
\[ |
1168 |
+ |
\{ F,G\} (\pi ) = [\nabla _\pi F(\pi )]^T J(\pi )\nabla _\pi G(\pi |
1169 |
+ |
) |
1170 |
+ |
\] |
1171 |
+ |
If the Poisson bracket of a function $F$ with an arbitrary smooth |
1172 |
+ |
function $G$ is zero, $F$ is a \emph{Casimir}, which is the |
1173 |
+ |
conserved quantity in Poisson system. We can easily verify that the |
1174 |
+ |
norm of the angular momentum, $\parallel \pi |
1175 |
+ |
\parallel$, is a \emph{Casimir}. Let$ F(\pi ) = S(\frac{{\parallel |
1176 |
+ |
\pi \parallel ^2 }}{2})$ for an arbitrary function $ S:R \to R$ , |
1177 |
+ |
then by the chain rule |
1178 |
+ |
\[ |
1179 |
+ |
\nabla _\pi F(\pi ) = S'(\frac{{\parallel \pi \parallel ^2 |
1180 |
+ |
}}{2})\pi |
1181 |
+ |
\] |
1182 |
+ |
Thus $ [\nabla _\pi F(\pi )]^T J(\pi ) = - S'(\frac{{\parallel \pi |
1183 |
+ |
\parallel ^2 }}{2})\pi \times \pi = 0 $. This explicit |
1184 |
+ |
Lie-Poisson integrator is found to be extremely efficient and stable |
1185 |
+ |
which can be explained by the fact the small angle approximation is |
1186 |
+ |
used and the norm of the angular momentum is conserved. |
1187 |
|
|
1188 |
< |
\section{\label{introSection:langevinDynamics}Langevin Dynamics} |
1188 |
> |
\subsection{\label{introSection:RBHamiltonianSplitting} Hamiltonian |
1189 |
> |
Splitting for Rigid Body} |
1190 |
|
|
1191 |
< |
\subsection{\label{introSection:LDIntroduction}Introduction and application of Langevin Dynamics} |
1191 |
> |
The Hamiltonian of rigid body can be separated in terms of kinetic |
1192 |
> |
energy and potential energy, |
1193 |
> |
\[ |
1194 |
> |
H = T(p,\pi ) + V(q,Q) |
1195 |
> |
\] |
1196 |
> |
The equations of motion corresponding to potential energy and |
1197 |
> |
kinetic energy are listed in the below table, |
1198 |
> |
\begin{center} |
1199 |
> |
\begin{tabular}{|l|l|} |
1200 |
> |
\hline |
1201 |
> |
% after \\: \hline or \cline{col1-col2} \cline{col3-col4} ... |
1202 |
> |
Potential & Kinetic \\ |
1203 |
> |
$\frac{{dq}}{{dt}} = \frac{p}{m}$ & $\frac{d}{{dt}}q = p$ \\ |
1204 |
> |
$\frac{d}{{dt}}p = - \frac{{\partial V}}{{\partial q}}$ & $ \frac{d}{{dt}}p = 0$ \\ |
1205 |
> |
$\frac{d}{{dt}}Q = 0$ & $ \frac{d}{{dt}}Q = Qskew(I^{ - 1} j)$ \\ |
1206 |
> |
$ \frac{d}{{dt}}\pi = \sum\limits_i {\left( {Q^T F_i (r,Q)} \right) \times X_i }$ & $\frac{d}{{dt}}\pi = \pi \times I^{ - 1} \pi$\\ |
1207 |
> |
\hline |
1208 |
> |
\end{tabular} |
1209 |
> |
\end{center} |
1210 |
> |
A second-order symplectic method is now obtained by the composition |
1211 |
> |
of the flow maps, |
1212 |
> |
\[ |
1213 |
> |
\varphi _{\Delta t} = \varphi _{\Delta t/2,V} \circ \varphi |
1214 |
> |
_{\Delta t,T} \circ \varphi _{\Delta t/2,V}. |
1215 |
> |
\] |
1216 |
> |
Moreover, \varphi _{\Delta t/2,V} can be divided into two sub-flows |
1217 |
> |
which corresponding to force and torque respectively, |
1218 |
> |
\[ |
1219 |
> |
\varphi _{\Delta t/2,V} = \varphi _{\Delta t/2,F} \circ \varphi |
1220 |
> |
_{\Delta t/2,\tau }. |
1221 |
> |
\] |
1222 |
> |
Since the associated operators of $\varphi _{\Delta t/2,F} $ and |
1223 |
> |
$\circ \varphi _{\Delta t/2,\tau }$ are commuted, the composition |
1224 |
> |
order inside \varphi _{\Delta t/2,V} does not matter. |
1225 |
|
|
1226 |
+ |
Furthermore, kinetic potential can be separated to translational |
1227 |
+ |
kinetic term, $T^t (p)$, and rotational kinetic term, $T^r (\pi )$, |
1228 |
+ |
\begin{equation} |
1229 |
+ |
T(p,\pi ) =T^t (p) + T^r (\pi ). |
1230 |
+ |
\end{equation} |
1231 |
+ |
where $ T^t (p) = \frac{1}{2}p^T m^{ - 1} p $ and $T^r (\pi )$ is |
1232 |
+ |
defined by \ref{introEquation:rotationalKineticRB}. Therefore, the |
1233 |
+ |
corresponding flow maps are given by |
1234 |
+ |
\[ |
1235 |
+ |
\varphi _{\Delta t,T} = \varphi _{\Delta t,T^t } \circ \varphi |
1236 |
+ |
_{\Delta t,T^r }. |
1237 |
+ |
\] |
1238 |
+ |
Finally, we obtain the overall symplectic flow maps for free moving |
1239 |
+ |
rigid body |
1240 |
+ |
\begin{equation} |
1241 |
+ |
\begin{array}{c} |
1242 |
+ |
\varphi _{\Delta t} = \varphi _{\Delta t/2,F} \circ \varphi _{\Delta t/2,\tau } \\ |
1243 |
+ |
\circ \varphi _{\Delta t,T^t } \circ \varphi _{\Delta t/2,\pi _1 } \circ \varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t,\pi _3 } \circ \varphi _{\Delta t/2,\pi _2 } \circ \varphi _{\Delta t/2,\pi _1 } \\ |
1244 |
+ |
\circ \varphi _{\Delta t/2,\tau } \circ \varphi _{\Delta t/2,F} .\\ |
1245 |
+ |
\end{array} |
1246 |
+ |
\label{introEquation:overallRBFlowMaps} |
1247 |
+ |
\end{equation} |
1248 |
+ |
|
1249 |
+ |
\section{\label{introSection:langevinDynamics}Langevin Dynamics} |
1250 |
+ |
As an alternative to newtonian dynamics, Langevin dynamics, which |
1251 |
+ |
mimics a simple heat bath with stochastic and dissipative forces, |
1252 |
+ |
has been applied in a variety of studies. This section will review |
1253 |
+ |
the theory of Langevin dynamics simulation. A brief derivation of |
1254 |
+ |
generalized Langevin Dynamics will be given first. Follow that, we |
1255 |
+ |
will discuss the physical meaning of the terms appearing in the |
1256 |
+ |
equation as well as the calculation of friction tensor from |
1257 |
+ |
hydrodynamics theory. |
1258 |
+ |
|
1259 |
|
\subsection{\label{introSection:generalizedLangevinDynamics}Generalized Langevin Dynamics} |
1260 |
|
|
1261 |
|
\begin{equation} |
1448 |
|
\label{introEquation:secondFluctuationDissipation} |
1449 |
|
\end{equation} |
1450 |
|
|
1322 |
– |
\section{\label{introSection:hydroynamics}Hydrodynamics} |
1323 |
– |
|
1451 |
|
\subsection{\label{introSection:frictionTensor} Friction Tensor} |
1452 |
< |
\subsection{\label{introSection:analyticalApproach}Analytical |
1453 |
< |
Approach} |
1454 |
< |
|
1455 |
< |
\subsection{\label{introSection:approximationApproach}Approximation |
1456 |
< |
Approach} |
1452 |
> |
Theoretically, the friction kernel can be determined using velocity |
1453 |
> |
autocorrelation function. However, this approach become impractical |
1454 |
> |
when the system become more and more complicate. Instead, various |
1455 |
> |
approaches based on hydrodynamics have been developed to calculate |
1456 |
> |
the friction coefficients. The friction effect is isotropic in |
1457 |
> |
Equation, \zeta can be taken as a scalar. In general, friction |
1458 |
> |
tensor \Xi is a $6\times 6$ matrix given by |
1459 |
> |
\[ |
1460 |
> |
\Xi = \left( {\begin{array}{*{20}c} |
1461 |
> |
{\Xi _{}^{tt} } & {\Xi _{}^{rt} } \\ |
1462 |
> |
{\Xi _{}^{tr} } & {\Xi _{}^{rr} } \\ |
1463 |
> |
\end{array}} \right). |
1464 |
> |
\] |
1465 |
> |
Here, $ {\Xi^{tt} }$ and $ {\Xi^{rr} }$ are translational friction |
1466 |
> |
tensor and rotational friction tensor respectively, while ${\Xi^{tr} |
1467 |
> |
}$ is translation-rotation coupling tensor and $ {\Xi^{rt} }$ is |
1468 |
> |
rotation-translation coupling tensor. |
1469 |
|
|
1470 |
< |
\subsection{\label{introSection:centersRigidBody}Centers of Rigid |
1471 |
< |
Body} |
1470 |
> |
\[ |
1471 |
> |
\left( \begin{array}{l} |
1472 |
> |
F_t \\ |
1473 |
> |
\tau \\ |
1474 |
> |
\end{array} \right) = - \left( {\begin{array}{*{20}c} |
1475 |
> |
{\Xi ^{tt} } & {\Xi ^{rt} } \\ |
1476 |
> |
{\Xi ^{tr} } & {\Xi ^{rr} } \\ |
1477 |
> |
\end{array}} \right)\left( \begin{array}{l} |
1478 |
> |
v \\ |
1479 |
> |
w \\ |
1480 |
> |
\end{array} \right) |
1481 |
> |
\] |
1482 |
|
|
1483 |
< |
\section{\label{introSection:correlationFunctions}Correlation Functions} |
1483 |
> |
\subsubsection{\label{introSection:analyticalApproach}The Friction Tensor for Regular Shape} |
1484 |
> |
For a spherical particle, the translational and rotational friction |
1485 |
> |
constant can be calculated from Stoke's law, |
1486 |
> |
\[ |
1487 |
> |
\Xi ^{tt} = \left( {\begin{array}{*{20}c} |
1488 |
> |
{6\pi \eta R} & 0 & 0 \\ |
1489 |
> |
0 & {6\pi \eta R} & 0 \\ |
1490 |
> |
0 & 0 & {6\pi \eta R} \\ |
1491 |
> |
\end{array}} \right) |
1492 |
> |
\] |
1493 |
> |
and |
1494 |
> |
\[ |
1495 |
> |
\Xi ^{rr} = \left( {\begin{array}{*{20}c} |
1496 |
> |
{8\pi \eta R^3 } & 0 & 0 \\ |
1497 |
> |
0 & {8\pi \eta R^3 } & 0 \\ |
1498 |
> |
0 & 0 & {8\pi \eta R^3 } \\ |
1499 |
> |
\end{array}} \right) |
1500 |
> |
\] |
1501 |
> |
where $\eta$ is the viscosity of the solvent and $R$ is the |
1502 |
> |
hydrodynamics radius. |
1503 |
> |
|
1504 |
> |
Other non-spherical particles have more complex properties. |
1505 |
> |
|
1506 |
> |
\[ |
1507 |
> |
S = \frac{2}{{\sqrt {a^2 - b^2 } }}\ln \frac{{a + \sqrt {a^2 - b^2 |
1508 |
> |
} }}{b} |
1509 |
> |
\] |
1510 |
> |
|
1511 |
> |
|
1512 |
> |
\[ |
1513 |
> |
S = \frac{2}{{\sqrt {b^2 - a^2 } }}arctg\frac{{\sqrt {b^2 - a^2 } |
1514 |
> |
}}{a} |
1515 |
> |
\] |
1516 |
> |
|
1517 |
> |
\[ |
1518 |
> |
\begin{array}{l} |
1519 |
> |
\Xi _a^{tt} = 16\pi \eta \frac{{a^2 - b^2 }}{{(2a^2 - b^2 )S - 2a}} \\ |
1520 |
> |
\Xi _b^{tt} = \Xi _c^{tt} = 32\pi \eta \frac{{a^2 - b^2 }}{{(2a^2 - 3b^2 )S + 2a}} \\ |
1521 |
> |
\end{array} |
1522 |
> |
\] |
1523 |
> |
|
1524 |
> |
\[ |
1525 |
> |
\begin{array}{l} |
1526 |
> |
\Xi _a^{rr} = \frac{{32\pi }}{3}\eta \frac{{(a^2 - b^2 )b^2 }}{{2a - b^2 S}} \\ |
1527 |
> |
\Xi _b^{rr} = \Xi _c^{rr} = \frac{{32\pi }}{3}\eta \frac{{(a^4 - b^4 )}}{{(2a^2 - b^2 )S - 2a}} \\ |
1528 |
> |
\end{array} |
1529 |
> |
\] |
1530 |
> |
|
1531 |
> |
|
1532 |
> |
\subsubsection{\label{introSection:approximationApproach}The Friction Tensor for Arbitrary Shape} |
1533 |
> |
Unlike spherical and other regular shaped molecules, there is not |
1534 |
> |
analytical solution for friction tensor of any arbitrary shaped |
1535 |
> |
rigid molecules. The ellipsoid of revolution model and general |
1536 |
> |
triaxial ellipsoid model have been used to approximate the |
1537 |
> |
hydrodynamic properties of rigid bodies. However, since the mapping |
1538 |
> |
from all possible ellipsoidal space, $r$-space, to all possible |
1539 |
> |
combination of rotational diffusion coefficients, $D$-space is not |
1540 |
> |
unique\cite{Wegener79} as well as the intrinsic coupling between |
1541 |
> |
translational and rotational motion of rigid body\cite{}, general |
1542 |
> |
ellipsoid is not always suitable for modeling arbitrarily shaped |
1543 |
> |
rigid molecule. A number of studies have been devoted to determine |
1544 |
> |
the friction tensor for irregularly shaped rigid bodies using more |
1545 |
> |
advanced method\cite{} where the molecule of interest was modeled by |
1546 |
> |
combinations of spheres(beads)\cite{} and the hydrodynamics |
1547 |
> |
properties of the molecule can be calculated using the hydrodynamic |
1548 |
> |
interaction tensor. Let us consider a rigid assembly of $N$ beads |
1549 |
> |
immersed in a continuous medium. Due to hydrodynamics interaction, |
1550 |
> |
the ``net'' velocity of $i$th bead, $v'_i$ is different than its |
1551 |
> |
unperturbed velocity $v_i$, |
1552 |
> |
\[ |
1553 |
> |
v'_i = v_i - \sum\limits_{j \ne i} {T_{ij} F_j } |
1554 |
> |
\] |
1555 |
> |
where $F_i$ is the frictional force, and $T_{ij}$ is the |
1556 |
> |
hydrodynamic interaction tensor. The friction force of $i$th bead is |
1557 |
> |
proportional to its ``net'' velocity |
1558 |
> |
\begin{equation} |
1559 |
> |
F_i = \zeta _i v_i - \zeta _i \sum\limits_{j \ne i} {T_{ij} F_j }. |
1560 |
> |
\label{introEquation:tensorExpression} |
1561 |
> |
\end{equation} |
1562 |
> |
This equation is the basis for deriving the hydrodynamic tensor. In |
1563 |
> |
1930, Oseen and Burgers gave a simple solution to Equation |
1564 |
> |
\ref{introEquation:tensorExpression} |
1565 |
> |
\begin{equation} |
1566 |
> |
T_{ij} = \frac{1}{{8\pi \eta r_{ij} }}\left( {I + \frac{{R_{ij} |
1567 |
> |
R_{ij}^T }}{{R_{ij}^2 }}} \right). |
1568 |
> |
\label{introEquation:oseenTensor} |
1569 |
> |
\end{equation} |
1570 |
> |
Here $R_{ij}$ is the distance vector between bead $i$ and bead $j$. |
1571 |
> |
A second order expression for element of different size was |
1572 |
> |
introduced by Rotne and Prager\cite{} and improved by Garc\'{i}a de |
1573 |
> |
la Torre and Bloomfield, |
1574 |
> |
\begin{equation} |
1575 |
> |
T_{ij} = \frac{1}{{8\pi \eta R_{ij} }}\left[ {\left( {I + |
1576 |
> |
\frac{{R_{ij} R_{ij}^T }}{{R_{ij}^2 }}} \right) + R\frac{{\sigma |
1577 |
> |
_i^2 + \sigma _j^2 }}{{r_{ij}^2 }}\left( {\frac{I}{3} - |
1578 |
> |
\frac{{R_{ij} R_{ij}^T }}{{R_{ij}^2 }}} \right)} \right]. |
1579 |
> |
\label{introEquation:RPTensorNonOverlapped} |
1580 |
> |
\end{equation} |
1581 |
> |
Both of the Equation \ref{introEquation:oseenTensor} and Equation |
1582 |
> |
\ref{introEquation:RPTensorNonOverlapped} have an assumption $R_{ij} |
1583 |
> |
\ge \sigma _i + \sigma _j$. An alternative expression for |
1584 |
> |
overlapping beads with the same radius, $\sigma$, is given by |
1585 |
> |
\begin{equation} |
1586 |
> |
T_{ij} = \frac{1}{{6\pi \eta R_{ij} }}\left[ {\left( {1 - |
1587 |
> |
\frac{2}{{32}}\frac{{R_{ij} }}{\sigma }} \right)I + |
1588 |
> |
\frac{2}{{32}}\frac{{R_{ij} R_{ij}^T }}{{R_{ij} \sigma }}} \right] |
1589 |
> |
\label{introEquation:RPTensorOverlapped} |
1590 |
> |
\end{equation} |
1591 |
> |
|
1592 |
> |
%Bead Modeling |
1593 |
> |
|
1594 |
> |
\[ |
1595 |
> |
B = \left( {\begin{array}{*{20}c} |
1596 |
> |
{T_{11} } & \ldots & {T_{1N} } \\ |
1597 |
> |
\vdots & \ddots & \vdots \\ |
1598 |
> |
{T_{N1} } & \cdots & {T_{NN} } \\ |
1599 |
> |
\end{array}} \right) |
1600 |
> |
\] |
1601 |
> |
|
1602 |
> |
\[ |
1603 |
> |
C = B^{ - 1} = \left( {\begin{array}{*{20}c} |
1604 |
> |
{C_{11} } & \ldots & {C_{1N} } \\ |
1605 |
> |
\vdots & \ddots & \vdots \\ |
1606 |
> |
{C_{N1} } & \cdots & {C_{NN} } \\ |
1607 |
> |
\end{array}} \right) |
1608 |
> |
\] |
1609 |
> |
|
1610 |
> |
\begin{equation} |
1611 |
> |
\begin{array}{l} |
1612 |
> |
\Xi _{}^{tt} = \sum\limits_i {\sum\limits_j {C_{ij} } } , \\ |
1613 |
> |
\Xi _{}^{tr} = \Xi _{}^{rt} = \sum\limits_i {\sum\limits_j {U_i C_{ij} } } , \\ |
1614 |
> |
\Xi _{}^{rr} = - \sum\limits_i {\sum\limits_j {U_i C_{ij} } } U_j \\ |
1615 |
> |
\end{array} |
1616 |
> |
\end{equation} |
1617 |
> |
where |
1618 |
> |
\[ |
1619 |
> |
U_i = \left( {\begin{array}{*{20}c} |
1620 |
> |
0 & { - z_i } & {y_i } \\ |
1621 |
> |
{z_i } & 0 & { - x_i } \\ |
1622 |
> |
{ - y_i } & {x_i } & 0 \\ |
1623 |
> |
\end{array}} \right) |
1624 |
> |
\] |
1625 |
> |
|
1626 |
> |
\[ |
1627 |
> |
r_{OR} = \left( \begin{array}{l} |
1628 |
> |
x_{OR} \\ |
1629 |
> |
y_{OR} \\ |
1630 |
> |
z_{OR} \\ |
1631 |
> |
\end{array} \right) = \left( {\begin{array}{*{20}c} |
1632 |
> |
{\Xi _{yy}^{rr} + \Xi _{zz}^{rr} } & { - \Xi _{xy}^{rr} } & { - \Xi _{xz}^{rr} } \\ |
1633 |
> |
{ - \Xi _{yx}^{rr} } & {\Xi _{zz}^{rr} + \Xi _{xx}^{rr} } & { - \Xi _{yz}^{rr} } \\ |
1634 |
> |
{ - \Xi _{zx}^{rr} } & { - \Xi _{yz}^{rr} } & {\Xi _{xx}^{rr} + \Xi _{yy}^{rr} } \\ |
1635 |
> |
\end{array}} \right)^{ - 1} \left( \begin{array}{l} |
1636 |
> |
\Xi _{yz}^{tr} - \Xi _{zy}^{tr} \\ |
1637 |
> |
\Xi _{zx}^{tr} - \Xi _{xz}^{tr} \\ |
1638 |
> |
\Xi _{xy}^{tr} - \Xi _{yx}^{tr} \\ |
1639 |
> |
\end{array} \right) |
1640 |
> |
\] |
1641 |
> |
|
1642 |
> |
\[ |
1643 |
> |
U_{OR} = \left( {\begin{array}{*{20}c} |
1644 |
> |
0 & { - z_{OR} } & {y_{OR} } \\ |
1645 |
> |
{z_i } & 0 & { - x_{OR} } \\ |
1646 |
> |
{ - y_{OR} } & {x_{OR} } & 0 \\ |
1647 |
> |
\end{array}} \right) |
1648 |
> |
\] |
1649 |
> |
|
1650 |
> |
\[ |
1651 |
> |
\begin{array}{l} |
1652 |
> |
\Xi _R^{tt} = \Xi _{}^{tt} \\ |
1653 |
> |
\Xi _R^{tr} = \Xi _R^{rt} = \Xi _{}^{tr} - U_{OR} \Xi _{}^{tt} \\ |
1654 |
> |
\Xi _R^{rr} = \Xi _{}^{rr} - U_{OR} \Xi _{}^{tt} U_{OR} + \Xi _{}^{tr} U_{OR} - U_{OR} \Xi _{}^{tr} ^{^T } \\ |
1655 |
> |
\end{array} |
1656 |
> |
\] |
1657 |
> |
|
1658 |
> |
\[ |
1659 |
> |
D_R = \left( {\begin{array}{*{20}c} |
1660 |
> |
{D_R^{tt} } & {D_R^{rt} } \\ |
1661 |
> |
{D_R^{tr} } & {D_R^{rr} } \\ |
1662 |
> |
\end{array}} \right) = k_b T\left( {\begin{array}{*{20}c} |
1663 |
> |
{\Xi _R^{tt} } & {\Xi _R^{rt} } \\ |
1664 |
> |
{\Xi _R^{tr} } & {\Xi _R^{rr} } \\ |
1665 |
> |
\end{array}} \right)^{ - 1} |
1666 |
> |
\] |
1667 |
> |
|
1668 |
> |
|
1669 |
> |
%Approximation Methods |
1670 |
> |
|
1671 |
> |
%\section{\label{introSection:correlationFunctions}Correlation Functions} |