Earl Thomas Conley was a country music singer-songwriter who during the 1980s and 1990s had 24 Top-10 country singles including 18 that were Number One. Only Alabama and Ronnie Milsap had more number one hits during the decade.
This month, at age 77, Conley died after spending many months in hospice care for cerebral atrophy, a condition that had caused progressive loss of memory over several years. Popular performing musicians are prone to this condition because they are usually sleep deprived -- they perform at night, and while on tours they sleep in a bus during the day. They are also exposed to a lot of smoke as well as to people who use drugs and alcohol. Cerebral atrophy is associated with anything that can damage the brain such as head trauma, infectious diseases, strokes, diabetes or arteriosclerosis, but I could find no media evidence that he had any of these conditions.
Conley was born in 1941, the third of eight children, in the small country town of Portsmouth, Ohio. When he was 14, his father lost his job with the railroad, so he moved to live with one of his older sisters in Jamestown, Ohio. After high school, he was offered a scholarship to attend art school but instead joined the Army, where he began to write songs and sing in a religious revival group. At age 27, he left the army and worked on the railroad and in steel mills and commuted to Nashville to try to further his music career.
At age 34, he had his first big breakthrough when the song "Smokey Mountain Memories" that he wrote for another musician made the top 40 country hit list. At age 35, he wrote "This Time I've Hurt Her More Than She Loves Me" and Conway Twitty made it the number one country hit. At age 40 he had his own first number one hit, "Fire & Smoke." In 1983, at age 43, he was nominated for multiple Grammy Awards for his song, "Holding Her and Loving You".
In 1992 at age 52, because his records were not selling, he was dropped from his record label and did not record again for seven years. In interviews he told reporters that he had respiratory allergies. At age 57, he recorded a few songs and at age 61, he had a top 20 recording, "All Over Me". His last years were clouded by progressive dementia that eventually led to hospice care for several months before he died at age 77. The cause of death was given as cerebral atrophy.
Most obituaries for people who have died from cerebral atrophy list "natural causes," but the most common cause of death is heart failure, which is never "natural." Cerebral atrophy means that a person progressively loses brain cells and the brain looks progressively smaller on an MRI. First they have difficulty remembering recent events, then names and places, then recognizing people and eventually they don't even know their relatives or friends, or where they are.
With progressive loss of the ability to remember anything, you eventually spend most of your time in bed. Not using your muscles regularly progressively weakens you. Your heart is a muscle and when you lie in bed all the time, your heart weakens and eventually your heart becomes too weak to pump blood through your body and you die of heart failure.
Since both dementia and heart attacks are associated with inflammation (an overactive immune system), every person with failing memory should immediately begin an anti-inflammatory lifestyle.
If you are not already eating a healthful plant-based diet and engaging in regular exercise, check with your doctor and then try to start a new diet and exercise program as soon as possible.


Browse listings of Member singles here at Meet a Trucker that are tagged with German. Dating others that have similar interests is a pefect way to find things to do on a first date. Register for a Totally Free Account to Find your perfect match!
I'm tall and not at all small. Currently I drive OTR but starting to look for a regional or local job. Outside of the truck music is my life. I love live music of all kinds but prefer small clubs that feature newer bands that write their own music.
In a relationship. Just want to text.


John McCain just trotted out his usual line about corporations in America facing the second highest tax rate in the world.
It's a very misleading claim: Most corporations pay far less than the stated rates, because of loopholes.
For the full explanation, see this Nobel Prize-winning economist.


text:
\section{ Introduction}
A great deal of attention has been devoted to non-contact friction between
nanostructures, including, for example, the frictional drag force between
two-dimensional quantum wells \cite{Gramila1,Gramila2,Sivan} , and the
friction force between an atomic force microscope tip and a substrate \cite
{Dorofeev,Gostmann,Stipe,Mamin,Hoffmann}.

In non-contact friction the bodies are separated by a potential barrier
thick enough to prevent electrons or other particles with a finite rest mass
from tunneling across it, but allowing interaction via the long-range
electromagnetic field, which is always present in the gap between bodies.
The presence of inhomogeneous tip-sample electric fields is difficult to
avoid, even under the best experimental conditions \cite{Stipe}. For
example, even if both the tip and the sample were metallic single crystals,
the tip would still have corners present and more than one crystallographic
plane exposed. The presence of atomic steps, adsorbates, and other defects
will also contribute to the inhomogeneous electric field. The electric field
can be easily changed by applying a voltage between the tip and the
sample.

The electromagnetic field can also be created by the fluctuating current density,
 due to
thermal and quantum fluctuations inside the solids. This fluctuating
electromagnetic field is always present close to the surface of any body,
and consist partly of traveling waves and partly of evanescent waves which
decay exponentially with the distance away from the surface of the body. The
fluctuating electromagnetic field originating from the fluctuating current
density inside the bodies gives
rise to the well-known long-range attractive van der Waals interaction
between two bodies \cite{Lifshitz}. If the bodies are in relative motion, the
same fluctuating electromagnetic field will give rise to a friction which is
frequently named as the van der Waals friction.
 Van der Waals friction can be
considered as mediated by photon exchange between the bodies: One body emit
a photon, and the other absorbs it, thus transferring momentum between the
bodies, resulting in a friction force. At large distances between the
bodies, the main contribution to friction comes from photon exchange,
corresponding to the propagating electromagnetic waves. However this
contribution is very small because the photons corresponding to propagating
waves carry very small momentum, no larger than  $ k_BT/c\hbar $. The photons,
corresponding to the evanescent electromagnetic waves, carry the momentum $%
q\sim d^{-1}$. Thus for distances $d$ between two bodies smaller
characteristic distance $d_T=\hbar c/k_BT$, which depends on temperature (at
room temperature $d_T\sim 10^5$\AA ), the main contribution to friction
comes from the evanescent electromagnetic field. In analogy with electron
tunneling, this mechanism of momentum transfer can be considered as
associated with the photon tunneling.

Although the dissipation of energy connected with the non-contact friction
always is of electromagnetic  origin, the detailed mechanism is not
totally clear, since there are several different mechanisms of energy
dissipation connected with the electromagnetic interaction between bodies.
First, the electromagnetic field from one body will penetrate into the other
body, and induce an electric current. In this case friction is due to Ohmic
losses inside the bodies. The fluctuating electromagnetic
 field can also excite the vibrations of the adsorbates or other
surface localized modes, e.g. surface plasmons and polaritons.
In this case friction is due to energy relaxation of the surface modes.
 Another contribution to friction from the
electromagnetic field is associated with the time-dependent stress acting
on the surface of the bodies. This stress can excite acoustic waves, or
induce time-dependent deformations which may result in a temperature
gradient. It can also induce motion of defects either in the bulk, or on the
surface of the bodies. The contribution to friction due to non-adiabatic heat
flow, or motion of defects, is usually denoted as internal friction.

It is very worthwhile to get a better understanding of different mechanisms
of non-contact friction because of it
practical importance for
ultrasensitive force detection experiments. This is because the ability to
detect small forces is inextricably linked to friction via the
fluctuation-dissipation theorem. For example, the detection of single spins
by magnetic resonance force microscopy, which has been proposed for
three-dimensional atomic imaging \cite{Sidles} and quantum computation \cite
{Berman}, will require force fluctuations to be reduced to unprecedented
levels. In addition, the search for quantum gravitation effects at short
length scale \cite{Arkani} and future measurements of the dynamical Casimir
forces \cite{Mohideen} may eventually be limited by non-contact friction
effects.

Recently Gotsmann and
Fuchs  \cite{Gostmann} observed long-range non-contact friction between an aluminum
tip and
a gold (111) surface. The friction force $F$ acting on the tip is
proportional to the velocity $v$, $F=\Gamma v$. For motion of the tip
normal to the surface
the  friction coefficient $\Gamma (d)=b\cdot d^{-3}$,
where $d$ is the tip-sample spacing and $b=(8.0_{-4.5}^{+5.5})\times
10^{-35}\mathrm{N\,s\,m}^2$  \cite{Gostmann}. Later Stipe \textit{et.al.}\cite{Stipe}
observed non-contact friction effect between a gold surface and a gold-coated
cantilever as a function of tip-sample spacing $d$, the temperature $T$, and the
bias voltage $V$. For vibration of the tip parallel to the surface they
found $\Gamma (d)=\alpha (T)(V^2+V_0^2)/d^n$, where $n=1.3\pm 0.2,$ and $%
V_0\sim 0.2\,\mathrm{V.}$ At 295\textrm{K, }for the spacing $d=$ 100\textrm{%
\AA\ }they found $\Gamma =1.5\times 10^{-13}\mathrm{\,kgs}^{-1},$ which is $%
\sim $500 times smaller that reported in Ref. \cite{Gostmann} at the same
distance using a parallel cantilever configuration.

In a recent Letter, Dorofeev \textit{et.al.} \cite{Dorofeev} claim that a
the non-contact friction effect observed in \cite{Dorofeev,Gostmann} is due to
Ohmic losses mediated by the fluctuating electromagnetic field . This result
is controversial, however, since the van der Waals friction has
been shown \cite{Volokitin1,Persson and Volokitin,Volokitin2,Volokitin3} to
be many orders of magnitude smaller than the friction  observed by Dorofeev \textit{%
et.al.} Presently, the origin of the difference in magnitude and distance
dependence of the long-range non-contact friction effect observed in \cite
{Gostmann} and \cite{Stipe} is not well understood.

In order to improve the basic understanding of  non-contact friction,
 we present new results for van der Waals friction.
In \cite{Volokitin1} we developed a theory of van der Waals friction
for surfaces in parallel relative motion.
Here we generalize the theory to include also the case when the
surfaces are in
normal relative motion, and we show that there is drastic difference between
these two cases. Thus,  for normal relative motion of clean good conductor surfaces,
the friction is many orders of magnitude larger than for parallel relative motion,
but  still  smaller than observed  experimentally.
Another enhancement mechanism of the non-contact friction can be connected
with resonant photon tunneling between  states localized on the different
surfaces. Recently it was discovered that resonant photon tunneling between
surface plasmon modes give rise to extraordinary enhancement of the optical
transmission through sub-wavelength hole arrays \cite{Ebbesen}. The same
surface modes enhancement  can be expected  for van der Waals friction if the
frequency of these modes is sufficiently low to be excited by thermal radiation.
At room temperature only the modes with frequencies below
$\sim 10^{13}s^{-1}$ can be excited.
For normal metals surface plasmons have much too high frequencies; at
thermal frequencies
the dielectric function of normal metals becomes nearly
purely imaginary, which exclude surface plasmon enhancement of the van der Waals
friction for good conductors. However surface plasmons
for semiconductors are characterized by much
smaller frequencies and damping constants, and they can give an important contribution
to van der Waals friction.
Other  surface modes which can be excited
by thermal radiation are
adsorbate vibrational modes. Especially for parallel vibrations these modes
may have very low frequencies.

All information about the long-range electromagnetic interaction between two
non-contacting bodies is, in principle, contained in the reflection factors
of the electromagnetic field. At present time very little is known about the
reflection factors for large wave vectors and for extremely small
frequencies. In the calculations of the reflection factors one must
take into account the non-local response of the electron gas on the external
electromagnetic field. There are two correlation length which determine this
nonlocal response. First is the skin depth, which determines the long-range
length scale
of  the nonlocality in the volume, and the second is the screening length.
 The latter length scale determines the short range  correlation length for non-local
response in the surface region.
In our previous calculations of the Van der Waals friction \cite
{Volokitin1,Persson and Volokitin,Volokitin2,Volokitin3} we mostly
considered good conductors. In this case it was shown that the important
contribution comes from the non-local optic effects in the surface region.
However it was shown that the Van der Waals friction becomes much larger for
high resistivity material, for which the volume contribution from non-local
effects is also important. It is easy to see that within local optic
approximation the Van der Waals friction diverge when the conductivity of
materials tend to zero. This means that the local optic approximation breaks
down for high-resistivity materials. This situation is completely different
from the heat transfer between bodies via photon tunneling \cite
{Pendry,Volokitin2}, where the heat flux is maximal at conductivities
corresponding to semi-metals. In order to clarify the situation we study the
dependence of the van der Waals friction on the dielectric properties of the
materials within the non-local dielectric approach, which was proposed some
years ago for the investigation of the anomalous skin effects \cite{Fuchs
and Kliever}.

\section{Calculation of the fluctuating electromagnetic field}

 We consider two semi-infinite metals
\textbf{1} and \textbf{2} having parallel flat surfaces. We introduce a
coordinate system with $xy$ plane in the surface of body \textbf{1} ,
 and the $z
$ axis along the upward normal. The surface of body \textbf{2} is located at
$z=d$, performing small amplitude vibrations along the $z$ axes with
displacement coordinate $u_z(t)=u_0e^{-i\omega _0t}.$ Since the system is
 translation invariant in the $\mathbf{x}=(x,y)$ plane, the electromagnetic
field can be represented by the Fourier integral
\begin{eqnarray}
\mathbf{E}(\mathbf{x},z)=\int \frac{d^2q}{(2\pi)^2}e^{i\mathbf{q} \cdot \mathbf{x}}
\mathbf{E}(\mathbf{q},z),   \\
\mathbf{B}(\mathbf{x},z)=\int \frac{d^2q}{(2\pi)^2}e^{i\mathbf{q} \cdot \mathbf{x}}
\mathbf{B}(\mathbf{q},z),
\end{eqnarray}
where $\mathbf{E}$ and $\mathbf{B}$ are the electric and magnetic induction field,
and $\mathbf{q}$ is the two-dimensional wave vector in $(x,y)$ plane. After the
Fourier transformation it is convenient to choose the coordinate axis in the
(x,y) plane along the vectors $\mathbf{q}$ and $\mathbf{n}=[\hat{z}\times \mathbf{q}
]$. In the vacuum
gap between the bodies  the electric field $\mathbf{E}(\mathbf{q},\omega,z)$,
 and the
magnetic induction field $\mathbf{B}(\mathbf{q},\omega,z)$, can, to the linear order
in the vibrational coordinate, be written in the form
\begin{equation}
\mathbf{E}(\mathbf{q},\omega ,z)=\left( \left( \mathbf{w}_{0}e^{ipz}
+ \mathbf{v}_{0}e^{-ipz}\right)+\left(\mathbf{w}_{1}e^{ip^{+}z}+\mathbf{v}_{1}e^{-ip^{+}z}
\right)e^{-i\omega_0 t}
\right)
e^{-i\omega t}  \label{one}
\end{equation}
\begin{eqnarray}
\mathbf{B}(\mathbf{q},\omega ,z)=c\left[\frac 1{\omega} \left([\mathbf{k}^{-}\times
\mathbf{v}_{0}]e^{-ipz}+ [ \mathbf{k}^{+}\times\mathbf{w}_{0}]e^{ipz}\right)
 \right.  \nonumber   \\
\left. +\frac{1}{\omega +\omega _0}\left(
[ \mathbf{k}^{-}_+\times\mathbf{v}_{1}]e^{-ip^+z}+ [\mathbf{k}^{+}_+
\times\mathbf{w}_{1}e^{ip^+z}]\right)e^{-i\omega _0t}
\right] e^{-i\omega t}  \label{two}
\end{eqnarray}
where $\mathbf{k}^{\pm}=\mathbf{q}\pm \hat{z}p,\,
p=((\omega/c)^2-q^2)^{1/2},\,p^+=p(\omega+\omega_0),\,\mathbf{k}^{+}_{+}
=\mathbf{k}^{+}(\omega+\omega_0),\,\mathbf{k}^{-}_{+}
=\mathbf{k}^{-}(\omega+\omega_0).$ At the surfaces of the bodies the amplitude
of the outgoing electromagnetic wave must be equal to the amplitude of the reflected
wave plus the amplitude of the radiated wave. It is convenient to decompose the
electromagnetic field into the $p$- and $s$ - polarized electromagnetic waves.
For $p$-polarized electromagnetic waves the electric field is in the incident
plane determined by the vectors $\mathbf{q}$ and $\mathbf{n}$, and for $s$-
polarized electromagnetic waves the electric field is normal to the incident
 Thus the boundary conditions
for the electromagnetic
field at $z=0$
can be written in the form
\begin{equation}
w_{0z(y)}=R_{1p(s)}(\omega )v_{0z(y)}+E^{f}_{1z(y)}(\omega )
\label{three}
\end{equation}
\begin{equation}
w_{1z(y)}=R_{1p(s)}(\omega +\omega _0)v_{1z(y)}  \label{four}
\end{equation}
where $R_{1p(s)}(\omega )$ is the reflection factor for surface \textbf{1}
 for $p(s)$ - polarized electromagnetic field, and where $%
E^{f}_{1z(y)}(\omega )$ are the components of the
 fluctuating electric field outside the surface \textbf{1} in the
absence of the body \textbf{2}. The boundary condition at the surface of
the body \textbf{2} must be written in the reference frame where the body \textbf{2}
is at rest. The electric field in this reference frame is determined by a Lorentz
transformation. Performing a Lorentz transformation of the electric field to linear order in
$\omega _0$ gives
\begin{equation}
\mathbf{E}^{\prime }=\mathbf{E}-\frac{i\omega _0u(t)\left[ \mathbf{\hat e}%
_z\times \mathbf{B}\right] }c  \label{five}
\end{equation}
For the $p$-polarized electromagnetic waves the second term in (\ref{five})
is of the order of magnitude $\omega_0 u_0 \omega/pc^2$ relative to the first one and
can be neglected for the most practical cases. However, for the $s$-polarized
electromagnetic
waves the second term is of the order of magnitude $\omega_0 u_0p/\omega$ and can be
of the same order of magnitude as the first term. In the rest frame of body \textbf{2}
there is also mixture of $s$- and $p-$ polarized electromagnetic waves. In \cite
{Volokitin1} it was was shown that this  gives contribution of the
order $(\omega_0u_0/c)^2$
and thus can be neglected. After performing Lorentz transformation to linear order in
$\omega_0$ and $u_0$ we get
$ \mathbf{v}_{0}^{\prime}=
\mathbf{v}_{0},\,\mathbf{w}_{0}^{\prime}=\mathbf{w}_{0}$
\[
v_{1z(x)}^{\prime}=v_{1z(x)}-ipu_0v_{0z(x)};\,\,
w_{1z(x)}^{\prime}=w_{1z(x)}+ipu_0w_{0z(x)};
\]
\[
w_{1y}^{\prime}=w_{1y}+\frac{\omega +\omega_0}{\omega}ipu_0w_{0y};\,\,
v_{1y}^{\prime}=v_{1y}-\frac{\omega +\omega_0}{\omega}ipu_0v_{0y}
\]
The boundary conditions for the electromagnetic field at  $z=d+u(t)$ in the rest
frame of body \textbf{2}
can be written in the form
\begin{equation}
v_{0z(y)}=e^{2ipd}R_{2p(s)}(\omega )w_{0z(y)}+e^{ipd}E^{f}_{2z(y)}(\omega )
\label{six}
\end{equation}
\begin{equation}
v_{1z}-ipu_0v_{0z}=e^{2ip^{+}d}R_{2p}^{+}(w_{1z}+ipu_0w_{0z})
\label{seven}
\end{equation}
\begin{equation}
v_{1y}-ipu_0\frac{(\omega +\omega _0)v_{0y}}\omega =e^{2ipd}R_{2s}^{+}
\left(w_{1y}+ipu_0\frac{(\omega +\omega _0)w_{0y}}\omega\right)
\label{eight}
\end{equation}
where $R_{2p(s)}(\omega )$ is the reflection factor for surface \textbf{2}
  for $p(s)$ - polarized electromagnetic field, and where $
E_{2z(y)}^f(\omega )$ are the components of the
 fluctuating electric field outside the surface \textbf{1} in the
absence of the body \textbf{1}.
From (\ref{three},\ref{four}) and (\ref{six}-\ref{eight}) we get
\begin{equation}
w_{0z(y)}=\frac{R_{1p(s)}E^{f}_{2z(y)}e^{ipd}+E^{f}_{1z(y)}}{\Delta}  \label{nine}
\end{equation}
\begin{equation}
v_{0z(y)}=\frac{e^{2ipd}R_{2p(s)}E^{f}_{1z(y)}+E^{f}_{2z(y)}e^{ipd}}{\Delta}
\label{ten}
\end{equation}
\begin{equation}
v_{1z}=ipu_0 \frac{(e^{2ipd}R^{f}_{2p}+e^{2ip^{+}d}R_{2p}^{+})E^{f}_{1z}+
(1+e^{2ip^{+}d}R_{2p}^{+}
R_1)E^{f}_{2z}e^{ipd}}
{\Delta_p \Delta_p^{+}}  \label{eleven}
\end{equation}
\begin{equation}
v_{1y}=ipu_0\frac{\omega + \omega_0}{\omega}
 \frac{(e^{2ipd}R_{2s}+e^{2ip^{+}d}R_{2s}^{+})E_{1y}^f+
(1+e^{2ip^{+}d}R_{2s}^{+}R_{1s})E_{2y}^fe^{ipd}}
{\Delta_s \Delta_s^{+}}  \label{twelve}
\end{equation}
\begin{equation}
w_{1z(y)}=R_{1p(s)}^{+}v_{1z(y)}  \label{thirteen}
\end{equation}
where $R_{p(s}^{+}=R_{p(s)}(\omega +\omega_0),\, \Delta_{p(s)}=1-e^{2ipd}R_{2p(s)}
R_{1p(s)},$ and $
\Delta_{p(s)}^{+}=\Delta_{p(s)}(\omega +\omega_0)$. Other components of the
fluctuating electromagnetic field can be found from the transversality conditions
\begin{equation}
qw_x+pw_z=0,\,\, qv_x-pv_z=0
\end{equation}
The fundamental characteristic
of the fluctuating electromagnetic field is the correlation function, determining
the average product of components $\mathbf{E}^{f}(\mathbf{q},\omega)$.
Accordingly to the
general theory of the fluctuating electromagnetic field
(see for a example \cite{Volokitin2}) these correlation
function are given by
\begin{equation}
<|E^{f}_{y}(\mathbf{q},\omega)|^2>=\frac{\hbar \omega^2}
{2c^2|p|^2} \left(n(\omega)+\frac{1}{2}\right)
[(p+p^*)(1-|R_s|^2)+(p-p^*)(R_s^*-R_s)]  \label{corfs}
\end{equation}
\begin{equation}
<|E^{f}_{z}(\mathbf{q},\omega)|^2>=\frac{\hbar q^2}
{2|p|^2} \left(n(\omega)+\frac{1}{2}\right)
[(p+p^*)(1-|R_p|^2)+(p-p^*)(R_p^*-R_p)]
\label{corfp}
\end{equation}
where $<...>$ denote statistical average over the random field,
and  where the Bose-Einstein factor
\[
n(\omega )=\frac 1{e^{\hbar \omega /k_BT}-1}
\]

We note that $p$ is real for $q<\omega/c$ (propagating waves), and  purely
imaginary for  $q>\omega/c$ (evanescent waves).
Thus for $q<\omega/c$
and $q>\omega/c$ the
correlation functions are determined by the first and the second
terms in Eqs. (\ref{corfs})and (\ref{corfp}), respectively.

\section{Calculation of the friction force between two semi-infinite bodies in normal
relative motion}

The frictional stress $\sigma$ which act on the surfaces of the two bodies
can be obtained from $zz-$ component of the Maxwell stress tensor $\sigma_{ij}$
, evaluated at $z=0$:
\[
\sigma _{zz} =\frac 1{4\pi }\int_0^\infty d\omega \int \frac{d^2q}{(2\pi)^2}
\Big[ <\left|
E_z(\mathbf{q},\omega ,z)\right| ^2>+<\left| B_z(\mathbf{q},\omega
,z)\right| ^2>
\]
\[
  -<\left| E_x(\mathbf{q},\omega ,z)\right| ^2> -<\left| E_y(\mathbf{q},\omega ,z)\right| ^2>
\]
\begin{equation}
 -<\left| B_x(\mathbf{q}
,\omega ,z)\right| ^2> - <\left| B_y(\mathbf{q}
,\omega ,z)\right| ^2>\Big] _{z=0}   \label{3thirteen}
\end{equation}
 To linear order in the
vibrational coordinate $u(t)$ and the frequency $%
\omega _{0\text{ }},$ the stress acting on the surface \textbf{1} can be
written in the form
\begin{equation}
\sigma _{zz}=\sigma _{0zz}(d)+u(t)\frac \partial {\partial d}\sigma
_{0zz}(d)+i\omega _0\gamma _{\perp }u(t)  \label{3fifteen}
\end{equation}
Here the first term determines the conservative van der Waals stress and the
second term is the adiabatic change of the conservative van der Waals stress during
vibration. The last term determines the frictional stress with friction coefficient
$\gamma_{\perp}$. For normal relative
motion (see Appendix A) we obtain the friction coefficient
$\gamma _{\perp} =\gamma_{\perp}^{rad}+\gamma_{\perp}^{evan}$,
where the contribution to the friction coefficient from the propagating
electromagnetic waves is given by
\[
\gamma_{\perp}^{rad}=\frac{\hbar}{4\pi^2}\int_0^{\infty}d\omega
\left(-\frac{\partial n}{\partial \omega}\right)\int_0^{\omega/c}dq\,qp^2
\]
\[
\times   \big[(1-|R_{1p}R_{2p}|^2)^2+|(1-|R_{1p}|^2)R_{2p}e^{ipd}
\]
\begin{equation}
+(1-|R_{2p}|^2)R_{1p}^{*}e^{-ipd}|^2\big]\frac 1{\left|1-e^{2ipd}R_{1p}R_{2p}\right|^4}
+[p\rightarrow s],  \label{3seventeen}
\end{equation}
and where the contribution to the friction from the evanescent electromagnetic
waves is given by
\[
\gamma_{\perp}^{evan}=\frac{\hbar}{\pi^2}\int_{\omega/c}^{\infty}d\omega
\left(-\frac{\partial n}{\partial \omega}\right)\int_{\omega/c}^{\infty}dq\,
qk^2e^{-2kd}
\]
\[
\times \big[\big(\mathrm{Im}R_{1p}+
e^{-2kd}\left|R_{1p}\right|^2\mathrm{Im}R_{2p}\big)\big(\mathrm{Im}R_{2p}+
e^{-2kd}\left|R_{2p}\right|^2\mathrm{Im}R_{1p}\big)
\]
\begin{equation}
+e^{-2kd}\big(\mathrm{Im}\big(R_{1p}R_{2p}\big)\big)^2\big]
\frac 1{\left|1-e^{-2kd}R_{1p}R_{2p}\right|^4}
+[p\rightarrow s],
\label{3eighteen}
\end{equation}
where $k=|p|$. The symbol $[p\rightarrow s]$ in Eqs. (\ref{3seventeen}) and
(\ref{3eighteen}) denotes the term which is
obtained from the first one by replacement of the reflection factors $%
R_p(\omega ),$ for $p-$ polarized waves, by the reflection factors $%
R_s(\omega )$ for $s-$ polarized waves. The friction coefficient for
two flat surfaces in parallel relative motion was obtained by us before,
 \cite{Volokitin1} and
can be written as
$\gamma _{\parallel} =\gamma_{\parallel}^{rad}+\gamma_{\parallel}^{evan}$,
where the contribution to the friction coefficient from the propagating
electromagnetic waves is given by
\[
\gamma_{\parallel}^{rad}=\frac{\hbar}{8\pi^2}\int_0^{\infty}d\omega
\left(-\frac{\partial n}{\partial \omega}\right)\int_0^{\omega/c}dq\,q^3
\]
\begin{equation}
\times   \frac{(1-|R_{1p}|^2)
(1-|R_{2p}|^2)}{\left|1-e^{2ipd}R_{1p}R_{2p}\right|^2}
+[p\rightarrow s],  \label{3nineteen}
\end{equation}
and where the contribution to the friction from the evanescent electromagnetic
waves is given by
\[
\gamma_{\parallel}^{rad}=\frac{\hbar}{2\pi^2}\int_0^{\infty}d\omega
\left(-\frac{\partial n}{\partial \omega}\right)\int_{\omega/c}^{\infty}dq\,
q^3e^{-2kd}
\]
\begin{equation}
\times \mathrm{Im}R_{1p}
\mathrm{Im}R_{2p}
\frac1{\left|1-e^{-2kd}R_{1p}R_{2p}\right|^2}
+ [p\rightarrow s].
\label{3twenty}
\end{equation}
There is a principal difference
between the friction coefficient for normal and parallel relative motion,
related to the denominator in the formulas for the friction coefficient.
The resonant condition corresponds to the case when the denominator of the integrand
in Eqs. (\ref{3seventeen}-\ref{3twenty}), which is due to multiple
scattering of the evanescent electromagnetic
waves from the opposite surfaces, is small. For two identical surfaces and
$R_{i}<<1\le R_r$,
where $R_i$ and $R_r$ are the imaginary and real part, respectively, this
corresponds to the resonant condition $R_r^{2}\rm{exp}(-2kd)\approx 1$. At
resonance the integrand in Eqs. (\ref{3nineteen}) and (\ref{3twenty})
has a large factor $\sim 1/R_i^2$,
in  sharp contrast to the case of parallel relative motion, where  there is no such
enhancement factor. The resonance condition can be fullfiled even for the case
when $\rm{exp}(-2kd)<<1$ because for evanescent electromagnetic waves there is no
restriction on the magnitude of the real part or the modulus of $R$.
This open up the possibility of
resonant denominators for $R_r^2>>1$.

To estimate the friction coefficient $\Gamma$ for an atomic force microscope
tip we can use an approximate formula \cite{Hartmann,Johansson}
\begin{equation}
\Gamma=2\pi\int_0^\infty d\rho\rho\gamma(z(\rho))
\label{approx}
\end{equation}
where it is assumed that the tip has cylinder symmetry. Here $z(\rho)$
denotes the tip - surface distance as a function of the distance $\rho$
from the tip symmetry axis, and the friction coefficient $\gamma(z(\rho)$
is determined by the expressions for the flat surfaces. This scheme was
proposed in \cite{Hartmann} for the calculation of the conservative van der
Waals interaction. The error of these scheme is not larger than 5-10\% in
practice in an atomic force microscopy experiment, and 25\% in a worst case
satiation \cite{Johansson}. Although this scheme was proposed for the
conservative van der Waals interaction, we assume that the same scheme is
also valid for the calculation of the van der Waals friction. We assume that
the tip has a paraboloid shape given [in cylindrical coordinates ($z,\rho$)]
by the formula:$z=d+\rho^2/2R$, where $d$ is the distance between the tip
and the flat surface, and where $R$ is the radius of curvature of the tip.
In the case of the power dependence
\[
\gamma(\rho) = \frac{C}{\left(d+\frac{\rho^2}{2R}\right)^n}
\]
we get
\[
\Gamma=\frac{2\pi R}{n-1}\frac{C}{d^{n-1}}=\frac{2\pi Rd}{n-1}\gamma(d)
\]
In a more  general case one must use  numerical integration.

In the local optic approximation, where the dielectric function
is assumed to depend only on the frequency $\omega$,
the reflection factors  $R_{p}$ and $R_{s}$ for flat surfaces,
 covered by an adsorbate layer, are
 given by \cite{Langreth}:
\begin{equation}
R_{p}=\frac {p   -s/\epsilon-4\pi in_aq
[s\alpha_{\parallel}/\epsilon-q \alpha_{\perp}]}
{p+s/\epsilon-4\pi in_aq[s\alpha_{\parallel}/\epsilon+q \alpha_{\perp}]},
\label{3twentyone}
\end{equation}
\begin{equation}
R_{s}=\frac {p   -s-4\pi in_a(\omega/c)^2\alpha_{\parallel}}
{p   +s+4\pi in_a(\omega/c)^2\alpha_{\parallel}}, \label{3twentytwo}
\end{equation}
where
\begin{equation}
s=\sqrt{\left(\frac{\omega}{c}\right)^2\epsilon - q^2},
\end{equation}
and where $\alpha_{\parallel}$ and $\alpha_{\perp}$ are the
polarizabilities of adsorbates
in a direction parallel and normal to the surface,  respectively. Here
$\epsilon=\epsilon(\omega)$
is the bulk  dielectric function and $n_a$ is
the concentration of adsorbates. For clean surfaces $n_a=0$, and in this
case formulas (\ref{3twentytwo,3twentythree}) reduce to the well-known Fresnel formula.

At $d<l,v_F/\omega$ and $k_F\sim 1$, where $l$ is the electron mean
free path, and where $v_F$ and $k_F$ are the Fermi velocity and Fermi wave number,
respectively,
the system will be characterized by
non-local dielectric function $\epsilon(\mathbf{q},\omega)$.
In this paper  we use
the non-local optic dielectric
approach, proposed some years ago for the investigations of the
optical properties of a semi-infinite electron gas \cite{Fuchs and Kliever}.

Accordingly  to  \cite{Fuchs and Kliever}, the reflection factor for $p$
- polarized electromagnetic field, incident on the flat surface, is
determined by \cite{Fuchs and Kliever}
\begin{equation}
R_p=\frac{p-Z_p}{q+Z_p},  \label{rone}
\end{equation}
 where the surface impedance $Z_p$ is given by
\begin{equation}
Z_p=\frac {2i}{\pi} \int_0^\infty \frac{\mathrm{d}q_z}{Q^2}\left( \frac{q^2}{%
\epsilon _l(\omega ,Q)}+\frac{(\omega /c)^2q_z^2}{(\omega /c)^2\epsilon
_t(\omega ,Q)-Q^2}\right) ,  \label{rtwo}
\end{equation}
where $\epsilon _l$ is the finite- life- time generalization of the
longitudinal Lindhard dielectric function which accordingly to \cite{Mermin}
can be written as:
\begin{equation}
\epsilon _l(\omega ,Q)=1+\frac{(1+\mathrm{i}/\omega \tau )(\epsilon
_l^0(\omega +\mathrm{i}/\tau ,Q)-1)}{1+(\mathrm{i}/\omega \tau )(\epsilon
_l^0(\omega +\mathrm{i}/\tau ,Q)-1)/(\epsilon _l^0(0,Q)-1)},  \label{rthree}
\end{equation}
\begin{equation}
\epsilon _l^0(\omega ,Q)=1+\frac{3\omega _p^2}{Q^2v_F^2}f_l,  \label{rfour}
\end{equation}
\begin{equation}
f_l=\frac 12+\frac 1{8z}\left( [1-(z-u)^2]\ln \frac{z-u+1}{z-u-1}%
+[1-(z+u)^2]\ln \frac{z+u+1}{z+u-1}\right) ,  \label{rfive}
\end{equation}
where $Q^2=q^2+q_z^2,z=Q/2k_F,u=\omega /(Qv_F)$, $\omega _p$ is the plasma
frequency, $\tau $ is the Drude relaxation time, and where $v_F$ and $k_F$
are the Fermi velocity and wave vector, respectively. For $s-$ polarization
the reflection factor is determined by
\begin{equation}
R_s=\frac{1-Z_sp}{1+Z_sp}  \label{rsix}
\end{equation}
where
\begin{eqnarray}
Z_s &=&\frac {2i}{\pi} \int_0^\infty \frac{\mathrm{d}q_z}{(\omega /c)^2\epsilon
_t(\omega ,Q)-Q^2}  \label{rseven} \\
\epsilon _t(\omega ,Q) &=&1-\frac{\omega _p^2}{\omega (\omega +\mathrm{i}%
\gamma )}f_t,  \label{reight} \\
f_t &=&\frac 38(z^2+3u^{\prime 2}+1)-\frac 3{32z}\left( [1-(z-u^{\prime
})^2]^2\ln \frac{z-u^{\prime }+1}{z-u^{\prime }-1}\right.  \nonumber \\
&&\left. +[1-(z+u^{\prime })^2]^2\ln \frac{z+u^{\prime }+1}{z+u^{\prime }-1}%
\right)  \label{rnine}
\end{eqnarray}
with $u^{\prime }=(\omega +\mathrm{i}\tau ^{-1})/(Qv_F)$. We show in Sec.4
that the maximum of the electromagnetic friction is reached for small
electron densities, where the electron gas becomes non-degenerate (the electro
 gas is degenerate for $k_BT<<\varepsilon_F$ and non-degenerate for $k_BT\ge
\varepsilon_F$, where $\varepsilon_F$ is the Fermi energy). For non-degenerate
 electron gas  we use the following classical expressions for dielectric functions
\cite{Landau}
\begin{eqnarray}
\epsilon _l^0(\omega ,Q) &=&1+\left( \frac{\omega _p}{Qv_T}\right) ^2\left[
1+F\left( \frac \omega {\sqrt{2}Qv_T}\right) \right]  \label{rten} \\
\epsilon _t(\omega ,Q) &=&1+\frac{\omega _p^2}{\omega (\omega +i\gamma )}%
F\left( \frac{\omega +i\gamma }{\sqrt{2}Qv_T}\right)  \label{releven}
\end{eqnarray}
where the function $F(x)$ is defined by the integral
\begin{equation}
F(x)=\frac x{\sqrt{\pi }}\int_{-\infty }^{+\infty }dz\frac{e^{-z^2}}{z-x-i0}
\end{equation}
and $v_T=\sqrt{k_BT/m}$, where $m$ is the electron mass.

\section{The case of the good conductors}

By a well-conducting metal we mean one whose dielectric function
 $\epsilon=1-4\pi i\sigma/\omega$ ($\sigma$ is the conductivity)
 has an absolute value much larger than unity. For good conductors
 at thermal frequencies $R_{pi}<<1$ and $R_{pr}\approx1$. Thus an
enhancement in friction is possible only for very small $q<<1/d$ .

It is convenient to write the  friction coefficient
for the two flat surfaces
in the form
\begin{equation}
\gamma=\hbar\int_0^{\infty}d\omega
\left(-\frac{\partial n}{\partial \omega}\right)\left(I_{ p}
+I_{s}\right)
\end{equation}
Taking into account that $qdq=kdk$,
 from Eq. (\ref{3eighteen}) for normal relative motion of  clean surfaces
within
local optic approximation
 we get contribution to friction from evanescent $p$-and $s$-polarized electromagnetic
waves
\[
I_{\perp p}^{evan}=\int_0^{\infty}\frac{dk}{\pi^2}\,k^5\big[\mathrm{Re}(s/\epsilon)\big]^2
\Big[\big[(k^2+|s/\epsilon|^2)\mathrm{cosh}kd +2k\big[\mathrm{Im}
(s/\epsilon)\big]\mathrm{sinh}kd\big]^2
\]
\begin{equation}
+ (k^2-|s/\epsilon|^2)^2\Big]\frac{1}{\left|\big((s/\epsilon)^2-k^2\big)
\mathrm{sinh}kd
 + 2ik(s/\epsilon)\mathrm{cosh}kd\right|^4}
\label{4one}
\end{equation}
\[
I_{\perp s}^{evan}=\int_0^{\infty}\frac{dk}{\pi^2}\,k^5\big[\mathrm{Re}s\big]^2
\Big[\big[(k^2+|s|^2)\mathrm{cosh}kd +2k\mathrm{Im}
s\mathrm{sinh}kd\big]^2
\]
\begin{equation}
+ (k^2-|s|^2)^2\Big]\frac{1}{\left|\big(s^2-k^2\big)
\mathrm{sinh}kd
 + 2iks\mathrm{cosh  }kd\right|^4}
\label{4two}
\end{equation}
As $k\rightarrow 0$, there is no singularity in $I_{\perp s}^{evan}$,
and for $I_{\perp p}^{evan}$,
for $(c/\omega)|\epsilon|^{-3/2}<d<(c/\omega)|\epsilon|^{1/2}$, than
taking into account that in this limit
 $\mathrm{sinh}kd\approx kd$ and $\mathrm{cosh}kd\approx 1$, we get
\[
I_{\perp p}^{evan} = 2(\omega/c)^2\zeta^{\prime}\int_0^{\infty}
\frac{dk}{\pi^2}\frac{k^5}{\left|k^2d-2i(\omega/c)
(\zeta)\right|^4}
\]
\begin{equation}
=\frac {\omega\zeta^{\prime}}{\pi^2 cd^3}\left(\frac{\pi}{2}+\arctan
\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right). \label{4three}
\end{equation}
where the surface impedance  $\zeta=\epsilon^{-1/2}=
\zeta^{\prime}-i\zeta^{\prime \prime}$.
For $d<(c/\omega)|\epsilon|^{-1/2}$, $I_s$ becomes slowly dependent on $d$:
\begin{equation}
I_{\perp s} \approx \frac{1}{8\pi^2}(\omega/c)^4|\epsilon|^2
(1.22-\ln(2d|\epsilon|^{1/2}\omega/c)  \label{4four}
\end{equation}
For $d>(c/\omega)|\epsilon|^{-1/2}$ we get
\begin{equation}
I_{\perp s}\approx (c/\omega)^2\zeta^{\prime 2}d^{-6}
\label{4five}
\end{equation}
For the propagating electromagnetic waves, taking into account that $qdq=-pdp$,
we get
\begin{equation}
I_{\perp p}^{rad}=(\omega/c)^2\zeta^{\prime 2}\int_0^{\omega/c}\frac{dp}{\pi^2}p^5
\frac{1+\cos^2(pd)}{|p\sin pd +2i(\omega/c)\zeta\cos pd|^4},
\label{4six}
\end{equation}
\begin{equation}
I_{\perp s}^{rad}=(\omega/c)^2\zeta^{\prime 2}\int_0^{\omega/c}\frac{dp}{\pi^2}p^5
\frac{1+\cos^2(pd)}{|(\omega/c)\sin pd+ 2ip\zeta\cos pd|^4}
\label{4seven}
\end{equation}
For $d<(c/\omega)|\epsilon|^{-1/2}$ the contribution to friction from propagating
wave is negligibly small in the comparison with the contribution from the
evanescent waves. For $d>(c/\omega)|\epsilon|^{-1/2}$
 as $p\rightarrow 0$, the integral $I_{\perp s}^{rad}$ has no singularity, and
we  get for $I_p^{rad}$
\begin{equation}
I_{\perp p}^{rad}\approx\frac {\omega\zeta^{\prime}}{4\pi^2 cd^3}
\left(\frac{\pi}{2}-\arctan
\zeta^{\prime \prime}/\zeta^{\prime} +\frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right). \label{4eight}
\end{equation}
In addition, $I^{rad}$ has singularities at the other zeroes of $\sin pl$,
 i.e., near the values $p_n=n\pi/d<\omega/c$ ($n$ is an integer). In the vicinity of $p_n$,
putting $p=p_n+p^{\prime}$, we have $\sin pd\approx(-1)^n$ and $\cos pd\approx(-1)^n$,
\[
I_{\perp p}^{rad}\approx2(\omega/c)^2\zeta^{\prime 2}\int\frac{dp^{\prime}}{\pi^2}
\frac{1}{|p_np^{\prime}d+2i(\omega/c)\zeta|^4}
\]
\begin{equation}
\approx \frac{p_n^4c}{8\pi^2\omega d\zeta^{\prime}}\left(\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right)
\label{4nine}
\end{equation}
The number $m$ of such contribution is obviously equal to the integer part
 of the quantity $y=\omega d/\pi c$ ($m=[y]$), so that all $p_n$ (with
the exception of $p=0$) make a summary contribution
\[
 \frac{\pi^2c}{8\omega d^5\zeta^{\prime}}\left(\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right)\sum_1^m n^4=
\]
\[
\frac{\pi^2c}{8\omega d^5\zeta^{\prime}}\left(\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right)
\]
\begin{equation}
\times \left[\frac{(m+1)^5}{5}-\frac{(m+1)^4}{2}+\frac{(m+1)^3}{3} -
\frac{m}{30}-\frac {1}{30}\right]
\label{4ten}
\end{equation}
In the integral $I_{\perp s}^{rad}$, the contribution from the vicinity
of the point $p_n$ is
\[
2(\omega/c)^2\zeta^{\prime 2}\int_0^{\omega/c}\frac{dp^{\prime}}
{\pi^2}\frac{p_n^5}{|(\omega/c)p^{\prime}d+2ip_n\zeta|^4}=
\]
\[
=\frac{\omega n^2}{8cd^3\zeta^{\prime}}\left(
\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right)
\]
and consequently
\[
I_{\perp s}^{rad}=\frac{\omega }{8cd^3\zeta^{\prime}}\left(
\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right) \sum_1^m n^2=
\]
\begin{equation}
\frac{\omega }{48cd^3\zeta^{\prime}}\left(
\frac{\pi}{2}
-\arctan\zeta^{\prime \prime}/\zeta^{\prime}- \frac{\zeta^{\prime \prime}/
\zeta^{\prime }}{1+(\zeta^{\prime \prime}/
\zeta^{\prime})^2}\right)m(m+1)(2m+1)
\label{4eleven}
\end{equation}
At $m>>1$, when we can assume $m\approx \pi \omega/cd$, the $s-$ and $p-$
wave contribution are approximately equal, and for the total contribution
 from propagating electromagnetic waves in this limit we get
\begin{equation}
I_{\perp}^{rad}=I_{\perp p}^{rad} +I_{\perp s}^{rad}\approx\frac
{11\omega^4}{240\pi^3c^4\zeta^{\prime}}
\label{4twelve}
\end{equation}
The above formulas in this Section were obtained from the general Eqs.
(\ref{3seventeen}-\ref{3twenty}) assuming absence of spatial dispersion
of the dielectric function. But these formulas contain only surface
impedance $\zeta$ that describe the ratio of the tangential components of the
           electric and magnetic fields on the boundary of the body. Thus, the
results in this section remain in force also in the presence of spatial
dispersion, provided only that the surface impedance of the medium is
small enough. We would have arrived at the same formulas also if we were
to assume from the very beginning that the Leontovich boundary condition
$\mathbf{E}=\zeta\mathbf{H}\times\mathbf{n}$ is satisfied on the surface
of the metal.

At not too low temperatures, the impedances of metals are given by the
formula for normal skin effect
\begin{equation}
\zeta^{\prime}=\zeta^{\prime \prime}=(\omega/8\pi\sigma)^{1/2}
\label{4thirteen}
\end{equation}
where $\sigma$ is the conductivity. In the local optic approximation it is
assuming that there is no dependence of $\sigma$ on $\mathbf{q}$. In the
Wien region of frequencies it is also good approximation to neglect by
the frequency dependence of $\sigma$. In this approximation using (\ref{4three})
 for $\lambda_W(k_{B}T/4\pi\hbar\sigma)^{3/2}<d<\lambda_W(4\pi\hbar\sigma/
(k_{B}T)^{1/2}$ ($\lambda_W=c\hbar/(k_{B}T $)
we get
\begin{equation}
\gamma_{\perp p}^{evan}=\hbar\int_0^{\infty}d\omega\left(-\frac{\partial n}
{\partial \omega}\right)I_{\perp p}^{evan}\approx 0.13\frac{\hbar}{d^3\lambda_{W}}
\left(\frac{k_{B}T}{4\pi\hbar\sigma}\right)^{1/2}
\label{4fourteen}
\end{equation}
For the comparison the $p$-wave contribution for parallel relative motion
 for $d<\lambda_c,\,
(\lambda_c=c/(4\pi\sigma k_{B}T)^{1/2})$
is given by (\cite{Volokitin1,Volokitin2})
\begin{equation}
\gamma_{\parallel p}^{evan}\approx 0.3\frac{\hbar}{d^4}\left(\frac{k_BT}{4\pi\hbar
\sigma}\right)^2
\label{4fifteen}
\end{equation}
It is interesting to note that for normal relative motion in contrast to the parallel
relative motion practically for all $d>0$ the main contribution to friction comes
from retardation effects because Eqs. (\ref{4fourteen}) in contrast to
 Eq. (\ref{4fifteen}) contains the light velocity.

From Eq. (\ref{4four}) we get $s$-wave contribution to friction
 for $d<\lambda_c$
\begin{equation}
\gamma_{\perp s}^{evan}\approx10^{-2}\frac{\hbar}{\lambda_c^4}(3-
5\ln(2d/\lambda_c))
\label{4sixteen}
\end{equation}
For parallel relative motion the $s$-wave contribution is in two times
smaller.

For $d>\lambda_c$, taking into account that Eq. (\ref{4five}) is valid
only for $\omega>c^2/4\pi\sigma d^2$, we get
\begin{equation}
\gamma_s^{evan}\approx\frac{\pi k_BT\sigma}{d^2c^2}
\label{44one}
\end{equation}

From Eq. (\ref{4twelve}) we get distance independent contribution to
friction from propagating electromagnetic waves for $d>\lambda_W$
\begin{equation}
\gamma_{perp}^{rad}\approx1.9\cdot10^{-2}\frac{\hbar}{\lambda_W^3\lambda_c}
\label{4seventeen}
\end{equation}

Figures 1-2  show the calculated contribution to the friction
coefficient $\gamma $ from evanescent electromagnetic waves
for two semi-infinite solids, with parameters chosen
to correspond to copper ($\tau ^{-1}=2.5\cdot 10^{13}s^{-1}$, $\omega
_p=1.6\cdot 10^{16}s^{-1})$ at $T=273\,K$, for parallel (Fig.1) and normal
(Fig.2) relative motion. Results are shown separately for
both the $s$- and $p$- wave contribution. The dashed line show the result
when the local (long-wavelength) dielectric function $\epsilon (\omega
)=\epsilon _l=\epsilon _t$ is used, where
\begin{equation}
\epsilon (\omega )=1-\frac{\omega _p^2}{\omega (\omega +\mathrm{i}\tau ^{-1})%
}
\end{equation}
In this case the integration in (\ref{rtwo}) and (\ref{rseven}) can be
performed analytically and we get Fresnel formulas.
Fig. 1 shows that the non-local optic effects become important
for parallel relative motion for the $p-$
wave contribution for sufficiently small separations ($d<1000\,\mathrm{\AA }$%
). However, for the $s-$ wave contribution for both parallel and
 normal motion the non-local optic effects are
negligibly small for practically all separations. For normal relative
motion for $p$-wave contribution the non-local optic effects are less important
than for the parallel relative motion. In the present
calculations we use the non-local dielectric approach which take into
account the non-local optic effects on the length scale of the skin-depth. There
are also the short range non-local optic effects coming from the non-local
nature of the screening response near the surface.
 This gives the  surface non-local
contribution which we investigated in our previous publications \cite
{Persson and Volokitin,Volokitin2}. Comparing our previous calculations with
the present one, we find that for $d>10\mathrm{\AA }$ the volume
contribution from the non-local effects is of the same importance as the
surface contribution. For $d>10\,$\AA\ the main contribution to the friction
coefficient $\gamma $ comes from $s$-polarized waves. In particularly, at $%
d=100$ \AA\ the $s$-wave contribution $\gamma _s\approx
10^{-5}kgs^{-1}m^{-2} $, so that with the surface area $A\approx 10^{-14}$m$%
^{-2}$ ( typical for probe scanning microscopy), the friction coefficient is
$\Gamma \approx \gamma _sA\sim 10^{-19}kgs^{-1}$. The $s-$wave contribution
is characterized by weak distance dependence for $d<100$\AA , and $\gamma
\sim d^{-2}$ for $d>100$\AA . For good conductors like copper, even for very
short distances, the main contribution to the friction coefficient comes
from the $s-$ polarized electromagnetic waves. This difference between $p-$
and $s-$ polarized waves results from screening effects: Good conductors are
good reflectors for $p-$ polarized field, which implies that they are
ineffective in the emission and absorption of evanescent $p-$ polarized
waves. However these screening effects are less important for $s-$ polarized
waves.

As pointed out in \cite{Volokitin1,Volokitin2,Volokitin3,Volokitin4},
the $p$ -wave contribution increase and the $s-$wave contribution decrease
when the free electron density decrease. Within the local optic
approximation the force of friction diverges when one go to the limit of
zero conductivity. This situation is different from the radiative heat
transfer, where, even in the case of local optics, a maximum in the heat
transfer occurs for conductivities corresponding to semi-metals.
Fig.3 shows the dependence of coefficient of friction on the electron
density. When the electron density decreases there is transition from a
degenerate electron gas to a non-degenerate electron gas at the density $%
n_F\sim (k_BTm)^{3/2}/\pi ^2\hbar ^3$. At $T=273\,K$ the transition density $%
n_F\sim 10^{25}\,m^{-3}$. For $n>n_F$ we use the (non-local) dielectric
function appropriate for a degenerate electron gas, while for $n<n_F$ we use
an expression corresponding to a non- degenerate electron gas. In the
calculations we used the electron mean free path $l\approx 600\,\mathrm{\AA }
$. At $d=100$\AA\   the maximum value $\gamma _{max}\sim 10^{-4}\,kg\cdot s^{-1}$ is obtained
for $n_{max}\sim 10^{22}\,m^{-3}$, corresponding to the DC conductivity $%
\sigma \sim 1(\Omega \cdot m)^{-1}.$

\section{Photon tunneling enhancement of the van der Waals friction}

We rewrite the denominator in Eq. (\ref{3eighteen}) in the form
\[
|1-e^{-2kd}R|^4=[(1-e^{-kd}R_r)^2+e^{-2kd}R_i^2]^2
\]
\begin{equation}
\times [(1+e^{-kd}R_r)^2+e^{-2kd}R_i^2]^2
\label{5one}
\end{equation}
where $R_r$ and $R_i$ are real and imaginary part of $R$, respectively
($R=R_r+iR_i$). Let us suppose that $|R_r|>>R_i$. In this case resonant
conditions are determined by equation
\begin{equation}
R_r(\omega_{\pm}(q)=\pm e^{qd}
\label{5two}
\end{equation}
Close to resonance we can write
\[
[(1\pm e^{-qd}R_r)^2\pm e^{-2qd}R_i^2]
\]
\begin{equation}
\approx e^{-2qd} R_r^{\prime 2}(\omega_{\pm})[(\omega-\omega_{\pm})^2+
(R_i(\omega_{\pm})/ R_r^{\prime}(\omega_{\pm}))^2]
\label{5three}
\end{equation}
where
\[
R_r^{\prime}(\omega_{\pm})=\left.\frac{dR_r^{\prime}(\omega)}{d\omega}
\right|_{\omega=\omega_{\pm}}
\]
which leads to the following contribution to the friction coefficient:
\begin{equation}
\gamma_{\pm} \approx \frac{\hbar^2}{16k_BT}\int_0^{q_c}dk\,k^3
\frac{e^{2kd}}{[|R_r^{\prime}(\omega_{\pm})|
R_i(\omega_{\pm})\sinh^2\hbar\omega_{\pm}/2k_BT]}
\label{5four}
\end{equation}
The parameter $q_c$ in this expression defines the value of $q$ where
the two poles approximation is valid. To proceed further let us make
the following simplifications. Close to the poles we can
 use approximation
\begin{equation}
R=\frac{a}{\omega-\omega_0-i\eta}
\label{5six}
\end{equation}
where $a$ is a constant. Then from resonant condition (\ref{5two}) we get
\[
\omega_{\pm}=\omega_0\pm ae^{-qd}
\]
For the two poles approximation to be valid the difference $\Delta\omega =
|\omega_+-\omega_-|$ must be greater than the width of the resonance $\eta$.
 From this condition we get
$q_c\le\ln(2a/\eta)/d$.
For the short distances the parameter $q_c$ defines the value of $q$ where
the solution of Eq. (\ref{5two}) ceases to exit.

For $\omega_0>a$ and $q_cd>1$ from Eq. (\ref{5four}) we get
\begin{equation}
\gamma_{\perp\pm}=\frac{3}{128}\frac{\hbar^2a^2}{d^4k_{B}T\eta}
\frac{1}{\sinh^2(\hbar\omega_0/2k_BT)}
\label{5seven}
\end{equation}

For the parallel relative motion using the same approximation we get
\begin{equation}
\gamma_{\parallel}=\frac{\hbar^2 \eta q_c^4}{128\pi k_{B}T}
\frac{1}{\sinh^2(\hbar\omega_0/2k_BT)}
\label{5eight}
\end{equation}
Interesting, the explicit $d$ dependence has dropped out of Eq. (\ref{5eight}).
However, $\gamma_{\parallel}$ is still $d$ dependent, through the $d$ dependence
of $q_c$. For the small distances one can expect that $q_c$ is determined
by the dielectric properties of the material and does not depend on $d$. In this
case the friction will be also distance independent. Probably, the weak distance
dependence observed in \cite{Stipe} can be explained by the resonant photon
tunneling.

Resonant photon tunneling enhancement of the van der
Waals friction is possible for two semiconductor surfaces which can support
low-frequency surface plasmon modes. As an example we consider
two clean surfaces of silicon carbide (SiC). The
optical properties of this material can be described using an oscillator
model \cite{Palik}
\begin{equation}
\epsilon(\omega)=\epsilon_{\infty}\left(1+\frac{\omega_L^2 - \omega_T^2}
{\omega_T^2 - \omega^2 -i\Gamma \omega}\right)
\label{5nine}
\end{equation}
with $\epsilon_{\infty}=6.7, \,\omega_L=1.8\cdot10^{14}s^{-1},\,
\omega_T=1.49\cdot10^{14}s^{-1},\,$ and $\Gamma=8.9\cdot10^{11}s^{-1}.$ The
frequency of surface plasmons is determined by condition
$\epsilon_r(\omega_p)=
-1$ and from (\ref{three}) we get $\omega_p=1.78\cdot10^{14}s^{-1}$. In Fig.2
we plot the friction coefficient $\gamma(d)$: note that the
friction between the two semiconductor surfaces is  several order of magnitude
larger than between two clean  good conductor surfaces.

Another enhancement mechanism is connected with resonant photon tunneling
between adsorbate vibrational modes localized on different surfaces.
As an example, let us consider ions with charge $e^*$ adsorbed on metal surfaces.
The polarizability for ion vibration normal to the surface is given by
\begin{equation}
\alpha_{\perp}=\frac {e^{*2}}{M(\omega_{\perp}^2-\omega ^2 -i\omega \eta_{\perp})},
\end{equation}
where $\omega_{\perp}$ is the frequency of the normal adsorbate  vibration,
and $\eta_{\perp}$ is the damping constant.
In Eq. (\ref{3twentyone}) the contribution  from parallel vibrations
is reduced by the small factor $1/\epsilon$. However, the contribution
of parallel vibrations to the van der Waals friction
 can nevertheless   be important
due to the indirect interaction of parallel adsorbate vibration with the electric field,
via the metal conduction electron \cite{Persson and Volokitin2}. Thus, the small
parallel component
of the electric field will induce a strong electric current in the metal.
The drag force between
the electron flow and adsorbates can induce adsorbate vibrations  parallel to the
surface. This gives the polarizability:
\begin{equation}
\alpha_{\parallel}=\frac {\epsilon -1}{n}\frac {e^{*}}{e}\frac {\omega \eta_{\parallel}}
{(\omega^2_{\parallel}-\omega^2 -i\omega \eta_{\parallel})}
\end{equation}
where $n$ is the conduction electron concentration.
As an illustration, in Fig.3 we show coefficient of friction for the two
Cu(001) surfaces covered by a low concentration of potassium atoms
( $n_a=10^{18}m^{-2}$)
. In  the $q-$
integral in Eqs.(\ref{3eighteen},\ref{3twenty}) we used the cut off
$q_c \sim \pi/a$ (where $a\approx1nm$
is the inter-adsorbate
distance) because our microscopic approach is applicable only when the wave length
of the electromagnetic field is larger than double average distance between the
adsorbates.
 In comparison, the friction
between two clean surface at separation $d=1nm$ is seven order of
magnitude smaller.
 At $d=1nm$
the friction coefficient $\Gamma$ for an atomic force microscope tip
with $R \sim 1\mu m$
is $\sim 10^{-12}kgs^{-1}$ ($\gamma \sim 10^{3}kgs^{-1}m^{-2}$, see
Fig.2);
this is of the same order of magnitude
as the  observed friction \cite{Stipe}.

\section{Summary and conclusion}

We have calculated the van der Waals friction between two flat surfaces
for normal relative motion and found a drastic difference in the comparison
with parallel relative motion. This difference is connected with resonance
produced by the multiple scattering of the electromagnetic waves from the opposite
surfaces. In the case of sharp resonance it gives much larger contribution to
friction in the case of normal relative motion than for parallel relative
motion.

We have studied in the detail the friction between two good conductors and have
found that for normal relative motion even for very small distances the main
contribution to friction comes from the retardation effects. The non-local optic
effects are very important for $p$-wave contribution to friction for parallel
relative and much less important for normal relative motion. For $s$-wave
contribution the non-local optic effects are unimportant for both direction
of relative motion.

In the case of van der Waals friction we have found that for distances
between bodies $\sim 100$\AA ,\ for good conductors with a high free
electrons concentration, the main contribution to friction is associated
with the $s$-polarized electromagnetic waves. For $d<100$\AA\ this mechanism
gives a friction coefficient per unit area $\gamma \sim 10^{-5}$kgs$^{-1}$m$
^{-2},$ nearly independent of the distance $d,$ while for $d>100$\AA\ the
friction coefficient $\gamma $ depends on distance as $d^{-2}.$ For an
atomic force microscope tip with the near substrate area $A\sim 10^{-14}$m$
^2,$ we got  the friction coefficient $\Gamma \sim \gamma A\sim 10^{-19}$kgs
$^{-1}$ for $d<100$\AA. When the concentration of electrons decreases,
the $s-$contribution to the friction decreases while the $p-$ contribution
increases. At $d=100$\AA\   and with the electron lifetime $\tau = 4 \cdot
 10^{-14}$s, the $p-$ contribution reaches maximum $\gamma _{\max }\sim
10^{-4}$kgs$^{-1}$m$^{-2}$ at the electron concentration $n\sim 10^{22}$m$
^{-3},$ which corresponds to the conductivity $\sigma \sim 1\,$($\Omega $m)$
^{-1}.$

We have shown that the van der Waals friction can be enhanced by several orders of
magnitude in the case of resonant photon tunneling between low-frequency
surface plasmon modes and adsorbate vibrational modes. In the case of friction
for two Cu(100) surfaces covered by a low concentration of potassium atoms
at $d=10\AA$ we have found friction of the same order of magnitude as it was
observed in experiment \cite{Stipe}. However, the distance dependence in this
case is more stronger than it was observed in \cite{Stipe}. Further experiments
with simple and well defined composition of the tip and sample must be performed
to elucidate different energy dissipation mechanisms in the non-contact friction.

The obtained results should have broad application in non-contact friction microscopy,
and in design of new tools for studying adsorbate vibrational dynamics and optical
properties of the surface plasmons.

\vskip 0.5cm \textbf{Acknowledgment }

A.I.V acknowledges financial support from DFG and the Russian Foundation for
Basic Research (Project No. 01-02-16202) B.N.J. P acknowledges financial
support from BMBF. We thank R.O. Jones for help in the numerical
calculations.\vskip 1cm

redpajama_set_name: RedPajamaArXiv


text:
Q: Is there a url parameter to make Google Custom Search Engine load to a refinement by default? Is there a url parameter that I can add to the search string to trigger Google Custom Search to load to a certain refinement?
I can easily add it to a
, like this:

However, I am trying to append the search query with something like this:
search but it didn't work.
I also tried to implement a javascript code, but did not work too:
search

All trials lead to loading the search results in the default search page without triggering the required refinement.
Can someone help me please? Thanks in advance.

A: You can add a string in the advanced settings to be added to every query.
So, add this - more:p:, followed by your refinement name, and it will always be executed.

redpajama_set_name: RedPajamaStackExchange


text:
Asahi Masuyama (jap. , Masuyama Asahi; * 29. Januar 1997 in Fukuoka, Präfektur Fukuoka) ist ein japanischer Fußballspieler.

Karriere
Asahi Masuyama erlernte das Fußballspielen in der Schulmannschaft der Higashi Fukuoka High School. Seinen ersten Profivertrag unterschrieb er 2015 bei Vissel Kōbe. Der Verein aus Kōbe, einer Großstadt auf der Insel Honshū, spielte in der höchsten japanischen Liga, der J1 League. Die Saison 2015 wurde er an den Yokohama FC ausgeliehen. Mit dem Verein aus Yokohama spielte er in der zweiten Liga, der J2 League. Für den Klub absolvierte er neun Zweitligaspiele. Anfang 2018 kehrte er nach der Ausleihe wieder zu Kōbe zurück. 2019 gewann er mit Vissel den Kaiserpokal. Im Finale besiegte man den Erstligisten Kashima Antlers mit 2:0. Anfang 2020 wurde er von dem Zweitligisten Avispa Fukuoka aus Fukuoka ausgeliehen. Ende der Saison wurde er mit dem Verein Vizemeister und stieg in die erste Liga auf. Nach der Ausleihe kehrte er Anfang 2021 wieder zu Vissel zurück. Nach insgesamt 45 Ligaspielen für Vissel wechselte er im August 2021 zum ebenfalls in der ersten Liga spielenden Ōita Trinita. Am Ende der Saison 2021 musste er mit Ōita in die zweite Liga absteigen. Nach insgesamt 36 Ligaspielen wechselte er im Januar 2023 zum ebenfalls in der zweiten Liga spielenden V-Varen Nagasaki.

Erfolge
Avispa Fukuoka
 Japanischer Zweitligavizemeister: 2020

Vissel Kōbe
 Japanischer Pokalsieger: 2019

Weblinks

Fußballspieler (Vissel Kōbe)
Fußballspieler (Yokohama FC)
Fußballspieler (Avispa Fukuoka)
Fußballspieler (Ōita Trinita)
Fußballspieler (V-Varen Nagasaki)
Japaner
Geboren 1997
Mann

redpajama_set_name: RedPajamaWikipedia


text:
Common Redpoll
Common Redpoll Life History
NestingShrub
Common Redpolls breed worldwide in the far northern latitudes, in open woods of pine, spruce, alder, birch, and willow up to about 5,000 feet elevation. In the essentially treeless tundra they find hollows and shelters where deciduous shrubs or conifers can gain a foothold. They also live around towns. Most people get to see them in winter, when redpolls move south. In their winter range, which can be extremely variable as the birds seek unpredictable food sources, redpolls occur in open woodlands, scrubby and weedy fields, and backyard feeders. Back to top
Common Redpolls eat mainly small seeds, typically of trees such as birch, willow, alder, spruces, and pines, but also of grasses, sedges, and wildflowers such as buttercups and mustards, and occasional berries. During summer they also eat considerable numbers of spiders and insects. Winter diet is largely birch and alder seeds or, at feeders, millet and thistle or nyjer seed. Back to top
Females do most of the searching for nest sites. They place their nests over thin horizontal branches or crotches in spruces, alders, and willows. Nests tend to be low to the ground or, on the tundra, placed on driftwood, rock ledges, or other low ground cover.
The female builds the nest on a foundation of small twigs laid across thin branches. She makes the nest from grasses, fine twigs, roots, and tree moss. She lines the nest with a thick layer of ptarmigan or Spruce Grouse feathers, or with hair, lemming fur, wool, or downy plant material. The finished nest is up to 4 inches across with a nest cup of about 2.5 inches diameter and 2 inches deep. Redpolls may take material from old nests to make new ones, but typically do not reuse old nests.
Egg Length: 0.6-0.8 in (1.4-2 cm)
Incubation Period: 11 days
Egg Description: Pale green to pale blue, spotted with purple
Condition at Hatching: Naked and helpless.
Common Redpolls are energetic little birds that forage in flocks, gleaning, fluttering, or hanging upside down in the farthest tips of tree branches. Like many finches, they have an undulating, up-and-down pattern when they fly. To keep order in flocks, redpolls have several ways of indicating their intentions. When quarreling with flockmates, a redpoll fluffs its plumage, faces its adversary, and opens its bill, sometimes jutting its chin to display the black face patch. Males court females but flying in slow circles while calling and singing. Males may feed females during courtship. You may see small flocks of this social species even during the breeding season; during migration they may group into the thousands. In winter, some redpolls roost in tunnels under the snow, where the snowpack provides insulation and stays much warmer than the night air.Back to top
Common Redpolls are numerous. Partners in Flight estimates a global breeding population of 160 million, with 17% spending some part of the year in Canada, and 22% wintering in the U.S. They rate a 7 out of 20 on the Continental Concern Score and they are not on the 2014 State of the Birds Watch List. These birds breed in the far north, away from large numbers of humans and many of their environmental impacts. When they come south to visit more densely populated areas, they can succumb to salmonella infections at feeders. In Europe, they have been trapped for food and to keep as cage birds, although this is less common today. It remains to be seen what changes climate change may cause for their boreal and tundra habitat. Back to top
Common Redpolls eat seeds of a size to match their small bills. They're particularly likely to come to thistle or nyjer feeders, though they may also take black oil sunflower or scavenge opened seeds left behind by larger-billed birds. Find out more about what this bird likes to eat and what feeder is best by using the Project FeederWatch Common Feeder Birds bird list.
Knox, Alan G. and Peter E. Lowther. 2000. Common Redpoll (Acanthis flammea), version 2.0. In The Birds of North America (P. G. Rodewald, editor). Cornell Lab of Ornithology, Ithaca, New York, USA.
Hoary Redpoll
Pine Siskin
Cassin's Finch
Finches, Euphonias, and Allies(Order: Passeriformes, Family:Fringillidae)
Evening Grosbeak
Pine Grosbeak
Gray-crowned Rosy-Finch
Black Rosy-Finch
Brown-capped Rosy-Finch
Cassia Crossbill
White-winged Crossbill
Lesser Goldfinch
Lawrence's Goldfinch

redpajama_set_name: RedPajamaCommonCrawl


text:
import { createStore } from 'redux';
import Reducer from '../reducers/device';

let store = createStore(Reducer);

export default store;

redpajama_set_name: RedPajamaGithub


text:
Q: Can the inverse operator in Bartle-Graves theorem be linear? Bartle-Graves theorem states that a surjective continuous linear operator between Banach spaces has a right continuous inverse that doesn't have to be linear.
Is it possible that this inverse is linear under additional assumption that an operator has a dense kernel?

A: In general the right inverse of a linear bounded operator $T:X\to Y$  in Bartle-Graves theorem needs not to be linear, and there can be no linear bounded right inverse. In this case, any right inverse $S:Y\to X$ is everywhere not Fréchet differentiable nor Gateaux differentiable, because if $S$ is differentiable at $x_0$, by the chain rule $dS(x_0)$ is a bounded linear right inverse to $T$.
Note however that $\tilde S:Y\to X$ defined by $\tilde S(x):=\frac{\|x\|}2\Big( S\big(\frac x{\|x\|}\big)-S\big(-\frac x{\|x\|}\big) \Big)$ is also a right inverse to $T$, and it is
$1$-homogeneous, $S(tx)=tS(x)$. I'm not aware of other possible improvements one can do on $S$.
There can be no linear bounded right inverse: Precisely, a bounded linear operator $T:X\to Y$ between Banach spaces is a left, resp. right (bounded, linear) inverse,  iff it is surjective and its kernel splits, resp. it is injective and its range is closed and splits.
In fact, if $T:X\to Y$ and $S:Y\to X$  are bounded linear operators such that $TS=1_Y$, then $Y=\ker T\oplus \text{ran}\, S,$  with linear projectors $I-ST=[T,S ]$ and $ST$.


text:
Q: How to fix, Input string not in correct format unity 3d and serial I am using unity 3d to visualise a serial output from an Arduino and keep geting the error

FormatException: Input string was not in a correct format.
  System.Number.StringToNumber (System.String str,
  System.Globalization.NumberStyles options, System.Number+NumberBuffer&
  number, System.Globalization.NumberFormatInfo info, System.Boolean
  parseDecimal) (at <599589bf4ce248909b8a14cbe4a2034e>:0)
  System.Number.ParseInt32 (System.String s,
  System.Globalization.NumberStyles style,
  System.Globalization.NumberFormatInfo info) (at
  <599589bf4ce248909b8a14cbe4a2034e>:0) System.Int32.Parse
  (System.String s, System.IFormatProvider provider) (at
  <599589bf4ce248909b8a14cbe4a2034e>:0) System.Convert.ToInt32
  (System.String value) (at <599589bf4ce248909b8a14cbe4a2034e>:0)
  One_mputest.Update () (at Assets/One_mputest.cs:48)

i have tried using plugins and they did not work
C# script:
using System.Collections;
using System.Collections.Generic;
using UnityEngine;
using System.IO.Ports;
using System;
using System.Linq;

public class One_mputest : MonoBehaviour {

private int x;
private int y;
private int z;

private int roll;
private int pitch;
private int yaw;

static SerialPort serial = new SerialPort("COM3", 9600);

// Use this for initialization
void Start () {

    serial.ReadTimeout = 5000;
    if (!serial.IsOpen) {
        try {
            serial.Open ();
        } catch (TimeoutException) {

        }

    } else
        Debug.LogError ("Port already open");
    }

// Update is called once per frame
void Update () {
    if (!serial.IsOpen)
        serial.Open ();

    string ypr = serial.ReadLine ();

    List<String> stringList = ypr.Split('\t').ToList();

    int[] intArray = new int[7];

    for (int s = 0; s < 7; s++)
    {
        intArray[s] = Convert.ToInt32(stringList[s]);
    }

    x = intArray[3];
    y = intArray[0];
    z = intArray[1];

    transform.localEulerAngles = new Vector3(z, y, x);
}

}
The serial input:
-104.65  -10     5   65536.00    0.00    0.00    0.00
-102.74  -4  1   65536.00    0.00    0.00    0.00
-102.19  -2  0   65536.00    0.00    0.00    0.00
-102.09  0   0   65536.00    0.00    0.00    0.00
-101.75  0   0   65536.00    0.00    0.00    0.00
-101.61  0   -1  65536.00    0.00    0.00    0.00
-101.62  0   -1  65536.00    0.00    0.00    0.00
-101.68  0   -1  65536.00    0.00    0.00    0.00
-101.76  0   -1  65536.00    0.00    0.00    0.00
-102.02  0   -1  65536.00    0.00    0.00    0.00
-102.20  0   -1  65536.00    0.00    0.00    0.00
-102.33  0   -1  65536.00    0.00    0.00    0.00
-102.43  0   -1  65536.00    0.00    0.00    0.00
-102.57  0   -1  65536.00    0.00    0.00    0.00
-102.77  0   -1  65536.00    0.00    0.00    0.00
-102.90  0   -1  65536.00    0.00    0.00    0.00
-102.68  0   -1  65536.00    0.00    0.00    0.00
-102.48  0   -1  65536.00    0.00    0.00    0.00
-102.26  0   -1  65536.00    0.00    0.00    0.00
-102.01  0   -1  65536.00    0.00    0.00    0.00
-101.83  0   -1  65536.00    0.00    0.00    0.00
-102.15  0   -1  65536.00    0.00    0.00    0.00
-102.34  0   -1  65536.00    0.00    0.00    0.00
-102.17  0   -1  65536.00    0.00    0.00    0.00
-101.89  0   -1  65536.00    0.00    0.00    0.00
-101.74  0   -1  65536.00    0.00    0.00    0.00
-101.88  0   -1  65536.00    0.00    0.00    0.00
-101.95  0   -1  65536.00    0.00    0.00    0.00
-102.01  0   -1  65536.00    0.00    0.00    0.00
-102.05  0   -1  65536.00    0.00    0.00    0.00
-102.06  0   -1  65536.00    0.00    0.00    0.00
-102.00  0   -1  65536.00    0.00    0.00    0.00
-101.96  0   -1  65536.00    0.00    0.00    0.00
-102.06  0   -1  65536.00    0.00    0.00    0.00
-102.14  0   -1  65536.00    0.00    0.00    0.00
-102.37  0   -1  65536.00    0.00    0.00    0.00
-102.81  0   -1  65536.00    0.00    0.00    0.00

I expected the vector variable to change and move the object that the script was applied to
and only got the error about:  Input string was not in a correct format

A: Try & catch are your friends. It's possible there is an extra \t in the file and you are trying to convert a null into a number somewhere. Also a good tip is always use {} around if statements just to make sure nothing unexpected happens (eg: you think something is inside an if statement but it's outside)
One point I would look at is that you are trying to convert a String representing a Float to an Int32, this may be where things are going wrong.
Try something like this:
void Update () {
    var whatdoing = "starting try";

    try {
        if (!serial.IsOpen) {
            serial.Open (); }

        whatdoing               = "reading line";
        string ypr              = serial.ReadLine ();

        List<String> stringList = ypr.Split('\t').ToList();
        int[] intArray          = new int[7];

         for (int s = 0; s < 7; s++) {
             whatdoing = "converting: " + stringList[s];

             if(!Int.TryParse(stringList[s], out intArray[s]) {
                 throw new Exception("Could not parse string to Int: "+whatdoing); } }
          whatdoing = "Assigning xyz";
          x         = intArray[3];
          y         = intArray[0];
          z         = intArray[1];

          transform.localEulerAngles = new Vector3(z, y, x);}
catch(Exception e) {
 BREAK HERE and check exception & whatdoing.
} }


Lego minifig compatible Custom BrickWarriors Lantern Shield. They would light a fire on the back of the shield and then open the little window in hopes that the fire would blind their opponent and give them an opening to strike.
Click the button below to add the Lantern Shield to your wish list.


Accessories can make the outfit and this lovely ring really adds something special to a wardrobe. With its warm color palette and gorgeous sterling band, it's as flattering as it is feminine. Embellished with a stunning array of Swarovski crystals in a mix of golden orange, soft peach and evening black, this ring is as mesmerizing as the woman who wears it.


Rock and metal largely operate under the radar of the mainstream eye. The demonization of groups has emanated from media coverage surrounding negative events where an artist is often misrepresented or misunderstood as news anchors and analysts mistake image and lyrics for something conveniently fitting within the confines of their narrative.
Unfortunately, the finger is often pointed toward rock and metal groups in the wake of tragedy with Marilyn Manson infamously enduring a firestorm following the Columbine shooting in April of 1999. The killers were fans of Manson, even dressing in a similar fashion to the industrial shock rocker, which naturally intertwined his name with the mass murder.
In a separate event, Judas Priest's Rob Halford found himself defending vocal inflections on the song "Better By You, Better Than Me," a cover of a Spooky Tooth song which appeared on Stained Class. Halford testified in court that the song did not contain subliminal messages that said "do it" which allegedly caused one fan to take his own life.
We're not going to give away everything in this Loud List, but you can get more background on both of the previously mentioned events and more in the video above!


text:
The Love Lives of the Native Americans
Last week I spent a few days in the fine city of Rostov-on-Don (or Rostov na Donu as the locals call it). The local market was a musical treasure trove. They have a rather relaxed approach to copyright over there - I realise I am in no position to cast stones - with the result that you get some amazing bargains, like 15 Tom Waits' albums in mp3 format on a single disc for £1. For the same price I picked up what the gentleman assured me were "200 Russian rock classics". There are only 183 of them, and it remains to be seen if the rest of his description is any more accurate.
But the undoubted musical highlight of the trip was catching Sweet in the middle of their current Russian tour. There is only Andy Scott of the classic line-up left - Brian and Mick are sadly no longer with us, and Steve is in the States - but that did not matter to me and their small but ardent local fan base. They put on a great show.
I was going to give you a Sweet special today, but I got distracted by Wig Wam Bam. It struck me that it was only one of many songs that address the delicate matter of the romantic lives of Native Americans with a rigour that professional anthropologists can only envy. Here's a selection.
"Wig Wam Bam" - Sweet
"Running Bear" - Johnny Preston
"Indian Love Call" - Tex Ritter
"Indian Wedding Song" - The Indians
"Squaws Along The Yukon" - Hank Thompson
"Big Chief Litle Puss" - The Olympics
Now, the Rostov gig was closer to Old Age Rampage than Teenage Rampage, but never mind.
Two For Lou
One from the man himself, one from his old sparring partner. They said he could break a mountain in two.
"Fly Into The Sun" - Lou Reed
"Half Past France" - John Cale
Straight Off The Urals
Off to Russia tomorrow. First I have a few day's work in Moscow then I'm heading down to Cossack country to have a look around. Here are some songs about Russia and Russians to keep you going in my absence. See you in a week or so.
"Man From Russia" - The Blow Monkeys
"White Russian Doll" - Lucky Soul
"Mayday In Moscow" - The Fire Hydrant Men (featuring The Fabulous Fezzettes)
"Rockin' Behind The Iron Curtain" - Frankie Ford
"Stalin Wasn't Stallin'" - Robert Wyatt
"Rus Pu Tin" - Panadda Chayapark
Teanet Time!
The late, great Peta Teanet - the first King of Tsonga Disco - always goes down well with our core constituency. So, pandering to you as shamelessly as a Tory politician inventing immigration scare stories, here are a couple of tracks from his album "Double Pashash".
"Ha Hela" - Peta Teanet
"Dlawelwa Kulunga" - Peta Teanet
"Double Pashash" came out in 1995. Back in Blighty this was a big hit that year. I remember dancing to it in the Rio Nightclub in Leamington Spa with a group of drunken civil servants - happy days!
And of course you can't have that without this as a 2-for-1 treat. Mandy Dingle!
Very Big In Vilnius
I had a very pleasant time in Lithuania last week - definitely worth a visit if you have not had the chance to do so before (and, indeed, if you have).
One of the cultural highlights was seeing Arbata in concert in the very groovy Puntojazz Club in Kaunas, promoting their new album "Kiekvienas Tiesus". To put it another way, according to Google Translate, I saw Tea promoting their new album "Every Straight".
I enjoyed the show a lot. The accordion player gave them a feel of the Waterboys just at the point they started moving from The Big Music to Fisherman's Blues (not that I'm equating the two bands, you understand).
The album I enjoyed slightly less. It is a good listen, but on most tracks they replace the accordion with keyboards which makes their anthemic ambitions a bit more obvious. I've never been a great one for anthems, and it is perhaps no surprise that my favourite track on the album is the one that sounds most like the live version.
"As Tave Rasiu" - Arbata
I can also announce an exciting discovery for you fashion fans. As you can just about make out in this picture, the suit jacket with sleeves rolled up to the elbow look is still alive and well in Kaunas. It's like the 80s never left us.
You are not going to hear a lot from me this month, folks. In a couple of hours I'm off to Lithuania for a few days' work followed by a few days' holiday, I come back to change my socks, then I'm off to Russia for more of the same. Still, think of all the Lithuanian disco and Russian folk-rock you have to look forward to!
I'll leave you for now with a selection of tracks that we first featured back in our formative days but are well worth playing again. We start with something from an album of Virginian soul and funk that I bought in the State Library in Richmond (now that's a library!). We follow it up with some Filipino pop, some "post punk" from the UK and Belgium, before finishing with some South African reggae and a tribute to the Korean alphabet. Something for everyone.
"I Was Born To Be A Drummer" - The 35th Street Gang
"Shing-a-Ling Time" - Helen Gamboa
"Expert" - pragVEC
"Give Me A Gun" - Lavvi Ebbel
"Ke LeRasta 4 Life" - Rastaman Nkhushu
"Mi Ga Na Da Ka Ma Ba (My Loving Korean Alphabet)" - Kim Jung Mi
Regular readers know what you're going to get as the video clip when I'm off on my hols. But instead of the usual clip, here's the boys back together in 2004.
Freddy's Revenge
To get you in the mood for the weekend, here are some vintage tunes from that fast-talking son of a gun, Daddy Freddy.
"The Girl Is Fine" - Daddy Freddy
"The Crown" - Daddy Freddy
"Ickie Fashion" - Pepper & Daddy Freddy
He was at the height of his fame in the late 80s and early 90s, but Freddy has never really been away. Earlier this year he popped up, with many other old favourites, on Congo Natty's "UK Allstars":
Of course, Congo Natty himself has been around the the 80s as well, only then he was calling himself Rebel MC. Which gives me all the excuse I need to play this (not that any excuse is ever needed):


The contact information for The Corvette Shop Inc. is found below. If this is incorrect please click the "SEND" button to let us know. Do you own The Corvette Shop Inc.? If so please click the "Claim your free listing" image on the left to see why it is important to claim it. This is the business contact information for The Corvette Shop Inc., which is located at 2337 Glenda Ln in Dallas. Feel free to call them at (972) 243-3033. You may wish to view other businesses in our Automotive or Auto Parts & Services categories. To do so click the links above. For a map and driving directions to 2337 Glenda Ln in Dallas please scroll down and click the link under the map to "View Larger Map".


text:
describe('test', function() {
  it('is not asynchronous', function() {
  });
});


Our passion is to grow great food and give our customers a great food experience.
We focus on using the best certified organic methods to produce nutritious and flavourful vegetables and creating a healthy and happy environment for our staff.
We love talking about this at farmers' markets and with visitors to the farm, but it occurred to me that we've only had the chance to talk with a handful of our customers, and the rest don't even know what we look like!
So without further ado, let me introduce to you the family behind the farm!
Vicky communicates with our chefs and store produce managers every week to take their orders. She organizes the packaging of the vegetables for our chefs, stores and farmers' markets and prepares our driver, Tony, to hit the road every Tuesday, Thursday and Friday for deliveries. If you call the farm she will likely be the one to answer.
Mike does all the field planning, which means he decides which fields will be used to grow crop each year, which fields will be rested and when things will be planted. He organizes and works with 8 guys in the field during the growing season prepping beds, planting, harvesting and field maintenance (aka weeding). In the winter he manages the greenhouses and lends his muscle in the shed, where we are washing and packing organic vegetables every day.
That's me. I focus on making our produce as accessible as possible, to as many of you as possible, in stores, restaurants and at farmers' markets. I write our blog and work on marketing and business development.
If you are interested in using our product you can contact me anytime.
Caroline (our mum - yes, I spelled 'mum' not 'mom'- our family has British roots) takes care of all the administration and accounts. She also plans and manages Field 1, which is where all of our edible flowers, herbs and garnishes are grown in the summer.
Lily, my niece, loves visiting the farm and eating carrots- purple haze is her favourite!
We are also very lucky to have the support and advice from our dad, Simon, who has many years experience in agriculture.
We welcome you to contact us any time with any questions. If you would like to visit us and pick up produce from the farm please give us 24 hours notice.


We are continuing to build relationships through the art of communication, appreciation and respect. Simply being and being in the moment, these things are showing the way back to the basics. When we say "relationships" at Sacred Rok we mean with all life – air, water, and land. This is the Law for the Real World. When we say "communion with our senses" we mean tuning in and remembering how to feel as well as think. Our experiences continue to help us better understand the word education and commit to the reality of Education Nature's Way.
We are happy to say with your help we have had many day trips the last spring and camping trips throughout the summer with all our regulars – Merced Probation, Merced Boys and Girls Club, and the Mariposa Middle School. The beauty of these outings is getting to know each other, learning how to work together or let's say be together, enjoying Yosemite's ceremony of nature.
With the probation department we've taken our Yosemite outings into their classroom, working on a story sharing video from our pictures and video collection over the years. This has amazing potential to express the contrasting worlds of being incarcerated to standing under 1000 foot waterfalls with rainbows, fresh water springs, healthy food and stress free environments – as we experience the transformation of being free to be truly human.
Our Spring day trips set up the opportunity to follow the trail to summer camp in Tuolumne Meadows 8000 feet up the mountain. In July we had our first camping trip of the summer with the Boys and Girls Club and soon after we hosted our second camping trip with the Mariposa Middle School. We had worked with all of these youth before throughout the last two years but for some this was their first camping trip. This is always a unique and important step not only for Sacred Rok but also for the youth and we do our best to host them in the most nurturing way. In early August we had a group of youth from Green Acres in Sebastopol who spent a few days with us. This is a new and budding relationship and we look forward to continuing our work with them. Our last trip of the summer season was with the Merced Probation – reinforcing our connections. All of our trips taught us something about ourselves and furthered our dedication to our vision at Sacred Rok.
As of this summer, it's been 4 years since we started Sacred Rok. The lessons we have learned in bringing the youth into nature are profound. The institutions and the social conditions that form the environment that these young people experience every day contrast to our experiences in Yosemite.
We hope that the experiences of nature promote their human development. The trees that they smell, the wind that they feel, and the pools in the river that they dip in all become a permanent part of their cumulative life memories — a collection of their being. As well, we hope that our approach shows them that most of what we learn as humans comes from the inside. As adults, we are humble facilitators of the connection to the great teacher, nature.
By learning from the inside, I mean that the young people appreciation of nature happens not because we "tell them" but because they resonate to what already exists in the human spirit. Sacred Rok is a facilitator of this connection.
This lesson, something that I have learned over my many years from my teacher Yosemite when I was 14 – facilitated by the adults around me – is really what I want to share through Sacred Rok. And, over the past 4 years, I think that our opportunities– working with Merced foster care, Merced Probation, the Boys and Girls Club, the Planada youth, Native American youth, as well as some groups from outside this area – has reinforced this lesson. The youth who have participated with us, many of whom have come back repeatedly, have told me so, in so many ways. I deeply appreciate these experiences, which have, in turn, been my teacher.
Where is the source of education, and what is the adult role in it? That's really what it boils down to. My friend Kenji, who works in so many areas of formal education, tells me that that's one of the basic debates that goes on in his world of schools in the K-12 world. Some things for sure need to be explicitly taught – for example, connecting the script to the sounds of a language is basic to learning to read any language. But many others things need to be constructed through facilitated experience – for example, finding the deep meaning of a poem requires discussion and reflection, and diving into the self – this is hard to teach through drills and worksheets and fill-in-the-bubble approaches. Students learn by connecting meaning to their self and their spirit, and connecting to the natural world.
At Sacred Rok, nature provides our curriculum and our structure. Sunrise, sunset, wind and weather guide our activities. We follow the pace of nature, and this helps the kids to slow down and learn to breathe, walk, and listen to the water and the wind in the trees. This is not a one shot deal. These young people come back again and again, and over time we build our trust and strengthen our relationshipsthat are simply natural.
So through our experiences over the past 4 years, I think we have established the value of respecting the youth to connect in their own way given the chance, the value of providing healthy food, the value of place, and the continuity of learning over time. It seems as though formal institutions try to acknowledge the importance of learning from the inside, but they struggle with recognizing it fully. What we have shown is that this can be done at a small scale, working to facilitate small groups of youth with some continuity. When we established Sacred Rok in 2009, we knew that we wanted to support young people with the ceremony of nature. We had a vision, but we did not have a specific plan. But we have mapped it out during the last 4 years, demonstrating the feasibility and power of our vision.
So what is our next 5-year plan? Kenji and Nancy just spent two weeks at camp in Tuolumne and we had a good chance to reflect on our accomplishments and envision our future, surrounded by the signs of nature and reflecting on their meaning. Here is one reflection we had. There is a beautiful boulder which sits just across the river from my campsite. It got here having floated down the canyon carried on top of a glacier thousands of years ago, and was placed here as the glacier melted. The Tuolumne River is still flowing from the Lyell Glacier that receded but continues to provide the flow of this river, being watched by the boulder. This celebrates the art of nature. Through the help of great friends who have given us generous grants and individuals who have contributed by buying our books and photos, we have subsidized trips working with the Merced organizations who are working hard to support these youth. During the next 5 years, we plan to consolidate these successes further so that the organizations see this as a central part of their own mission, rather than as an add-on subsidized by outsiders.
As we do this, we hope to use our gifts, grants and donations to work toward the establishment of a "place" for Sacred Rok. Having a specific piece of land owned by Sacred Rok and established as a center for learning is important because the "sense of place" is central to our work. We see the mountains from which the water for much of California emanates as an essential link for our youths to the land. Because we want all of our youth touched by Sacred Rok to have a sense of place grounded in nature, a place for them to come and stay to re-connect with the earth, is essential. We are thus seeking a modest piece of land where we can start growing organic food, staying for gatherings, building fires, and having the time to inspire. Such a place may be in the foothills on the western or eastern side of the Sierras.
Finally, during the next 5 years, we are hoping to play more of a convening role for organizations that seek to help youth that share our philosophy. In our work with the various organizations in Merced, we have found like-minded souls within probation, youth organizations, Native American, and foster care organizations. We also have met many people in school systems throughout California who understand the barren agenda of school reform focused on narrow academic skills and neglecting the nurturing of the human spirit. We are contemplating the next 5 years as a period where we can develop leadership potential for people within these organizations, and to collaborate in the re-birth of humanity through partnerships with inspirational individuals who are in a position to transform their organizations. The land we hope to acquire will serve as a center where gatherings of these leaders can occur.
As a child my great grandfather grew a garden that supplied food for the table and the many months ahead. Things that didn't get eaten immediately were jarred, canned and frozen. Jams, salsas, stews and pickled items lined the shelves of the pantries of every member of our family. I remember the crisp cucumbers sprawled across the ground, the prickly merlitons and their weird smell, the stakes of snap peas, the canopy of grape leaves draped across the pecan trees in the back corner, and the hot house with it's tomatoes and box of potatoes.
The tomatoes were the best with their deep red flesh and the sweet water of the earth. I ate them like apples on occasion or my great grandmother would very gingerly peel and chop them and season with salt, pepper and vinegar. These became one of my favorite things to eat and I had a hard time understanding why many people would say they hated tomatoes.
My great grandfather took pride in his plants and he kept a journal of his garden – what he planted, when he planted, what pests came, what nutrients were needed, when was the frost, when was the drought, home remedies and theories. As I grew up I started to garden myself and I called him or wrote to him often asking advice on what I had growing. My gardens prospered and my tomatoes and peppers were almost as sweet as his.
In the south of Louisiana, especially with a hot house, one can grow tomatoes for most of the year but there are those few months in winter and early spring when this just isn't possible. Yet, in the stores there would always be tomatoes – their skin an odd, speckled orange red color, their feel a little too firm, and their flesh leaving something to be desired. These were not tomatoes, these were an insult to my paw-paws vine-ripe beauties. They hardly seemed edible yet they were everywhere – in the schools, in restaurants, in the markets, cafeterias, etc. I started to understand why people said they didn't like tomatoes – if these mushy, tasteless things were what they were eating then there was absolutely no reason to like them.These impostors were/are the result of large scale farming – otherwise known as industrialized farming.
Industrialized farming has done it's job at supplying "food" for the masses and it's also done it's job at homogenizing, monoculturing and taking then richness out of the food. In response to this a great food movement is occurring – hardworking people are pouring their spirits into small scale, organic farming. What comes out of it are fruits and vegetables and meats so rich and full of life that I recall my great grandfather out in his garden with his soil stained hands and his bucket of fresh food.
This is the food that I love and this is the food that Sacred Rok supports. We want the youth and adults we work with to understand this difference and to be nurtured by this food. This is why we largely support local, organic farming practices and try to buy most, if not all of our food from these types of people and places. We are fortunate to have great people like Brenda Ostrum and Mountain Meadow Farms, TD Wiley Farms, the High Country Health Food store in Mariposa, the Sierra Sundance Whole Foods in Mammoth, the Mono Market in Lee Vining and the Manor Market in Bishop – all of these people and places work with local, organic farmers to provide some of the best goods available. In honor of my great grandparents and for the benefit of all Scared Rok will continue it's vision of creating healthy meals with healthy food.


Metal roofing's Class A fire rating helps shield homes from flying sparks and embers. Photo courtesy of American Metal Roofs of Michigan.
PORTLAND, Ore.—July is peak wildfire season, the Metal Roofing Alliance (MRA) is urging homeowners to consider ways to better protect their homes.
That's especially true in the Western U.S. and Canada with recent hot temperatures and winds only exasperating the problem and making the danger of fires starting in nearby communities and threatening homes a very serious issue. Roofs are especially vulnerable to flying embers from nearby wildfires, which can travel up to a mile away.
7 Tips To Prevent Roof Fires from Metal Roofing Alliance on Vimeo.
To help protect homes, FEMA recommends that in fire-prone areas, if a roof is covered with wood or asphalt shingles, homeowners consider replacing it with a fire-resistant material, such as metal. Metal roofing has a Class A fire rating, the highest available. An unrated roof is the most vulnerable to fire and includes materials such as non-fire-retardant treated wood shakes or shingles.
Wildfire season in North America starts earlier, lasts longer and affects more areas than ever before, making it a priority for homeowners to consider better ways to protect their homes against the increasing threat. Over the past 12 years, every state in the western U.S. has experience an increase of large wildfires per year, compared to the annual average from 1980 to 2000.
Create a defensible barrier. Trim tree branches away from the roof. Keep gutters clean as dried leaves and vegetation can create the ideal ignition conditions for a wayward spark.
Pay attention to your roof's components. Use only vent covers that will not readily burn or melt.
Maintain your roof all year long. Have a professional roofer inspect your roof, clear off flammable debris and repair any missing or damaged components to prevent embers from nestling into vulnerable or exposed areas.
When reroofing, consider long-term performance and protection. Choose durable, nonflammable materials, such as metal roofs, and ensure your roof has a Class A rating for fire-resistant performance, especially near any wildfire-prone area.
Focus on your surroundings when using fireworks. Only use legal fireworks in a safe area, completely away from dry fields, forests and buildings. Keep water, a garden hose and garden tools nearby to safely extinguish fireworks and obey all local ordinances regulating the sale and use of fireworks.
Watch as ABC News covers how metal roofing contributed to saving one family's home from a wildfire.


text:
Alban George Henry Gibbs, 2nd Baron Aldenham (23 April 1846 – 9 May 1936), was a British Conservative Party politician and peer, the son of Henry Hucks Gibbs, 1st Baron Aldenham.

He was elected at the 1892 general election as a Member of Parliament (MP) for the City of London, and held the seat until his resignation from the House of Commons on 14 February 1906 by the procedural device of accepting appointment as Steward of the Manor of Northstead.

He succeeded to the title Baron Aldenham on 13 September 1907.

He married Bridget Beresford-Hope, daughter of Alexander Beresford-Hope, on 18 February 1873. They had three children:
Catherine Louisa Gibbs (1875–1967)
Mildred Dorothea  Gibbs (1876–1961)
Gerald Henry Beresford Gibbs, 3rd Baron Aldenham (1879–1939)

References

External links

Aldenham, Alban Gibbs, 2nd Baron of
Aldenham, Alban Gibbs, 2nd Baron of
Conservative Party (UK) MPs for English constituencies
UK MPs 1892–1895
UK MPs 1895–1900
UK MPs 1900–1906
UK MPs 1906–1910
UK MPs who inherited peerages
Fellows of the Society of Antiquaries of London
Members of Parliament of the United Kingdom for the City of London
Alban
Alban